Commun. Math. Phys. 361, 53–80 (2018) Communications in Digital Object Identiﬁer (DOI) https://doi.org/10.1007/s00220-018-3159-z Mathematical Physics Coupling the Gaussian Free Fields with Free and with Zero Boundary Conditions via Common Level Lines 1 2 Wei Qian , Wendelin Werner Center of Mathematical Sciences, Wilberforce Rd., Cambridge CB3 0WB UK. E-mail: wq214@cam.ac.uk Department of Mathematics, ETH Zürich, Rämistr. 101, 8092 Zurich Switzerland. E-mail: wendelin.werner@math.ethz.ch Received: 3 July 2017 / Accepted: 2 March 2018 Published online: 1 June 2018 – © The Author(s) 2018 Abstract: We point out a new simple way to couple the Gaussian Free Field (GFF) with free boundary conditions in a two-dimensional domain with the GFF with zero boundary conditions in the same domain: Starting from the latter, one just has to sample at random all the signs of the height gaps on its boundary-touching zero-level lines (these signs are alternating for the zero-boundary GFF) in order to obtain a free boundary GFF. Constructions and couplings of the free boundary GFF and its level lines via soups of reﬂected Brownian loops and their clusters are also discussed. Such considerations show for instance that in a domain with an axis of symmetry, if one looks at the overlay of a single usual Conformal Loop Ensemble CLE with its own symmetric image, one obtains the CLE -type collection of level lines of a GFF with mixed zero/free boundary conditions in the half-domain. Contents 1. Introduction ................................. 53 2. Background: The ALE of a Dirichlet GFF ................. 56 3. The Coupling of the Two Fields: Statement and Consequences ....... 59 4. Proof of the Coupling ............................ 63 5. Relation to Soups of Reﬂected Loops and Consequences .......... 69 6. Shifting the Scalar Version of the Neumann GFF and Related Comments .75 7. Further Questions and Remarks ....................... 78 Acknowledgements ................................ 79 References ..................................... 79 1. Introduction A large number of recent papers (see for instance [9,10,22–24,33,34,39] and references therein) have highlighted the close connection between Schramm-Loewner evolutions 54 W. Qian , W. Werner (SLE) and their variants such as SLE (ρ) processes or the conformal loop ensembles (CLE) with the two-dimensional Gaussian Free Field (GFF). This has led to a much better understanding of the geometric structures underlying the GFF, as well as to new results about SLE and CLE. A special role is played by the SLE process, the SLE (ρ) processes and the conformal 4 4 loop ensemble CLE , because, as pointed out by Schramm and Shefﬁeld for SLE (ρ) 4 4 curves in [33,34] (see also Dubédat [9]), they can be viewed as level lines of the GFF with constant or piecewise constant boundary conditions, or more precisely as lines along which the GFF has a certain height-gap 2λ = π/2. Gaussian Free Fields with other natural boundary conditions than constant boundary conditions are of course of wide interest. One prime example is the GFF with free boundary conditions in a domain D (that we will refer to from now on as the GFF with Neumann boundary conditions, or the Neumann GFF—we will also refer to the GFF with zero boundary conditions as the Dirichlet GFF). Recall that, as opposed to the Dirichlet GFF, the Neumann GFF is only deﬁned up to an additive constant (one way to think of this is that one knows the gradient of a generalized fuction, but not the function itself). However, away from the boundary of D, the (generalized) gradient of this Neumann GFF is absolutely continuous with respect to the (generalized) gradient of the Dirichlet GFF, so that it is also possible to make sense of the level-lines of this ﬁeld, that are also SLE -type curves (the precise description for mixed Dirichlet–Neumann boundary conditions has for instance been given by Izyurov and Kytölä in [12]). The Neumann GFF also plays a central role in the zipping/welding approach to SLE (see Shefﬁeld’s quantum zipper [39]), or via the interplay between SLE paths and Liouville Quantum Gravity, see for instance [10]. It seems that some simple CLE-type constructions or descriptions of the Neumann GFF and their consequences may have been overlooked, and one of the goals of the present paper is to ﬁll this gap. More precisely, in this direction we will: (1) Describe the collection of level lines of the Neumann GFF. The fact that this can be done is not really surprising (for instance given the results in [12]), but the consequence (2) was maybe more unexpected. (2) Point out a simple coupling of the Neumann GFF with a Dirichlet-GFF in the same domain: The difference between the two ﬁelds in this coupling is a function that is constant by parts, and the two ﬁelds will share a number of level lines. Only the signs of the height gaps for the boundary touching level lines of height 0 for the Dirichlet GFF will differ, so that the difference between the two GFFs will take its values in 4λZ (see Fig.1 for a sketch). More precisely, start with a Dirichlet GFF and deﬁne the collection A of its boundary touching level lines at height 0 (these are λ versus −λ height-gap lines). The complement of A consists of a family of cells in which behaves like a GFF with constant boundary conditions λ or −λ as on the left of Fig. 1 (this means that inside each cell, one considers a GFF with Dirichlet boundary conditions and adds the constant function λ or −λ depending on the cell). Here, the height gaps between two neighboring cells are alternating between 2λ and −2λ so that the height of all cells stays in {−λ, +λ}. Now, toss an independent fair coin for each arc of A in order to decide the corresponding height-gap between the two cells that it separates. This leads to the picture on the right of Fig. 1. Theorem 1 will state that adding an independent GFF in each cell to these new heights deﬁnes a scalar ﬁeld which is exactly a realization of a Neumann GFF (i.e., its gradient is that of a Neumann GFF). In other words, if one adds to the Dirichlet GFF the function that is constant in each cell and equal to the difference between the new and old heights in that cell, one does obtain a Neumann GFF. Coupling Gaussian Free Fields 55 Fig. 1. Sketch of the coupling: On the left, the boundary touching level lines of the GFF with Dirichlet boundary conditions. Adding to these values an independent GFF in each of the cells constructs a GFF with Dirichlet boundary conditions in the square. On the right, we keep the same set of boundary touching level lines but the signs of the height gaps are chosen at random. Adding to these values an independent GFF in each of the cells constructs a GFF with Neumann boundary conditions in the square The existence and properties of this coupling between Neumann GFF and Dirichlet GFF shows again—if needed—how natural these SLE level lines are in order to connect and understand these two ﬁelds. Another approach to the coupling between SLE (or CLE ) with the GFF with Dirich- 4 4 let boundary conditions uses the Brownian loop-soup introduced in [16]: On the one hand, CLE can be constructed as outermost boundaries of Brownian loop-soup clusters of appropriate intensity [40], so that it is a deterministic function of this loop-soup. On the other hand [17], one can show that the (appropriately renormalized) occupation time measure of the Brownian loop soup is distributed like the (appropriately deﬁned) square of a Dirichlet GFF—so that this square of the Dirichlet GFF is also a deterministic func- tion of the loop-soup. Furthermore [18], it is possible to use the loop-soup in order to reconstruct the Dirichlet GFF itself (loosely speaking, by tossing one independent coin for each loop-soup cluster to choose a sign). Combining these constructions provides a coupling of CLE with the GFF. As explained in our paper [30], it is possible to show (using also some further results of Lupu [19] and the relation to Dynkin’s isomorphism theorem) that this coupling can be made to coincide with the Miller-Shefﬁeld coupling where the CLE are the level lines at height ±λ of the Dirichlet GFF (see [5] for this). We will also address in the present paper the free boundary GFF counterparts of all these facts. Not surprisingly, it will involve soups of reﬂected Brownian loops: (3) We will explain that all the features about loop-soup clusters, their decompositions and the relation to the GFF, as shown in [30] for Dirichlet boundary conditions have natural analogs for Neumann boundary conditions. Recall that one consequence of the Brownian loop-soup approach to CLE is that it enables to derive relations between the various CLE ’s that seem out of reach by an SLE -based deﬁnition of the conformal loop ensembles. More precisely, since a CLE κ κ(c) for some explicit function κ(c) ∈ (8/3, 4] is the collection of outermost boundaries of loop-soup clusters with intensity c ≤ 1, one can construct it from two independent samplesofCLE and CLE when c + c = c by looking at the clusters in the κ(c ) κ(c ) 56 W. Qian , W. Werner union of these two CLEs (a noteworthy example is the fact that one can reconstruct a CLE using the overlay of two independent CLE ’s, which are known to be the scaling 4 3 limit of Ising model interfaces, see [7] and the references therein). This makes it natural to deﬁne also such “semi-groups” of CLEs for Neumann-type boundary conditions: (4) We will explain how to naturally deﬁne Neumann-type CLE ’s for all κ ∈ (8/3, 4]. This for instance leads to simple coupling between a usual (Dirichlet) CLE in the unit disc and a GFF with mixed Dirichlet–Neumann conditions in the half-disc (Dirichlet on the half-circle, Neumann on the diameter I ) by looking at the overlay in the half-disc of the CLE with its symmetric image with respect to the diameter I . The organization of the paper is the following: We will ﬁrst recall background on the collections of level lines for the Dirichlet GFF in Sect. 2. In Sect. 3, we state the coupling of the Neumann GFF with the Dirichlet GFF, Theorem 1, and make various comments. We then prove Theorem 1 in Sect. 4. Then, in Sect. 5, we discuss the relation and interpretation in terms of soups of reﬂected Brownian motions, and to the construction of other “reﬂected” CLEs. We then discuss results related to the fact that the Neumann GFF is deﬁned up to an additive constant, and we conclude with some further comments about related work and work in progress. Since some arguments that we will use are directly adapted from those that have been developed and used in the context of the Dirichlet GFF, we choose to provide the more detailed proofs only for the pivotal and novel parts. 