Why is Landau-Ginzburg link cohomology equivalent to Khovanov homology?

In this note we make an attempt to compare a cohomological theory of Hilbert spaces of ground states in the N=22\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathcal{N}=\left(2,2\right) $$\end{document} 2d Landau-Ginzburg theory in models describing link embeddings in ℝ3 to Khovanov and Khovanov-Rozansky homologies. To confirm the equivalence we exploit the invariance of Hilbert spaces of ground states for interfaces with respect to homotopy. In this attempt to study solitons and instantons in the LandauGiznburg theory we apply asymptotic analysis also known in the literature as exact WKB method, spectral networks method, or resurgence. In particular, we associate instantons in LG model to specific WKB line configurations we call null-webs.


Introduction and discussion
A quest for a TQFT describing Khovanov invariants [53], a categorification of Jones polynomials -Wilson loop averages in the 3d Chern-Simons theory [24,69,78], -or more desirably Khovanov-Rozansky invariants [54,55], or even more generally superpolynomials [21], delivering categorification to HOMFLY-PT invariants, has led to a wide and profound development in the both physics and mathematics, see e.g. [3, 4, 6, 14-17, 41-44, 55, 60, 64, 73, 82-84]. 1 See also a recent nice review [75]. In this note we will discuss an approach proposed by Witten [80,82] using equivariant Morse theory on a field space emerging as a Kaluza-Klein reduction of six-dimensional (2,0) theory on a cigar. The link is associated to a 'tHooft operator insertion giving specific boundary conditions for fields [67]. This formulation is enormously complicated for a practical use, say, an explicit calculation of invariants. Then further simplifications were proposed in [29,31]. The theory descends to an effective IR 2d N = (2, 2) Landau-Ginzburg (LG) theory with the target space given by a universal cover of the monopole moduli space. The link is encoded in a half-supersymmetric interface representing a "moving" singular monopole probe.
This note is a companion of [39] where this idea was checked. It was shown that to construct an analog of Khovanov homology for a link L it is enough to consider a moduli space of a certain fixed number of monopoles. The Hilbert space E(L) of perturbative ground states is spanned by vectors associated to critical points of a Morse height functional h(L). It is naturally bi-graded by the fermion number F and by central charge Z appearing in discrete portions of πi, so that Z = πiP, where P ∈ Z. In the presence of a link interface one nilpotent supercharge Q is preserved. Hilbert space E(L) plays the role of Morse-Smale-Witten complex, while Q acts as a differential on this complex [76]. The non-perturbative Hilbert space is defined as cohomology: LGCoh(L) := H * (E(L), Q) = The Euler characteristic -supersymmetric index [11] -of this complex gives Jones polynomials. In [39] LGCoh(L) was argued to be an invariant of Reidemeister moves and therefore an invariant of link L. As well it was shown in several examples to be isomorphic as a bi-graded vector space to the Khovanov link homology we denote here as KHom(L). Generic argument for equivalence between LGCoh(L) and KHom(L) is still missing: LGCoh(L) This note is devoted to an attempt to deliver this missing argument. 1 The literature on generalizations and physical constructions of knot/link invariants is extremely rich.
Here we try to mention just some of possible directions. We use the following arguments. One associates to embedding of link L certain interface path℘ on parameter space P of the LG theory (see figure 1). The invariance of this construction for different link embeddings follows form the isomorphism of cohomologies: for homotopic paths℘ and℘ . Despite this isomorphism the very complexes E(℘) and E(℘ ) may be quite different. Relations between their generators -soliton-interface bound states -are governed by 2d wall-crossing phenomena [13]. So the cohomology is indeed an invariant of the path homotopy equivalence class [℘], while complexes E(℘) may vary from representative℘ ∈ [℘] to another representative. We will find distinguished representa-tive℘ 0 for each class [℘] such that the corresponding complex repeats the combinatorial construction of the Khovanov homology [8]: JHEP05(2019)085 points in our setup. Moreover we conjecture that instantons in the LG model correspond to a specific critical WKB web configurations we call null-webs.
In section 3 we review the construction of LGCoh(L) under the prism of spectral analysis, consider wall-crossings acting by morphisms on LGCoh(L), and finally construct a wall crossing morphims mapping LGCoh(L) to a complex isomorphic to KHom(L). The vacua in the LG model on the SU(n) monopole moduli space are in one-to-one correspondence with tensor powers of SU(n) irreducible representations. However this set has two descriptions -two "nice" basis choices: tensor product basis and isotypical basis. R-matrix acquires a simple diagonal form in the isotypical basis. And to establish the morphism between LGCoh(L) and KHom(L) we exploit an "isotypical" interface performing isotypical decomposition of LG vacua.
Afterwards in section 4 we construct su n Landau-Ginzburg link cohomology n LGCoh(L) starting from the monopole moduli space arising in a (2,0) six-dimensional theory with a gauge algebra su n [10]. We argue that n LGCoh(L) is an invariant of link L. And, finally, in section 5 we compare n LGCoh(L) to Khovanov-Rozansky link homology [55], we denote it as n KRHom(L). In particular, we argue that LG cohomology for a link and its resolutions should satisfy an exact triangle relation: LGCoh t This exact triangle relation is a categorification of skein relations for the HOMFLY link diagrams, a starting point for Khovanov-Rozansky construction. In appendix we put some examples of explicit applications of methods discussed along this note, in particular, we calculate explicitly 3 LGCoh(H) for Hopf link H and observe it coincides with 3 KRHom(H). Remarks 1. It is well-known that the link invariants are actually invariants of knotted and linked ribbons rather than thin strands due to framing anomaly. Ribbon twists affect an overall monomial multiplier of the link polynomial. Stripping off this monomial factor one gets link invariants. Therefore we consider all the polynomial equivalences modulo overall monomial factor. Alternatively, we claim bi-graded vector space isomorphisms modulo overall degree shifts (P, F) → (P + a, F + b).
2. We should mention that asymptotic expansion we use differs slightly from one used in the spectral networks literature [32-37, 46, 62], see footnote 4 on page 7. Therefore despite the methodology does not change we trade the term "spectral network" for "WKB web". 3. In [31] rich algebraic A ∞ -and L ∞ -structures were discovered hidden in the instanton processes governing LG models. Our construction of null-webs is motivated by a -3 -