2. Background: The ALE of a Dirichlet GFF In this section, we will describe what we will refer to as the ALE of a GFF with Dirichlet boundary conditions. We survey here known facts that are part of the general framework of level lines of the GFF as ﬁrst pointed out in [9,33,34], see also [28,41,42,46]for survey and variants. For all of this section, we refer to [5] for background and details (further related items are discussed in [2,4]). Recall that the GFF with Dirichlet boundary conditions in D can be viewed as a centered Gaussian process indexed by the set of continuous functions f in D with compact support in D. The covariance of this process (which therefore deﬁnes the law of )is E [( f )(g)]= G (z, z ) f (z)g(z )dzdz D×D where G = G is the Green’s function in D with Dirichlet boundary conditions (here and in the sequel, dz will stand for the two-dimensional Lebesgue measure). Throughout the paper, we will use the normalization of Green’s functions G(z, z ) such that G(z, z ) ∼ −1 (−2π) log |z − z | as z → z when z is in the interior of the considered domain. With this normalization, the natural height-gap as introduced by [9,33,34] is equal to 2λ, where λ = π/8 (this value of λ will be ﬁxed throughout the paper). We can note that one can in fact deﬁne on a larger set of functions (or measures). For instance, the previous deﬁnition obviously works also for the set of continuous functions This terminology, referring among other things to Arc Loop Ensembles, had been proposed by J. Aru and Avelio S. in the course of the preparation of [5], and at that time the third coauthor was reluctant to introduce such a new terminology, especially in relation with the Beatles of the free ﬁeld introduced in [5]. We ﬁnally opt here for this terminology to stress that the work done in [5] was inﬂuential for the present one. ALE should be ideally come with a Chilean or Estonian accent. Coupling Gaussian Free Fields 57 f in D such that G (z, z ) f (z) f (z )dzdz < ∞ D×D and we will implicitely use this extension at various instances in the paper (when we deﬁne the ALE decomposition of the GFF for instance, we will consider continuous bounded functions in a bounded domain D). However, when one knows the process deﬁned on the set of continuous functions with compact support, one can extend to this larger set of functions by a continuity argument. We will use the same procedure when we will consider and deﬁne the Gaussian Free Fields with different boundary conditions (Neumann, or mixed Neumann–Dirichlet) in a domain D as random processes indexed by the set of continuous compactly supported functions in D. It is useful to ﬁrst recall the Miller-Shefﬁeld [21] coupling of CLE with the GFF (see also [5] for details): Consider a simply connected domain D with non-polar boundary, and a simple non-nested CLE in D. Recall that this is a random collection (γ ) of 4 j j ∈J disjoint simple loops in D such that: (a) Each given point in D is almost surely surrounded by exactly one loop of the CLE . (b) The law of the CLE is invariant under any conformal automorphism of D. Note that (a) and (b) imply that the set of points that are surrounded by no loop (this set is called the CLE carpet) has zero Lebesgue measure. In fact, it can be shown that its Hausdorff dimension is almost surely equal to 15/16 [27,35]. Once one has sampled this CLE , one can toss an independent fair coin ε ∈{−1, +1} for each CLE loop, and 4 j 4 consider for each realization of the CLE , the random function that is equal to 2λε in 4 j each domain O encircled by γ , and to 0 in D\∪ O , i.e., the function 2λε 1 . j j j j j O j j Then (i.e., conditionally on the CLE ), inside of each O , deﬁne an independent 4 j GFF with Dirichlet boundary conditions. The coupling states that the ﬁeld ( + j j 2λε 1 ) is a Dirichlet GFF in D. Note that when f is a compactly supported function j O in D, for each j, the function f restricted to O is a continuous bounded function in O , so that one can deﬁne ( f 1 ). Note that conditionally on the CLE , the series j j O 4 ( ( f 1 ) +2λε f (z)dz) j O j is a series of independent random variables with zero mean, and the usual L criterion ensures that it almost surely converges. One important feature of this coupling, also pointed out by Miller and Shefﬁeld, is that the CLE and the labels ε are in fact deterministic functions of the GFF that they 4 j construct in this way (see again [5]). Heuristically, the CLE loops can be viewed as level lines, or more precisely as height-gap lines: The coupling shows indeed that on the inside of γ , the GFF behaves like a GFF with boundary conditions 2ε λ, while on the outside of O , γ plays the j j j role of a Dirichlet boundary condition for the GFF. The curves (γ ) can be therefore informally described as 2λ v. 0 (or −2λ v. 0) height-gap lines. They are the ﬁrst set of such loops that one encounter when one starts from ∂ D (where the height of the GFF is 0). In the sequel, we will say that refer to an a-level line for an a + λ v. a − λ height-gap line (so that the CLE loops are λ level lines, or −λ level lines). The nested CLE is then obtained by iterating the same construction for each and 4 j so on—see for instance [5] and the references therein. 58 W. Qian , W. Werner Fig. 2. Structures within a Dirichlet GFF: The ALE with the alternating heights ±λ, some of the embedded CLE loops with their heights ±2λ We now describe the closely related coupling that will play a very important role in the present paper. Instead of looking at the ﬁrst set of loops with height λ or −λ that one encounters when starting from ∂ D (thisisthe CLE depicted on the right-hand side of Fig. 2), it is be possible to make sense rigorously of the collection of all ﬁrst level lines of height 0 that one encounters when one starts from the boundary – these are the level lines at height 0 that do intersect ∂ D (depicted on the left-hand side of Fig. 2). As explained in [5], it is in some sense the most natural and sparsest level-hitting set that one can deﬁne in a Dirichlet GFF. This set A can be deﬁned by a branching family of SLE (−1, −1) processes, and is denoted by A in [5]—it is also one very special 4 −λ,λ particular case of the boundary conformal loop ensembles deﬁned in [25] (and has also appeared before, see [34,42]). This is what we will call an ALE in the present paper. Let us ﬁrst summarize its main properties: (a) An ALE is formed by a countable union of disjoint SLE -type arcs in D joining two boundary points of D. It is locally ﬁnite (each compact subset of D intersects only ﬁnitely many ALE arcs). (b) The law of the ALE is invariant under the group of conformal automorphisms of D. A consequence of these items is that the Hausdorff dimension of the ALE is that of individual SLE curves i.e., 3/2(see [6,31]). Furthermore, each ALE arc will be a shared boundary between two adjacent connected components of the complement O of the ALE in D. In particular, the family of connected components of O comes naturally equipped with a tree-like structure given by the adjacency relation. We will sometimes refer to the connected components O as the cells of the ALE. The construction via SLE (−1) shows that the dimension of the intersection of the boundary of a cell with the boundary of D is equal to 3/4 when the boundary of D is smooth (using for instance Theorem 1.6 of [26]). One can then couple a GFF with Dirichlet boundary conditions with an ALE as follows: Toss ﬁrst one fair coin ε ∈{−1, 1} in order to decide the label of the connected component of O that contains the origin, and then deﬁne deterministically the labels ε of all the other components O of O in such a way that any two adjacent components have opposite labels (with obvious terminology, ε will be equal to ε on the even components j Coupling Gaussian Free Fields 59 O and to −ε on the odd ones). Deﬁne also an independent GFF with Dirichlet j j boundary conditions in each O . Then, it turns out that the ﬁeld := ( + λε 1 ) j j O is a GFF with Dirichlet boundary conditions in D.Again (see [5] and the references therein for all these facts), the ALE and its labels are in fact a deterministic function of (we can therefore call “the” ALE A = A() of ). One way to characterize A as a deterministic function of is to say that it is the collection of all the 0-level-lines of that touch the boundary of D. Note that there are two ways to think of the ALE. For each connected component O , the outer boundary of O will consist of the concatenation of ALE arcs, and form j j one single level line that is bouncing off from the boundary of D. In other words, one could also view the ALE as a collection of loops. But, in view of the next section, we choose to deﬁne the ALE as a collection of disjoint level-arcs (i.e., level lines inside the domain that start and end on the boundary). As explained in [5], starting from an ALE, it is easy to iterate the procedure by considering the ALE of each and so on, until one ﬁnds the ﬁrst ±λ level lines: One can then view the CLE as an iterated nested ALE (see again Fig. 2 for a sketch). Note that the number of iterations needed before discovering the CLE loop that surrounds a given point is random (which explains why the dimension of the CLE carpet is larger than 3/2). 3. The Coupling of the Two Fields: Statement and Consequences Recall that the Neumann GFF in a domain D is a similar (rather rough) conformally invariant centered Gaussian random ﬁeld as the GFF with Dirichlet boundary condi- tions, but that it is deﬁned only up to an additive constant. In other words, one deﬁnes only its gradient, or equivalently, it is possible to make sense of the centered Gaussian random variable ( f ) when f is a continuous function with compact support such that f (z)dz = 0, but one can not talk for instance of (1) or of the mean value of on a ball. Since we will only consider the Neumann GFF in simply connected domains, one handy quick way to deﬁne it is to ﬁrst deﬁne it in the upper half-plane and to then use conformal invariance to extend the deﬁnition to an simply connected domain D.Inthe upper half-plane H, the Neumann GFF is the centered Gaussian process ( ( f )), deﬁned on the set of continuous functions f with mean 0 with compact support in H, with covariance given by E [ ( f ) (g)]= f (z)g(z )G (z, z )dzdz . H×H The “Neumann Green’s function” G that we use here is deﬁned as N −1 G (z, z ) := (2π) (log |x − y| +log |x − y|). On the other hand, if we are actually given a scalar ﬁeld (i.e., a real-valued process (( f )) deﬁned on the set of smooth functions supported on compact subsets of D and that is linear with respect to f ), we can call it a realization of the Neumann GFF if it 60 W. Qian , W. Werner Fig. 3. The analogue of Fig. 1 in a strip: Illustration of the Dirichlet and Neumann coupling. Top: The ALE with the corresponding alternating heights. Adding to those heights independent GFFs in each tile does construct a GFF with Dirichlet boundary conditions in the strip. Bottom: The same ALE but with the randomly chosen signs for height-gaps. Adding to those heights independent GFFs in each tile does construct a GFF with Neumann boundary conditions in the strip behaves the same way as the Neumann GFF when one restricts it to the set of functions with zero mean (then, adding any constant function to would indeed provide another realization of the same Neumann GFF ). We are now almost ready to explain our coupling of the Dirichlet GFF with the Neumann GFF: Consider ﬁrst the decomposition of with the ALE A, the ﬁelds and the labels ε as described in Sect. 2. We then deﬁne a simple random walk indexed by the tree structure of the ALE. More precisely, we deﬁne a new set of labels η with odd values iteratively as follows: The label of the connected component that contains the origin is chosen to be ε, and for each connected component adjacent to this ﬁrst connected component, one tosses an independent fair coin to decide if its label is ε +2 or ε −2. Then iteratively, toss another independent fair coin for each connected component adjacent to the previously labelled components to decide whether their labels differ by +2 or −2. In other words, when one follows a path of adjacent connected components that go to the boundary, instead of seeing the alternating ε labels ε, −ε, ε etc., one now sees a simple random walk with jumps of ±2. We call this new set of labels (η ). See Figs. 1 and 3 for an illustration (with labels multiplied by λ). Note that with this deﬁnition, η − ε ∈ 4Z for all j. j j Theorem 1 (The Neumann GFF - Dirichlet GFF coupling). The ﬁeld := ( + λη 1 ) is a realization of a GFF with Neumann boundary conditions. j O Recall that the ﬁeld = ( + λε 1 ) is a GFF with Dirichlet boundary condi- j j O j j tions. This theorem therefore provides a coupling of the GFF with Neumann boundary conditions with the GFF , such that − is the function that is exactly equal to λ(η −1) on the even connected components O of the ALE of , and to λ(η +1) on the odd j j ones. Note again that there is no problem in the theorem in order to deﬁne ( f ) for continuous functions with compact support in D because almost surely, the support of f intersects only ﬁnitely many O ’s. It is important to stress that this coupling is very different from the coupling obtained by ﬁrst reading off the boundary values of the Neumann GFF i.e., the harmonic extension Coupling Gaussian Free Fields 61 to D of these boundary values, and to view the Neumann GFF as the sum of this random harmonic function (that is deﬁned up to additive constants, just as the Neumann GFF is) with an independent Dirichlet GFF. In the coupling described in Theorem 1,the difference − is not a continuous function in D, and furthermore the Dirichlet GFF and the difference − are very strongly correlated (the discontinuity lines of the latter are the boundary-touching level lines of the former). Note that in the construction of Theorem 1,the lawof is indeed conformally invariant if one views it as deﬁned up to constants (as the special role played by the origin in the construction disappears): The image of via a given conformal automorphism of D that maps some point z onto the origin is distributed exactly like shifted by a random additive constant ﬁeld with values in 2λZ corresponding to the height of the ALE cell for that contained z . It is worthwhile comparing the collection of level lines of with those of ,assome aspects can appear confusing at ﬁrst sight: On the one hand, Theorem 1 implies that: – The family A of all boundary-touching level arcs at levels in 2λZ (here and in the sequel, this means that we look at the union of these level arcs, but that we do not record the actual value of their height in 2λZ)for and for do coincide. Note however that the height of such an arc for is necessarily 0 for but can be non-zero for . – The collection of all other (i.e., non-boundary touching) level lines with height in 2λZ (both for and ) which correspond to the nested CLE loops for the ’s are 4 j therefore the same. Hence, we can say that the whole collections of level arcs and loops with height in 2λZ do coincide for and (here again, we look at the union of these level-lines but do not record their actual height). We can recall (see [5] and the references therein) that one can reconstruct deterministically the Dirichlet GFF from its collection of nested ALEs together with the knowledge of the signs of the corresponding height-gaps (there is one random coin-toss per individual ALE in the nested ALE). Since restricted to each cell O is just + λη , one can iterate the j j j procedure for each Dirichlet GFF and eventually, just as for the Dirichlet GFF , reconstruct via its collection of nested level lines (and the data about the random signs of the height-gaps). – The coupling also shows that each level loop of that does not intersect the ALE will correspond to a level loop of that does not intersect the ALE, and vice-versa. The difference between the height of such loops for and for will be in 4λZ. It is worthwhile to note that for the level lines that do intersect the ALE, the story is different. Indeed, the way in which they bounce on the ALE arcs will depend on the sign of the height-gaps on those ALE arcs as illustrated on Fig. 4 (this is very much related to how ﬂow lines for the GFF interact, as discussed for instance in [22]). As we shall explain in Sect. 6, this will imply for instance that there exist level-arcs at level in λ +2λZ for that do hit the boundary of the domain (see again Fig. 4), while this is known not to be the case for . In the same spirit, it is also easy to see that for the Dirichlet GFF , the collections of boundary-touching ALE with height in 2λZ (i.e. the collection of boundary-touching level lines with height 0) have a different distribution than the collection of boundary touching level lines with height in a +2λZ for a given a in (0, 2λ) (this follows for instance from the fact that the Hausdorff dimension of the intersection of the boundary of a cell deﬁned by these level lines with the boundary of the domain is explicitely known and depends on a). On the other hand, the Neumann GFF is deﬁned “up to 62 W. Qian , W. Werner Fig. 4. The −λ level line for turns left on the ALE arcs with positive height-gap (in dotted) and right on the ALE arcs with negative height-gap (in dashed), and ends up hitting the boundary an additive constant” so that one can wonder whether, when one couples with its particular realization as in Theorem 1, the law of the collection of boundary-touching level lines of with height in a +2λZ is independent of the value of a or not. The answer will be given by the following result: Proposition 1. The law of the collection A of all the boundary-touching level lines of with height in a +2λZ is identical to the law of A which is an ALE. Furthermore, conditionally on A , the signs of the height-gaps on each of the arcs are again i.i.d., just as for A itself. Informally, this means that if one is given a GFF with Neumann boundary condi- tions, then one can choose a “reference height” uniformly in [0, 2λ) in order to determine the realization of the corresponding ALE. In other words, the ALE is a deterministic function of the Dirichlet GFF, but in the case of the Neumann GFF, there is a one- parameter family of possible ALEs associated to it. A more precise related statement that follows from this proposition goes as follows: Suppose that is a Neumann GFF and that is a realization of it. Then, if one chooses an independent uniform random variable ζ in [0, 2λ], the ﬁeld + ζ is another realization of such that the law of the coupling of with the boundary-touching level arcs of + ζ at height in 2λZ and the corresponding height gaps, is the same as the one given by the coupling of the Neumann GFF with an ALE and i.i.d. gaps as given by Theorem 1. This is similar to the question of deﬁning the nested CLE as a function of the GFF in the Riemann sphere (see [13]) which is also deﬁned up to an additive constant. These boundary touching arcs for the Neumann GFF play a similar role as the CLE loops play for the Dirichlet GFF (or for the Neumann GFF for the inside loops). Indeed, if one views the Neumann GFF as deﬁned on the upper-half-plane and symmetrizes the picture with respect to the real axis (one considers the union of the ﬁgure in the upper half- plane with its symmetric image) which is a very natural thing to do for such Neumann boundary conditions, then each arc of the ALE will hook-up with its symmetric image and create a loop. The story is then just as for CLE : One has a collection of disjoint simple and nested loops, and each loop tosses an independent fair coin in order to decide whether it is an upward or a downward ±2λ jump of the GFF. The union of the ALE and of the inside CLE loops that one can deﬁne in the complement of the ALE are then a way to describe (and reconstruct, when one adds all the randomly chosen labels) the Neumann GFF. This is consistent with the informal description of the Neumann GFF Coupling Gaussian Free Fields 63 in the upper half-plane to be the GFF in the entire plane, conditioned to be symmetric with respect to the real line, and restricted to the upper half-plane. See Fig. 9 in the analogous case of mixed boundary conditions. The dimension 3/4 of the intersection of an SLE (−1) path with the real line can then be interpreted as the dimension of the part of the real line that belongs to a Neumann CLE carpet. 4. Proof of the Coupling The main goal of this section is to prove Theorem 1 (Proposition 1 will be derived in Sect. 6). Let us ﬁrst brieﬂy give the deﬁnition of the GFF with mixed Dirichlet–Neumann boundary conditions that will play an important part in the rest of this paper. The Dirichlet GFF is associated with Brownian motion that is killed when it reaches the boundary of D. If one divides the boundary of D into two parts, one part ∂ where the Brownian motion is killed, and one part ∂ where it is reﬂected, then it is easy to deﬁne (for instance by conformal invariance) the law of Brownian motion reﬂected on the latter part of the boundary and killed when it reaches the former, and the corresponding Dirichlet–Neumann Green’s function. One can for instance ﬁrst deﬁne this function in some well-chosen reference domain, and then generalize it by conformal invariance. Here, it is convenient to consider the positive quadrant Q = (0, ∞) , and to deﬁne the mixed Dirichet-Neumann Green’s function with Dirichlet conditions on R and Neumann conditions on i R by ND G (z, z ) = G (z, z ) + G (−¯z, z ). H H Then, one can deﬁne the Neumann–Dirichlet GFF in Q in exactly the same way as the Dirichlet GFF using this Green’s function instead. When the boundary of D is smooth and H is a bounded harmonic function in D such that the normal derivative on ∂ vanishes, we deﬁne the GFF in D with boundary conditions equal to those of H on ∂ and Neumann boundary conditions on ∂ (we will D N refer to those conditions as mixed boundary conditions) to be the sum of the previous Neumann–Dirichlet GFF with H. Again, one can then extent this deﬁnition to domains with non-smooth boundaries by conformal invariance. We are now ready to describe the following warm-up to the proof of Theorem 1 : • Let us choose w< o on the real line. When one considers a GFF in the upper half- plane with boundary conditions −λ on (−∞,w), λ on (w, o) and 0 on (o, ∞), then one can trace the 0-level line γ that emanates from w (with −λ boundary conditions on its left, and λ boundary conditions on its right) as illustrated on Fig. 5. Given that when one looks at the GFF away from (o, ∞), it will be absolutely continuous with respect to the GFF with boundary conditions −λ on (−∞,w) and +λ on (w, ∞),the existence and uniqueness of γ until the time τ at which it hits (o, ∞) can be viewed as a consequence of the corresponding known fact in the latter boundary conditions. In fact, the conformal Markov property with one additional