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search for a simpler LG instanton construction. So it would be interesting to observe A ∞ -and L ∞ -structures hidden in null-webs if there are ones.

A relation between a notion of Chern-Simons (q, t)-refinement introduced in [3] and
LG cohomology in the formulation used in this note is still missing. One may hope to present such a relation in terms of spectral analysis. In this spectral analysis differentiable connections should be substituted by lattice-like difference operators, see e.g. [66,71,86], and recent development [23] in exponential deformation of spectral networks may turn out to be a suitable description on this route. 5. We argue that one can choose a distinguished path℘ 0 on P such that the LG complex becomes isomorphic to Khovanov's one, however there is an intriguing question if one can distinguish path℘ 0 from other representatives in its homotopy class giving different complexes a priori. Consider a Kähler manifold X of complex dimension N , we index its coordinates with capital Latin letters I = 1, . . . , N . This manifold is endowed with the Kähler metric g IJ . Also consider a holomorphic function W : X → C, in physical setup we refer to it as a superpotential. We will refer to critical points of W as vacua and denote them by small Latin letter indices from a vacuum set: i ∈ V.
Define a left (right) Lefschetz thimble L i (ζ) of phase ζ for a critical point φ i of W as a N -dimensional real surface in X, a union of paths satisfying: approaching a critical point φ i in the limit s → −∞ (s → +∞). Lefschetz thimbles are nice integration cycles for the integrals of type:

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Notice in the W -plane Lefschetz thimbles are represented by lines of constant slope πi + Arg ζ, consequently integral (2.2) taken along a Lefschetz thimble converges: Now we consider an n-dimensional complex space P spanned by coordinates z a and a family of functions W : X × P → C holomorphic in both types of variables. A bundle of integrals over P: has monodromies called Picard-Lefschetz monodromies corresponding to intersecting Lefschetz thimbles [47]. If a critical point j intersects a Lefschetz thimble L i (ζ) the integral (2.3) acquires a monodromy: Here µ ij is up to a sign an intersection number of thimbles L i (ζ) and L j (ζ) and is also referred to as a Maslov index [5]. From the physical point of view µ ij has an interpretation of an index [13,47,48] of ij-solitons.