marked point, and the characterization of SLE (ρ) processes as the only continuous processes that satisﬁes this property imply immediately that the law of γ up to τ is that of an SLE (ρ) for some value of ρ. The actual value of ρ is necessarily equal to −1, because in the previous setup, ∞ and o play somehow symmetric roles: γ is an SLE (ρ) from w to o with marked point at inﬁnity for the same value of ρ. This implies by the standard SLE coordinate change formulas (see for instance [36]) that κ − 6 − ρ = ρ with 64 W. Qian , W. Werner Fig. 5. The SLE (−1) corresponding to the 0-level line of the GFF with these boundary conditions Fig. 6. The same SLE (−1), this time corresponding to the 0-level line of a GFF with these new mixed boundary conditions (Neumann instead of 0 on (o, ∞)) κ = 4, i.e., ρ =−1. Of course, the previous lines are not the shortest derivation of the known fact that η is an SLE (−1) but we highlighted this argument in order to explain why the same result will hold in the next item. • Let us now consider instead a GFF in the upper half-plane, with boundary con- ditions −λ on (−∞,w), λ on (w, o), but this time, on (o, ∞), one takes Neumann boundary conditions. For the same absolute continuity reasons, one can deﬁne the 0-level line γ˜ that emanates from w (see Fig. 6) up to the ﬁrst time τ˜ at which it will hit (o, ∞), and until that time, it will be an SLE (ρ) curve from w to ∞ with marked point at o using the same argument based on the conformal Markov property. Again, ∞ and o play symmetric roles, so that it should also be an SLE (ρ) curve from w to o with marked point at ∞ for the same value of ρ, which shows that γ˜ is also an SLE (−1) curve (this is also not new, see for instance Izyurov-Kytölä [12]—we wrote out this little argument to highlight the basic reason for which the same SLE (−1) path appears in our two settings). Here, we can already couple these GFFs and with these different boundary conditions in such a way that γ and γ˜ coincide up to their hitting time of (o, ∞).The main question is now to see what one can do beyond the time τ . Note ﬁrst that in the case of , it is possible to continue the branching SLE (−1) as 0-level lines and to trace all the arcs of the ALE associated to via the SLE (−1) branching tree à la [38]. The question is what to do in the case of , when one has mixed boundary conditions. By symmetry, it will sufﬁce to describe how to continue to trace γ˜ targeting inﬁnity (the other branches will be deﬁned similarly). At time τ˜, the boundary conditions on the unbounded connected component of the complement of γ˜ are −λ on the left of the tip of the curve, and Neumann on (γ( ˜ τ) ˜ , ∞). By conformal invariance, this means that we are looking at the case of a GFF in the upper half-plane with boundary conditions −λ on R and Neumann on R (and that we want to couple it with a GFF in the upper − + half-plane with boundary conditions −λ on R and 0 on R ). Note ﬁrst that at every − + point, the expected value of this GFF (with mixed boundary conditions) is −λ. Here, the new input will be to notice that it is possible to directly adapt what has been done for instance for the deﬁnition of the CLE -GFF coupling out of the side-swapping SLE (−2) branching tree (see for instance [5,38,46,48]) to the present setting: If we were to insert a small interval (0,ε) with boundary height +λ, or with −3λ between the −λ and the Neumann boundary parts, then our previous analysis shows how to continue Coupling Gaussian Free Fields 65 Fig. 7. The SLE (−1) with randomly chosen heights at each excursion the interface for a little while, until it hits the Neumann boundary arc. Furthermore, if one tosses a fair coin to decide whether one inserts +λ or −3λ, one will preserve the fact that the mean value is −λ i.e., the martingale property of the height-function, and in fact the ﬂuctuations of the height will be symmetric in both cases. Iterating this procedure and letting ε → 0 would provide the desired coupling. After this warm-up, let us turn to the actual proof. Our ﬁrst goal will now be to couple a GFF with boundary conditions −λ on R and 0 on R with a GFF with boundary − + conditions −λ on R and Neumann on R . Based on the previous considerations, the − + strategy of the coupling (illustrated in Fig. 7) now goes as follows: • Sample an SLE (−1) from 0 to ∞ that we denote by η. This is known to be a simple continuous curve from 0 to inﬁnity, that touches R on a fractal set of points, and does not intersect R . It can be therefore viewed as the concatenation of disjoint excursions away from the positive real line. • Inside each of the bounded connected component of H\η (each excursion of η corresponds to one such connected component), toss an independent fair coin in order to decide whether to choose +λ or −3λ boundary conditions on the part of the boundary of that component traced by the corresponding excursion of η, and keep Neumann boundary conditions on R . On the unbounded connected component of the complement of η, choose uniform −λ boundary conditions. This includes R and the “left-side” of the entire curve η (see Fig. 7). • Then inside each of the connected components of the complement of η, sample an independent GFF with the above-mentioned boundary conditions i.e., the sum of a 0-boundary GFF with the harmonic function h that has these boundary conditions. Our ﬁrst step is to check that: Lemma 1. The obtained ﬁeld is indeed a GFF in H with boundary conditions given by −λ on R and Neumann on R . − + Proof. The proof of this lemma goes along the same lines as for the radial SLE (−2) coupling with the GFF as for instance outlined in [5]. First, one notices that by properties of Gaussian processes, it is sufﬁcient to show that the law of ( f ) for every individual continuous function f with compact support in the upper half-plane is Gaussian with the right mean and variance. So, we ﬁx such a function f with compact support in H. Then, for each excursion of η away from the real line, we toss an independent ±1 coin, and for every time t,we deﬁne the harmonic function h in the complement of η[0, t ] via the following boundary conditions: Neumann boundary conditions on R , constant boundary conditions equal to −λ on R as well as on the left-hand side of η[0, t ], and constant boundary conditions λ or −3λ on the right-hand side of η[0, t ], depending on the sign of the coin-tossing of the corresponding excursion of η. We denote by F the σ -ﬁeld generated by η[0, t ] and the coin-tosses that occured before time t (i.e., corresponding to all excursions of η that started before time t). 66 W. Qian , W. Werner If we are given a point z in the upper half-plane, we see that t → h (z) will evolve like a continuous local martingale during the excursion intervals of η. This is exactly a consequence of the previous observation about SLE (−1) processes coupled with mixed boundary conditions. Note also that by deﬁnition, h (z) remains in the interval [−3λ, λ] and converges as t →∞ to h(z). Let us deﬁne M := f (z)h (z)dz. t t By dominated convergence, it converges almost surely and in L to f (z)h(z)dz, and furthermore, for every given t > 0, if τ denotes the ﬁrst time after t at which η hits the real line, then s → M will be a continuous bounded martingale. Furthermore, min(t+s,τ ) the quadratic variation of this martingale on this interval is exactly compensating the decrease of the Green’s functions in the complement of η (this is exactly the integrated version of Proposition 4 of Izyurov-Kytölä [12], see also Shefﬁeld [39] for the Dirichlet version): ND dM =−d f (x ) f (y)G (x , y)dxdy H\η[0,t ] ND where G denotes the Green’s function with mixed Dirichlet–Neumann boundary conditions (Neumann on R and Dirichlet elsewhere). The ﬁrst additional item to check is that the martingale property is preserved after τ , which follows directly from the coin tossing procedure (indeed, if τ < t + s, then the conditional expectation of M given t t+s F will be exactly M —to see this we can ﬁrst discover η[τ , t + s] and then note that τ τ t t t the contributions due to the coin tosses that occur during [τ , t + s] are symmetric and cancel out). In other words, for all positive s, we have that M = E [M |F ], and letting t t+s t s →∞, M = E [M |F ]. t ∞ t The second additional item to check is the t → M is in fact continuous on all of R . This follows directly from the deﬁnition of M and the fact that t → η is known + t t to be a continuous curve. Hence, we now know that t → M is a continuous bounded martingale, i.e., a Brownian motion time-changed by its quadratic variation. In order to conclude, we just need to justify the fact that ND ND M = f (x ) f (y)(G (x , y) − G (x , y))dxdy. H H\η Indeed, if this holds, then we can conclude just as in [39]. So, what remains to be checked is that the measure dM puts zero mass on the closed set of times at which η hits the boundary. Here, we can use the fact that the deﬁnition of M shows for any stopping times σ< σ such that η and η lie on the real line, one has M = M unless η σ σ σ σ made an excursion into the support of f between σ and σ , and we know (because η is continuous and the compact support of f is at positive distance from the boundary) that almost surely, only ﬁnitely many excursions of η do make it into the support of f . The second step in the proof of the theorem is to notice that once all of η has been traced, it is possible to iterate this coupling inside each of the bounded connected compo- nents of the complement of η (indeed, the boundary conditions there are again constant on one arc, and Neumann on the real segment). More precisely, we deﬁne the random function h (z) obtained after n iterations of “layers” of SLE (−1) processes with the ran- n 4 dom height-gaps. The function h /λ takes its values in {−2n − 1, −2n +1,..., 2n − 1}. n Coupling Gaussian Free Fields 67 Iterating the previous constructions shows that adding h to the GFF with Dirichlet boundary and Neumann boundary values in the complement of these n SLE (−1) lay- ers constructs indeed a mixed-GFF in H with boundary conditions given by −λ on R and Neumann on R . − + Let us now again ﬁx a smooth function f with compact support away from the real line. Then, it is easy to see that almost surely, there will be a value n such that the n -th 0 0 n n SLE (−1) layer will be under the support of f , so that for all n ≥ n , ( f ) = ( f ). 4 0 Hence (given that if a sequence of Gaussian random variables converges almost surely, it converges also in law to a Gaussian random variable), we conclude readily that the limit ( f ) deﬁnes also mixed GFF in H with boundary conditions given by −λ on R and Neumann on R . − + In other words, it is possible to ﬁrst sample the entire inﬁnite branching tree of SLE (−1) processes, together with their labels, and then to sample conditionally inde- pendent GFFs in each of the connected components of its complement (mind that all these GFFs have constant boundary conditions, and that the constant is in λ +2λZ), and that one gets exactly a GFF in H with boundary values −λ on R and Neumann on R . − + A third step is to notice that this SLE (−1) exploration tree is exactly the same as the one that one would have drawn if one would have explored the collection of all boundary touching 0-level lines of a GFF with boundary conditions −λ on R and 0 on R .In − + particular, this shows that: Proposition 2. One can couple a GFF (with boundary conditions −λ on R and 0 on R )withaGFF (with boundary conditions −λ on R and Neumann on R )in + − + ˜ ˆ such a way that the only difference between and lies in the signs of the height jumps on the arcs of their common underlying branching tree. Note that the previous ALE-type decomposition of is in fact a deterministic function ˆ ˆ of ; the traced arcs are exactly the collection of all level lines of with height in 2λZ that intersect R . Finally, to conclude the proof of Theorem 1, we need to come back to the study of entirely Dirichlet vs. entirely Neumann boundary conditions. Let us start with a Dirichlet GFF , consider its boundary touching level arcs at height 0, toss an independent fair coin for each of them, and deﬁne as in Theorem 1. In order to prove that is a realization of a Neumann GFF, we use a limiting procedure: If we map the previous u u ˜ ˆ coupling of and onto the unit disc, we see that, if we deﬁne ∂ and ∂ the two 1 2 disjoint arcs on the unit circle separated by the points exp(i (π − u)) and exp(i (π + u)) ˆ ˜ for some very small u, and one considers the GFFs and with boundary conditions u u −λ on the small arc ∂ and on the long arc, 0 boundary condition for and Neumann condition for , one can couple the two ﬁelds so that they share the same ALEs and the difference is described as above. Now, when one lets u → 0: – On the one hand, one can see that it is possible to couple all with the GFF with Dirichlet boundary conditions, so that when one restricts it to any given set at positive distance from −1, then almost surely, coincides exactly with for all small enough u (one way to see this is to use the coupling of with a Brownian loop-soup + a Poisson point process of excursions away from the small arc, as for instance in [19,30]). This shows in particular that all the ALE arcs of that are at some positive distance from −1 will stabilize to those of : More precisely, each level arc at height 0 of will be almost surely a level arc of for all sufﬁciently small u. 68 W. Qian , W. Werner ˜ ˆ Fig. 8. Top: The boundary conditions for + λ and + λ in the semi-disc. Bottom: The same ALE with different heights. On the left, alternating 0 and 2λ will create the +λ boundary condition on the horizontal line. On the right, the random height-jumps will create the Neumann boundary condition on the horizontal line ˜ ˆ – If we couple each with an as in Proposition 2 and in such a way that the signs u u of the height-jumps on the boundary-touching level arcs of the latter coincide with those of on those arcs that are also boundary-touching level arcs of , then the ˆ ˆ gradient of will stabilize as well. In fact, if we shift in such a way that the u u boundary conditions of the ALE cell that contains the origin are the same for as the value for (this boundary value is ελ for ε = +1 or ε =−1), then this shifted ﬁeld will also almost surely stabilize to . – On the other hand, the law of , when viewed as acting on functions with zero mean will converge to that of a Neumann GFF in the unit disk (this follows from the fact that the corresponding covariances converge), so that the limiting ﬁeld is indeed a realization of the Neumann GFF. This concludes the proof of Theorem 1. Let us summarize in a picturesque way the CLE-type description of the GFF with mixed boundary conditions, in Figs. 8 and 9. Let us make here one comment that will be useful later in the paper. Consider the Neumann–Dirichlet ALE in the semi-disc as in Fig. 8, with Neumann boundary condi- tions on the horizontal segment. Just as for CLE in the unit disc, one can immediately relate the covariance of the ﬁeld at two points x and y to the expectation of number N (x , y) of loops or arcs that disconnect both these points from the semi-circle (indeed, the ﬁeld in the neighborhoods of x and y will be 2λ times the sums of the same N (x , y) coin tosses plus zero-expectation terms that are conditionally independent for x and y). More precisely (we state this as a lemma for future reference): ND Lemma 2. The Neumann–Dirichlet Green’s function G (x , y) in the semi-disk (which is equal to the sum G (x , y) + G (x , y) where G is the Dirichlet Green’s U U U function in the unit disc) is equal to (2λ) times the expectation of N (x , y). In particular, when x and y are both on the segment [−1, 1], then the Dirichlet–Neumann Green’s function G(x , y) in D (mind that when x and y are on the real axis G(y, x ) ∼ Coupling Gaussian Free Fields 69 Fig. 9. Left: Symmetrizing the boundary touching ALE for mixed Dirichlet–Neumann conditions creates a symmetric CLE -type picture. Right: One can then complete with independent usual CLE in the connected 4 4 components of the complement in the top half of the picture, toss an i.i.d.coin for the sign of the height-gap for each of the loops of the obtained ﬁgure, and one reconstructs a GFF with mixed Neumann–Dirichlet boundary conditions in the top semi-disc. If one forces the height-gaps of the loops that intersect the horizontal axis to alternate, then one constructs the Dirichlet GFF −1 π log(1/|y − x |) as y → x, i.e., it explodes twice faster as when x is not on the real axis) is exactly equal to (2λ) = π/2 times the expected number of nested ALE arcs that disconnects them both from the semi-circle in Fig. 8 (this number of arcs is then the ˜ ˆ same for both ﬁelds and ). 5. Relation to Soups of Reﬂected Loops and Consequences In the previous sections, we have generalized the construction of ALEs and CLE that had been performed for the Dirichlet GFF to the cases of the Neumann GFF and of the GFF with mixed Neumann–Dirichlet boundary conditions. The goal of the present section is to explain how to generalize the results of [18,19,30,40] that relate CLE and the Dirichlet GFF to Brownian loop-soups, to the case of Neumann boundary conditions. Here, we assume that the reader has these papers (and in particular [30]) in mind or at hand, as we will refer to them frequently. It is again more convenient to ﬁrst focus on the case of mixed Dirichlet–Neumann boundary conditions—the case of purely Neumann boundary conditions can then be deduced via a similar limiting procedure as above. Let us for instance choose to work in the semi-disc D ={z :|z| < 1, (z)> 0} with Dirichlet boundary conditions on the semi-circle (that we will denote by ∂) and Neumann boundary conditions on the segment I =[−1, 1]. We can then consider the Brownian motion in D, that is killed on ∂ and reﬂected orthogonally on I . This is a reversible Markov process, and all the construction of the corresponding loop measure and loop-soups works without further ado: – One can deﬁne the measure μ on (unrooted) loops of reﬂected Brownian motions in D (i.e., reﬂected on I and killed on ∂). One can relate it directly to the usual measure μ on unrooted Brownian loops in the unit disc as follows: Deﬁne ϕ the “folding” map that is equal to the identity in D and to z → z on the symmetric 70 W. Qian , W. Werner image of D with respect to the real axis. Then, the image of μ under ϕ is exactly 2μ (or equivalently, μ is the image of μ /2 under ϕ). – One can deﬁne for each positive c, the soup L of reﬂected loops in D (with reﬂection on I and killing on ∂) as the Poisson point process of loops with intensity cμ (here we choose the normalization of μ and therefore also μ such that the occupation time of the loop soup L with intensity cμ is related directly to the square of the GFF in U when c = 1). We see that one way to construct L is to view it as the image under ϕ of the loop-soup L . c/2 – The appropriately normalized occupation time measure of the loop-soup L (that is, for c = 1) is distributed exactly as the appropriately deﬁned square of the GFF with mixed Dirichlet–Neumann boundary conditions in D. In summary, the coupling between the loop-soup L and the square of the Neumann–Dirichlet GFF in D works directly. Let us now explain why the loop-soup clusters will give rise to the structures that we studied in the previous section, in the same way in which loop-soup clusters in U give rise to CLE as shown in [40]. Let us ﬁrst recapitulate the notation that we are using for the different loop-soups. For each c, L will denote the Neumann–Dirichlet loop-soup in U D the semi-disc D with intensity c, L and L will denote the usual Dirichlet loop-soups c c with intensity c in U and D respectively, and L will denote the set of loops of L that I D intersect and are reﬂected on I . Hence, for instance, L \L is distributed like L , and c c the image of L under ϕ is distributed like L . c/2 Not surprisingly, the collections L will satisfy a chordal conformal restriction prop- erty (see [14,44] for background on those): Lemma 3. Consider the upper boundary of the union of all loops in L . This is a simple curve that satisﬁes the chordal one-sided conformal restriction property in D with marked point at −1 and 1, with exponent c/16. Proof. Note ﬁrst that the fact that the upper boundary of the union of all loops in L satisﬁes the one-sided conformal restriction property for some positive exponent α that is a constant multiple of c follows immediately from the conformal invariance of the reﬂected loop measure, and the deﬁnition of L . It therefore only remains to identify the multiplicative constant 1/16. The fact that the image under ϕ of μ is 2μ makes it possible to compute directly the mass for μ of certain families of loops. It will be convenient to work in the upper half plane. Consider the loop-measure for Brownian motion reﬂected on R and killed on R , and let us estimate the mass m(ε) − + of the set of loops that touch both R and the very small vertical segment [1, 1+ εi ].By applying the z → z map and by considering the reﬂection of the ﬁrst quarter plane along its vertical boundary, we get that it will be sufﬁcient to estimate the mass of the (non-reﬂected) Brownian loops in H that intersect both the vertical half-line i R and the union of the two segments [1,1+ i ε/2] and [−1, −1+ i ε/2]. When ε is small, this is approximately twice the mass of the loops that intersect i R and [1,1+ i ε/2] (the mass of the set of loops that intersect both segments being a smaller order term). But this mass of the loops in the upper half-plane that intersect both i R and [1,1+ i ε/2] is approximately hcap([1, 1+ i ε/2])/2 = ε /16 times the mass of Brownian bubbles in H rooted at 1 and intersecting i R.By[16], the mass of such bubbles is given by −1/6 times the Schwarzian derivative of the map z → z at the point 1, i.e., to −Sf (1)/6for 2 2 2 f (z) = z . We can then conclude that m(ε) = ε /32 + o(ε ). In order to relate this to the restriction exponent, we can recall that the probability that no loop in the Poisson point process L of Brownian loops in H (reﬂected on R and c − Coupling Gaussian Free Fields 71 I D Fig. 10. Sketch of L (left), L (middle) and L (right). The upper boundary of the union of the loops on the c c left picture is a restriction sample with exponent c/16. The upper boundary of union of the cluster touching I in the right picture is an SLE (ρ(c))—when c = 1, it is an SLE (−1) κ(c) 4 killed on R ) with intensity c intersect both R and [1, 1+ εi ] is given by exp(−cm(ε)) + − 2 2 which behaves therefore like 1 − cε /32 + o(ε ) in the ε → 0 limit. On the other hand, if g denotes the conformal map from H\[1,1+ εi ] onto H that leaves the points 0, ∞ 2 2 invariant and such that g (z) ∼ z as z →∞, then g (0) = 1 − ε /2+ o(ε ).The probability that a one-sided restriction measure on R in H of exponent α does not α 2 2 intersect [1,1+ εi ] is given by g (0) = 1 − (α/2)ε + o(ε ). Therefore we conclude that indeed α = c/16. We can already note that this value 1/16 is not surprising given our previous results relating the GFF with Neumann boundary conditions to SLE (−1), and the fact that the upper boundary of the union of an independent restriction sample of exponent 1/16 in D attached to I with all the loop-soup clusters in L that it intersects is an SLE (−1), see [49]. Hence, the ﬁrst SLE (−1) layer of the ALE-type construction is obtained by boundary touching clusters of Brownian loops of L . This is a ﬁrst step towards relating the previous level lines of the Neumann GFF constructions to Brownian loop-soup construction of the SLE (−1) and of the square of the GFF—which will be explained at the end of the present section. Let us now describe some consequences of the identiﬁcation of this exponent c/16 for general c ≤ 1: Proposition 3. Consider the loop-soup L with mixed boundary conditions and intensity c. Then, the upper boundary of the union of the loop-soup clusters that do touch I (as depicted in Fig. 10) is an SLE (ρ) curve where κ ∈ (8/3, 4] is related to c by the usual identity c = (6 − κ)(3κ − 8)/(2κ) and (8 − κ)(κ − 2) 8 − κ ρ = ρ(c) = − . 8 2 Proof. We know that the upper boundary of the union of all loops in L forms a one- sided restriction sample with exponent c/16, and that L forms an independent loop- soup in D (and therefore deﬁnes a CLE for κ(c) as in the statement of the proposition). The proposition now follows immediately from the following result from [43,49]: The upper boundary of the union of a restriction sample of exponent β with the loops of an independent CLE that they do intersect is an SLE (ρ) curve from −1to1in D, where κ κ ρ is the unique value in (−2, ∞) such that (ρ +2)(ρ +6 − κ) = β. 4κ 72 W. Qian , W. Werner When c = 1, then κ = 4 and one indeed gets ρ(1) =−1. But for instance when c = 1/2, then κ = 3 and ρ(1/2) = 5/8 − 5/2 which is somewhat unusual expression in the SLE/GFF framework. Note that using Theorem 1.6 in [26], one gets the explicit expression of the dimension of the intersection of the “Dirichlet–Neumann CLE carpet” with this real line. This proposition describes the reﬂected loop-soup construction of the ﬁrst layer of the ALE of the Neumann–Dirichlet GFF when c = 1 and of its generalization for c < 1. In order to construct the subsequent lower layers of the ALE, we can notice that the law of the picture that one observes when just looking at the trace of the loop-soup L in D ∩{z :(z)>ε} is absolutely continuous with respect to the trace of the loop-soup L in D ∩{z, (z)>ε} (this can be seen by ﬁrst noting that almost surely, the number of loops of L that touch both I and {z :(z) = ε} is ﬁnite, and that one could replace the portions of those loops below {z :(z)<ε/2} by portions of loops that do not touch I ). This absolute continuity makes it possible to deduce from the corresponding result [30] for loop-soups in U, the following fact: Conditionally on the upper boundary δ of the closure of the union of the loop-soup clusters in L that intersect I , the conditional distribution of the Brownian loops of L that lie below δ and do not intersect δ is exactly a Brownian loop-soup in the domain between δ and I , with intensity c and Dirichlet boundary conditions on δ and Neumann boundary conditions on I . This is due to the fact that resampling the very small loops that lie near δ is already sufﬁcient to ensure that the union of those loops with the Brownian loops that do intersect δ form connected clusters, as explained in [30]. This makes it possible, inside each of the connected components of D\δ that are squeezed between δ and I to use the loops of the original loop-soup L in order to construct the next layers of loops and so on. In summary: The construction of nested CLE using one single loop-soup that we pointed out in [30] can be generalized in order to construct the entire collection of nested ALE arcs (i.e., their SLE (ρ) generalization for c < 1) using one single loop-soup L . Further results worth pointing out are the following direct consequence of the fact that ϕ(L ) is distributed as L . In the following statement, we consider c ≤ 1, and we c/2 deﬁne κ ˜ and κ in (8/3, 3] resp. in (8/3, 4] to be the values respectively associated to c/2 and c: (6 − κ)(3κ − 8)/(2κ) = c and (6 −˜ κ)(3κ ˜ − 8)/(2κ) ˜ = c/2. Corollary 1. Consider a standard CLE in the unit disc (viewed as a random collec- κ ˜ tion of disjoint loops in the unit disc) and consider its image under ϕ. In this picture, one now has collections of possibly overlapping simple loops in D ∪ I , that can be decomposed into connected components. Then, the upper boundary of the union of all connected components that touch I is distributed exactly like the SLE (ρ) path described in Proposition 3. Here, the case c = 1 turns out to be special as it allows to relate directly the usual CLE (which is the scaling limit of the Ising model (see [7]) directly to the Neumann– Dirichlet GFF (note that just as the previous corollary, the following statement does not mention loop-soups but that its proof very much uses them)—we write this as a separate statement for future reference (see Fig. 11 for an illustration of the result): Corollary 2. Consider a standard CLE in the unit disc (viewed as a random collection of disjoint loops in the unit disc), and consider its image under ϕ. In this picture, one now has collections of possibly overlapping simple loops in D ∪ I , that can be grouped Coupling Gaussian Free Fields 73 Fig. 11. From CLE to the Neumann–Dirichlet CLE (sketch): A CLE (left), the overlay of the CLE and 3 4 3 3 its symmetric image (middle), the obtained clusters form the Neumann–Dirichlet CLE (right) into connected components. Then, the upper boundary of the union of all connected components that touch I is distributed exactly like the SLE (−1) path that deﬁnes the ﬁrst-layer of the ALE of the Dirichlet–Neumann GFF. D I Note that one can also study in a similar way the soup L ∪ L for all c ∈[0, 1] c c and c ≥ 0. This gives rise in the same way to nested SLE (ρ) layers for κ = κ(ρ) and all possible ρ> −2 (keeping c ﬁxed and letting c vary), More precisely, the upper boundary of the union of the obtained clusters that do touch I forms an SLE (ρ) process where κ ∈[8/3, 4] and ρ> −2 are determined by (6 − κ)(3κ − 8) c (ρ +2)(ρ +6 − κ) c = and = . 2κ 16 4κ Let us state the special case c = 1/2 and c = 1 as a separate corollary: D I Corollary 3. Consider the overlay of L with an independent L . Or equivalently, 1/2 1 consider a loop-soup L in the unit disc, remove all loops that are strictly contained in 1/2 the lower half-plane, and take the image under ϕ of the remaining ones. Then, the upper boundary of the union of the obtained clusters that do touch I forms an SLE (−3/2) process. It is interesting to emphasize that the various players in this result can be related directly to the Ising model [7,8,11]: – The CLE in D deﬁned by L is the scaling limit of the boundary touching + 1/2 cluster for a critical Ising model with + boundary conditions (more precisely, the CLE carpet which is the set surrounded by no loop has the law of this scaling limit). – The SLE (−3/2) process is the scaling limit of the lower boundary of the + Ising cluster touching ∂ for the critical Ising model with + boundary conditions on ∂ and free boundary conditions on I (mind that the free boundary conditions for the Ising model are a priori not related to the Neumann boundary conditions for the GFF). Hence, this last corollary can be viewed as a rather simple coupling between the scaling limit of the critical Ising model with mixed boundary conditions (+ on ∂ and free on I ) and the scaling limit of the Ising model with + boundary conditions. Finally, we come back to the c = 1 loop-soup and to its relation with the GFF. We now have seen three couplings in this Dirichlet–Neumann setting: – Between the ALE structure and the GFF (this is the coupling described in the previous sections). 74 W. Qian , W. Werner – Between the ALE structure and clusters of reﬂected loops (that we have just pointed out). – Between the soups of reﬂected loops and the square of the GFF (this is the isomor- phism theorem à la Le Jan [17] that works here without further ado). We now brieﬂy argue that, just as for the analogous case of the Dirichlet GFF [30], these three couplings can be made to coincide. Let us browse through the steps of the arguments: The idea will be to realize the coupling of the GFF, of the ALE structure and of the loop-soup as the limit when the mesh-size goes to 0 of a corresponding coupling built on metric graphs. In this discrete case, the key is the observation by Lupu that one can sample the GFF starting from its square (that is deﬁned via the soup of Brownian loops on the metric graph) by choosing independent signs for different loop- soup clusters, because they correspond exactly to the excursion sets away from 0 by the GFF on the metric graph. So, in the discrete metric graph structure, one has a soup of reﬂected Brownian loops that create clusters and the square of the GFF with the mixed Neumann–Dirichlet conditions, and one can the construct the Neumann–Dirichlet GFF itself by taking the square root of the density of the occupation time measure, and sampling independently the signs of the GFF for each cluster. When the mesh-size goes to 0, we know that: – The discrete GFF with these mixed boundary conditions converges to some con- tinuous GFF (the convergence in law can be seen from the convergence of the covariance functions because one is looking at Gaussian processes). – The discrete loop soup converges to a continuous one—see [15] for related conver- gence of loop-measure issues. – The renormalized occupation time of the discrete loop-soup converges to T , which is the renormalized occupation time of the continuous loop-soup. – As explained in [30], we can make these convergences simultaneous such that T is exactly the renormalized square of . – The clusters of macroscopic Brownian loops are exactly described via the SLE (−1) and CLE structures that we described above (this is a statement about the Brownian loop-soup). On the other hand, they can only be larger than the limits of the clusters of the random walk loops when the mesh of the lattice goes to 0. Let us outline in a handwaving way one possible way to argue that the limit of the cluster of the cable system loops cannot be strictly larger than the corresponding cluster of the limiting macroscopic Brownian loops. First, we can notice that for both the version on cable systems as for the continuum version, when one restricts the loop-soup to the subset of D that lies at distance at least ε from I , the picture is absolutely continuous with respect to the corresponding picture with Dirichlet boundary conditions on I instead of Neumann boundary conditions. Furthermore, this Radon–Nikodym derivative (on the cable systems) does converge when the mesh of the lattice goes to 0 (for each ﬁxed ε). If one combines this with the main result of Lupu [19] (that for in the Dirichlet case, the scaling limit of the cable-system loop-soup clusters are never strictly larger than the clusters of macroscopic Brownian loops), we conclude that the only way in which in the Dirichlet–Neumann case, the limit of the cable-system loop-soup clusters could be strictly larger than the clusters of Dirichlet–Neumann Brownian loops would be that in the latter case, two boundary-touching clusters of loops would end up being connected “through I ”. In other words, the scaling limit of the cable-system loop-soup clusters would consist of families of boundary touching clusters of Brownian loops that are only “glued together” along the boundary. In any case, the boundaries of the discrete clusters Coupling Gaussian Free Fields 75 Fig. 12. Illustration of the loop-soup cluster decomposition. Left: The upper boundary δ of a loop-soup cluster of reﬂected Brownian loops for c = 1, with the loops in the Neumann–Dirichlet loop-soup that do touch this upper boundary. The union of these loops is then distributed like a Poisson point process of Brownian excursions away from this upper boundary and reﬂected on the real line. Right: The other Brownian loops under δ form a conditionally independent Neumann–Dirichlet soup of reﬂected loops in the domain inbetween δ j j (Dirichlet boundary) and the real line (Neumann boundary) do converge to the boundaries of the continuous ones. This already enables us to apply the same arguments as in [30], and argue that the outermost level lines of at height λ and −λ (which consists of the SLE (−1) and the CLE loops above it) are exactly the 4 4 boundaries of the loop soup clusters. This is because we can explore the loop soup from ∂ and all the arguments in [30] remain valid as long as we do not discover any clusters touching I . But on the other hand, conditionally on the SLE (−1), restricted to each connected component under the SLE (−1) curve have ±2λ boundary conditions according to i.i.d. fair coins. If some of the discrete clusters are indeed glued together along I in the limit, then restricted to the corresponding components under the SLE (−1) curve would take the same sign, instead of independent ones. This leads to a contradiction. Hence the limit of the discrete clusters are exactly equal to the continuous ones. With this in hand, it is then possible to adapt the arguments of the proof in the Dirichlet case that we presented in [30]. This allows to generalize also the corresponding result of [30] to this case of mixed Neumann–Dirichlet boundary conditions: Conditionally on δ, the trace of the set of Brownian loops in L that do intersect δ is distributed exactly like the union of a Poisson point process of Brownian excursions in U (δ),awayfrom δ and reﬂected on I , with intensity α = 1/4(seeFig. 12). In other words, the relation between the previous three couplings and Dynkin’s isomorphism work all in the same way as in the Dirichlet setting. 6. Shifting the Scalar Version of the Neumann GFF and Related Comments We now come back to the proof of Proposition 1. By symmetry, we can restrict ourselves to the case where a ≤ 0. Recall ﬁrst very brieﬂy how the coupling between the Neumann GFF, its realization and the corresponding ALE A was established: We considered a GFF in the unit disc with mixed boundary conditions, free on a large arc and −λ on the remaining very small arc ∂ around the boundary point −1. Then, we coupled it with a GFF with −λ boundary conditions on the small arc and 0 boundary conditions on the large arc, in such a way that the collection of boundary touching level arcs with height in 2λZ of the two ﬁelds did exactly coincide. Then, we shifted by a multiple of 2λ so that the height of the cell containing the origin was equal to that of , and called this ﬁeld . u u Finally, we did let the size of the short arc shrink, and looked at the limit of and of u 76 W. Qian , W. Werner its collection of boundary-touching level arcs with height in 2λZ, which provided the coupling of with the ALE. Let us deﬁne b =−λ + a ≤−λ, and consider a GFF in the unit disk, with mixed boundary conditions just as except that the boundary condition on ∂ is b instead of −λ. Note that this ﬁeld is distributed exactly as a + . In particular, the boundary-touching level arcs of with height in 2λZ will be distributed exactly like the boundary-touching level arcs of with height in −a +2λZ. The argument at the end of the proof of the theorem showed that for a well-chosen coupling, the shifted ﬁelds could be made to coincide away from −1 for sufﬁciently small u. This implies that the law of the collection of boundary-touching level arcs of with height in 2λZ does stabilize as well, so that in the coupling of the theorem, the law of the collection of boundary-touching level arcs of with height in −a +2λZ is the limit as u → 0 (for an appropriate topology) of the law of the collection of boundary-touching level arcs of with height in 2λZ. In order to prove Proposition 1, we therefore just have to argue that this limiting law is that of an ALE, i.e., that it does not depend on the value of b. This will be a direct consequence of the following lemma: Lemma 4. For each b < −λ and for a given u , there exists an arc γˆ that separates 0 b the small arc ∂ from 1 in U, such that given γˆ , the conditional law of restricted 1 u to the connected component Uof U\ˆ γ that has 1 on its boundary, is exactly a mixed Neumann–Dirichlet GFF with Neumann boundary conditions of the unit circle part of the boundary of U, and −λ boundary conditions on γˆ . This lemma readily implies Proposition 1. Indeed, we can choose to start with and b b ˆ ˆ then to deﬁne for all u < u as the image of via the Möbius transformation u u 0 u of the unit disc that maps 1 onto itself and ∂ onto ∂ . Then, as u tends to 0, the 1 1 diameter of the image of γˆ under this automorphism vanishes. In particular, the conformal transformation that maps U onto U that keeps 1 ﬁxed, has a derivative at 1 that is equal to 1 and maps γˆ onto some ∂ tends almost surely to the identity map as u → 0(for the uniform convergence when restricted to any subset of U that is at positive distance from −1). Hence, the collection of boundary-touching level lines with height in 2λZ of does indeed converge in distribution to an ALE. Hence, it remains to explain how to derive Lemma 4: Proof. By conformal invariance, and shifting the ﬁeld by −λ, we can consider a GFF in the upper half-plane H with mixed boundary conditions: Neumann on R\[−1, 1] and equal to a ≤ 0on [−1, 1]. We will ﬁnd an arc γˇ joining a point in (−∞, −1) to a point in (1, ∞) for this ﬁeld, so that conditionally on this arc, the law of the ﬁeld in the unbounded connected component of its complement is a mixed Neumann–Dirichlet GFF with Neumann conditions on the part of the boundary that is on the real line and 0 boundary conditions on that arc. Such a coupling can in fact be obtained in a number of different ways. A natural option (we will mention other options after the end of the proof) is to use the coupling of the Dirichlet–Neumann GFF with a Dirichlet– Neumann loop-soup in H and a Poisson point process of excursions away from [−1, 1] in H that are reﬂected on R\[−1, 1] (see Fig. 13). This coupling can be viewed as the ﬁne-mesh limit of the corresponding coupling on a cable-system approximation; on the cable system, in order to deﬁne the GFF, one considers the clusters of loops+excursions, the square of the GFF is then the intensity of the total occupation time measure, and Coupling Gaussian Free Fields 77 Fig. 13. The Poisson point process of excursions away from [−1, 1] reﬂected on the other part of R (left). Adding the loop-soup clusters of the Neumann–Dirichlet loop-soup that intersect them and drawing the outer boundary γˇ (right) tosses an independent fair coin to decide the sign of the GFF for each cluster, except those that contain an excursion away from the boundary segment, for which the sign is negative (this is exactly Dynkin’s isomorphism theorem phrased in terms of cable-system loop-soups as in Lupu [18], see also [2]). On the cable-system, one can look at the union of all connected components that do touch the segment [−1, 1]. Conditionally on this set, the law of the cable-system GFF on the complement of this set is clearly a mixed Neumann–Dirichlet GFF, with Neumann boundary conditions on the real line and 0 boundary conditions on the other boundary points. When the mesh-size of the lattice goes to 0, we can note that the outermost boundary of this set will tend to the corresponding outermost boundary of the union of all excursion+loop clusters that touch [−1, 1], which leads indeed the desired coupling between and γˇ (a similar argument was used in the proof of Lemma 6 in our paper [30]). Let us make some comments about this proof: It is worthwhile emphasizing that for the boundary point at inﬁnity, an apparent contradiction is that the expected value of the ﬁeld was b + λ while it becomes 0 for the mixed Neumann–Dirichlet (with zero values) above γˇ . This is just due to the fact that the local set consisting of the union of all excursions and loop-soup clusters that they hit is not a thin local set (loosely speaking, it carries mass of the GFF) and that the probability that it is very large does not decay fast (see [2,37] for related considerations). Let us note that instead of using the loop-soup approach, a second closely related option would have been to use absolute continuity between the laws of the ﬁeld and the Neumann–Dirichlet GFF in H with −λ boundary conditions on [−1, 1] instead of b boundary conditions. Indeed, when one restricts these two ﬁelds to the complement of a ball of large radius R around the origin, then the Radon-Nykodim derivative between the law of the two tends (in probability) to 1, so that one can then use directly the level-lines for that we described in the previous sections. In some sense, the argument described in our proof was making use of an explicit way to couple these two ﬁelds. Another approach would for instance have been to adapt our proof of Lemma 1 to the ﬁeld for b ∈ (−2λ, 0), i.e., to describe explicitely a curve γˇ via the concatenation of some SLE (ρ ,ρ )-type excursions, using the coupling between GFF with piecewise 4 1 2 constant/Neumann boundary conditions and SLE type curves before the curve hits the Neumann boundary as derived by Izyurov-Kytölä in [12]. Here, the boundary conditions on the complement of γˇ would be free on R\[−1, 1], b on the part that is in [−1, 1], and they would be exactly as in Lemma 1 on the curve γˇ (−λ on one side, and either λ or −3λ on the other side). This concatenation of arcs would then be a thin local set. Proposition 1 would then follow from this result in a similar manner as from Lemma 4. We leave all this to the interested reader. 78 W. Qian , W. Werner As promised in Sect. 3, we now discuss brieﬂy the relation between the boundary- touching level-arcs of and those of . Let us give some details for the simplest possible case: Suppose that one traces a level line at height 0 of the Dirichlet GFF inside a connected component O where j j the boundary conditions for are −λ. This is also clearly locally a −λ-level line of as long as it does not hit the ALE. If it hits the ALE, then this particular level line of stays in O and bounces off from the boundary of the ALE; it will in fact create a loop that is entirely contained in O , and it does so in such a way that the −2λ side of that loop lies in the inside of the loop and not on the side of the ALE (so, for instance, if the level-line is traced in such a way to have −2λ on its left side, then when hitting the ALE, it would have to turn left). This level-line loop of is then also exactly the boundary of an ALE-cell of i.e., a level-line of at height 0 (in fact, in this particular case, j j it would actually be a CLE loop of , as mentionned before). Note already that if one would have followed an arc of the same 0-level-line of but if the boundary values of the cell O (for )was +λ instead of −λ, then the corresponding level line of that this arc is part of would have to turn in the other direction: When it hits the ALE, the level line of would bounce to the right instead of to the left and it would have traced the boundary of a neighboring ALE cell of . So, we see that the way in which the level-arcs of are hooked-up in order to create level-lines of very much depend on the sign of the jumps on the ALE arcs that it hits. If we now are looking at the same 0-level line portion of and try to see what level line of the Neumann GFF it will be part of, we see that the interaction rule with the ALE will be to bounce in one direction or the other depending on the sign of the height-gap along the ALE arc that it is locally hitting. This shows immeditely that the corresponding level line of will in fact be forced to end on the boundary of the original domain as soon as it successively hits ALE arcs with opposite height-gaps (see Fig. 4 for a sketch). Hence, there will exist level arcs with height λ for that do join two boundary points of the domain. As on the other hand, we know that this is not the case for (the CLE loops do not touch the boundary). We can conclude that the collection of all level lines A with height in λ +2λZ for is not the same as the collection of all level lines with height in λ +2λZ for (the former is not empty while the latter is empty). These local interaction rules can be easily generalized to the interaction between level-lines with height in a +2λZ (and therefore of the ALE A ) with the level-arcs of the ALE A for all a ∈ (−2λ, 0) (the previous discussion was dealing with the case where a =−λ). 7. Further Questions and Remarks We conclude this paper mentioning closely related work and work in progress: (1) As explained in [1,3], the nested CLE (or nested ALEs) approach to the GFF gives a very natural conformally invariant way to approximate the Liouville measures associated to the GFF. The results of the present paper enable (see also [3]) to do the same for the boundary Liouville measure for the Neumann GFF. (2) It is possible to generalize fairly directly most of the loop-soup part of the arguments to the case of oblique reﬂection instead of orthogonal reﬂection. For each given reﬂection angle θ = uπ with u ∈ (0, 1), one replaces the orthogonal reﬂection (corresponding to θ = π/2) by reﬂection with angle θ. In particular, one can then look at the soup of Brownian loops in the semi-disc D, with Dirichlet boundary Coupling Gaussian Free Fields 79 conditions on ∂ and reﬂected with angle θ on I , and with intensity c. Then, a simple computation shows that: Lemma 5. The upper boundary of the union of all loops in this loop-soup that intersect I is a simple curve that satisﬁes the chordal one-sided conformal restriction property in D with marked point at −1 and 1, with exponent cu(1 − u)/4. One can then, in a similar way as in the orthogonal case, describe the upper boundary of the union of the loop-soup clusters that touch I as an SLE (ρ) process, where κ(c) is as before and ρ is the value in (−2, ∞) such that (ρ +2)(ρ +6 − κ)/(4κ) = cu(1 − u)/4. However, caution is needed when one tries to related these loop-soup considerations to Gaussian ﬁelds because these reﬂected Brownian motion are not reversible. (3) Other work in progress related to the present paper involves a loop-soup approach in the spirit of [47] to SLE-type welding issues. Another natural and closely related point under investigation is the relation between such Neumann–Dirichlet type cou- plings with imaginary ﬂow lines of the GFF (some arguments of the present paper can indeed be fairly directly adapted). Acknowledgements. We acknowledge support of the Grant No. 155922 (WQ, WW) and an Early Post- doc.Mobility Grant (WQ) of the SNF. The authors are/were part of NCCR SwissMAP. We also thank Juhan Aru and Avelio Sepúlveda for many stimulating discussions about ALEs, as well as the referees for their comments. Open Access This article is distributed under the terms of the Creative Commons Attribution 4.0 Inter- national License (http://creativecommons.org/licenses/by/4.0/), which permits unrestricted use, distribution, and reproduction in any medium, provided you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. References 1. Aidekon, E.: The Extremal Process in Nested Conformal Loops. Preprint (2015) 2. Aru, J., Lupu, T., Sepúlveda, A.: First Passage Sets of the 2D Continuum Gaussian Free Field. arXiv e-prints (2017) 3. Aru, J., Powell, E., Sepúlveda, A.: Approximating Liouville Measure Using Local Sets of the Gaussian Free Field. arXiv e-prints (2017) 4. Aru, J., Sepúlveda, A.: (In preparation) 5. Aru, J., Sepúlveda, A., Werner, W.: On bounded-type thin local sets (BTLS) of the two-dimensional Gaussian free ﬁeld. J. Inst. Math. Jussieu (to appear) 6. Beffara, V.: The dimension of the SLE curves. Ann. Probab. 36, 1421–1452 (2008) 7. Benoist, S., Hongler, C.: The scaling limit of critical Ising interfaces is CLE(3). Ann. Probab. (to appear) 8. Chelkak, D., Duminil-Copin, H., Hongler, C., Kemppainen, A., Smirnov, S.: Convergence of Ising inter- faces to Schramm’s SLE curves. C. R. Math. Acad. Sci. Paris. 352(2), 157–161 (2014) 9. Dubédat, J.: SLE and the free ﬁeld: partition functions and couplings. J. Am. Math. Soc. 22, 995– 1054 (2009) 10. Duplantier, B., Miller, J.P., Shefﬁeld, S.: Liouville Quantum Gravity as a Mating of Trees. arXiv e-prints (2014) 11. Hongler, C., Kytölä, K.: Ising Interfaces and Free Boundary Conditions. J. Am. Math. Soc. 26, 1107– 1189 (2013) 12. Izyurov, K., Kytölä, K.: Hadamard’s formula and couplings of SLEs with free ﬁeld. Probab. Theory Relat. Fields. 155, 35–69 (2013) 13. Kemppainen, A., Werner, W.: The nested conformal loop ensembles in the Riemann sphere. Probab. Theory. Relat. Fields. 165, 835–866 (2016) 14. Lawler, G.F., Schramm, O., Werner, W.: Conformal restriction: the chordal case. J. Am. Math. Soc. 16, 917–955 (2003) 15. Lawler, G.F., Trujillo-Ferreras, J.: Random walk loop soup. Trans. Am. Math. Soc. 359, 767–787 (2007) 16. Lawler, G.F., Werner, W.: The Brownian loop soup. Probab. Theory Relat. Fields. 128, 565–588 (2004) 80 W. Qian , W. Werner 17. Le Jan Y.: Markov Paths, Loops and Fields. L.N. in Math 2026. Springer, Berlin (2011) 18. Lupu, T.: From Loop clusters and random interlacement to the free ﬁeld. Ann. Probab. (to appear) 19. Lupu, T.: Convergence of the two-dimensional random walk loop soup clusters to CLE. J. Europ. Math. Soc. (to appear) 20. Lupu, T., Werner, W.: A note on Ising, random currents, Ising-FK, loop-soups and the GFF. Electr. Commun. Probab. 21(13), 1–7 (2016) 21. Miller, J.P., Shefﬁeld, S.: Private communication (2010) 22. Miller, J.P., Shefﬁeld, S.: Imaginary geometry I. Interacting SLEs. Probab. Theory Relat. Fields. 64, 553– 705 (2016) 23. Miller, J.P., Shefﬁeld, S.: Imaginary geometry II. Reversibility of SLE (ρ ; ρ ) for κ ∈ (0, 4). Ann. κ 1 2 Probab. 44, 1647–1722 (2016) 24. Miller, J.P., Shefﬁeld, S.: Imaginary geometry III. Reversibility of SLE for κ ∈ (4, 8). Ann. Math. 184, 455–486 (2016) 25. Miller, J.P., Shefﬁeld, S., Werner, W. CLE percolations. Forum Math. Pi 5(e4), 1–102 (2017) 26. Miller J.P, Wu H.: Intersections of SLE Paths: the double and cut point dimension of SLE. Probab. Theory Relat. Fields. 167, 45–105 (2017) 27. Nacu, S., ¸ Werner, W.: Random soups, carpets and fractal dimensions. J. Lond. Math. Soc. 83, 789– 809 (2011) 28. Powell, E., Wu, H.: Level lines of the GFF with general boundary data. Ann. Inst. Henri Poincaré (to appear) 29. Qian, W.: Conditioning a Brownian loop-soup cluster on a portion of its boundary. Ann. Inst. Henri Poincaré (to appear) 30. Qian, W., Werner, W.: Decomposition of Brownian loop-soup clusters. J. Europ. Math. Soc. (to appear) 31. Rohde, S., Schramm, O.: Basic properties of SLE. Ann. Math. 161, 883–924 (2005) 32. Schramm, O.: Scaling limits of loop-erased random walks and uniform spanning trees. Israel J. Math. 118, 221–288 (2000) 33. Schramm, O., Shefﬁeld, S.: Contour lines of the two-dimensional discrete Gaussian free ﬁeld. Acta Math. 202, 21–137 (2009) 34. Schramm, O., Shefﬁeld, S.: A contour line of the continuous Gaussian free ﬁeld, Probab. Theory Relat. Fields. 157, 47–80 (2013) 35. Schramm, O., Shefﬁeld, S., Wilson, D.B.: Conformal radii for conformal loop ensembles. Commun. Math. Phys. 288, 43–53 (2009) 36. Schramm, O., Wilson, D.B.: SLE coordinate changes. N.Y.J. Math. 11, 659–669 (2005) 37. Sepúlveda, A.: On Thin Local Sets of the Gaussian Free Field. arXiv e-prints (2017) 38. Shefﬁeld, S.: Exploration trees and conformal loop ensembles. Duke Math. J. 147, 79–129 (2009) 39. Shefﬁeld, S.: Conformal weldings of random surfaces: SLE and the quantum gravity zipper. Ann. Probab. 44(5), 3474–3545 (2016) 40. Shefﬁeld, S., Werner, W.: Conformal loop ensembles: the Markovian characterization and the loop-soup construction. Ann. Math. 176, 1827–1917 (2012) 41. Wang, M., Wu, H.: Level lines of Gaussian free ﬁeld I: zero-boundary GFF. Stoch. Proc. Appl. (to appear) 42. Wang, M., Wu, H.: Level Lines of Gaussian free ﬁeld II: whole-plane GFF. arXiv e-prints (2015) 43. Werner, W.: SLEs as boundaries of clusters of Brownian loops. C. R. Math. Acad. Sci. Paris 337, 481– 486 (2003) 44. Werner, W.: Conformal restriction and related questions. Prob. Surv. 2, 145–190 (2005) 45. Werner, W.: Some recent aspects of random conformally invariant systems. Ecole d’été de physique des Houches LXXXIII, 57–99 (2006) 46. Werner, W.: Topics on the Gaussian Free Field and CLE(4). Lecture Notes (2015) 47. Werner, W.: On the spatial Markov property of soups of oriented and unoriented loops, in Sém. Probabilités XLVIII. Lecture Notes in Mathematics 2168. Springer, pp. 481–503 (2016) 48. Werner, W., Wu, H.: On conformally invariant CLE explorations. Commun. Math. Phys. 320, 637– 661 (2013) 49. Werner, W., Wu, H.: From CLE(κ) to SLE(κ, ρ), Electr. J. Prob. 18(36), 1–20 (2013) Communicated by H. Duminil-Copin
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