Asymptotic Berry monodromy
An alternative way to construct this monodromy and therefore to count contribution of intersections of Lefschetz thimbles is to consider a natural Berry connection on this bundle of integrals. This connection constuction is somewhat analogous to the construction of tt *connection [13]. 2 In particular, in the quasi-classical limit ζ → 0 the major contribution to the integral (2.3) is accumulated near critical points of W , therefore any insertion in the integrand O a having a multiplier of dW along any direction in the X-space is quasiclassically 0. Therefore insertions O a form a ring isomorphic to C[φ I ]/dW , usually called a chiral ring of operators in the 2-dimensional N = (2, 2) Landau-Ginzburg model [48]. Furthermore we notice that the derivatives ∂ za along the base P act quasi-classically by multiplication by ∂ za W (φ I |z a ) in this ring, this operation induces a natural connection. To be more specific suppose we choose a set ofÔ a := ∂ za W (φ I |z a ) in the chiral ring, then the vector Ψ := ( O 1 , . . . , O n ), where denotes averaging with measure (2.3), is a section of a connection: 3 More elaborated relation between G-opers and Gauss-Manin connection constructed from solution to a G-Hitchin system can be found in [20]. 3 Notice that the real tt * -connection has an anti-holomorphic part in contrast inducing in this way a non-trivial Zamolodchikov metric on the parameter space P [12]. where C a are ring structure constants: and A a are connection components of order O(ζ 0 ). Further we consider a complex line z a (x) : C → P and pull back our connection ∇ a to ∇ := ∇ a dza dx on C. Then Ψ is a solution of a linear system of ordinary differential equations: Then the analysis is quite similar to the study of differential equation solution asymptotics due to G. Stokes, also known as a Wentzel-Kramers-Brillouin (WKB) method in physics (see e.g. [25]). We search for a solution in the following form: The zero order approximation reduces to an algebraic equation for the eikonal pdx, this algebraic equation defines a branched cover Σ over C: This is an equation defining a complex curve Σ with a meromorphic differential λ := p dx. We choose some trivialization of the branched cover π : Σ → C: a collection of branching points -zeroes of the discriminant of (2.9) with respect to p -and a collection of cuts (see figure 2). On a set C c = C \ {branch cuts} a global choice of the order of the roots p (i) can be made. Thus we have a well defined map s : Σ \ π −1 {cuts} → Z that associates to each point on Σ not lying on the cut an order number of the cover sheet it is lying on. We continue the definition of the root ordering to the branching points and associate to each branch point and cut an element of the Galois group of the spectral cover (2.9) as a polynomial in p. Different roots p (i) are naturally identified with the choice of the Lefschetz thimble, or vacuum, in (2.3). In theories whith some extra symmetry where the vacua can be labelled by weights of some group the Galois group of the cover can be naturally identified with the Weyl group [32-36, 46, 62]. Now one has a linear space of asymptotic solutions to (2.7), however, it turns out, an expansion over the asymptotic solutions with constant coefficients can not be a good global solution to equation (2.7). An easy way to see this is to notice that in branching points the asympotic solutions get Galois monodromies as we mentioned, however connection ∇ is flat in projections of the branching points down to C. And it is clear that in the neighbourhood of the branching point of type (ij) the asymptotic form (2.8) is invalid since p (i) − p (j) is close to zero. Let us have here a recipe to construct a corrected version of the asymptotic expansion, details and derivation of it can be found in various literature sources [25,[32][33][34][35][36][37].
WKB recipe. We cut the base C by real WKB lines (also called Stokes lines, or S-walls).
The set of lines consists of two subsets: primary lines and descendant ones. A primary line of type ij starts from the projection of the branching point of type (ij) and satisfies: where ∂ t is a tangent vector to the line (see figure 3(a,b)). Notice that ij-line and ji-line are not equivalent, and there are two possible generic patterns of WKB lines near a projection of a simple branching point. In joints of primary lines new descendant lines are born, in particular, if ij-and jk-lines intersect each other, a new ik line is born in the joint, it satisfies the same equation (2.10) (see figure 3(c)).
Then any new intersection of primary lines with descendant and of descendant ones among themselves gives a birth to new descendant lines. We call a collection of all WKB lines for given ζ a WKB web W ζ . 4 Consider a set L formed by formal sums of oriented real paths on Σ with coefficients being non-negative integers. We can endow this set with associative unital multiplication by imposing a multiplication law for two arbitrary paths ℘ 1 and ℘ 2 : 0, if the beggining of ℘ 1 does not coincide with the end of ℘ 2 concatenation of ℘ 1 and ℘ 2 , otherwise (2.11) 4 The rules for constructing WKB webs and calculating their contributions are the same as ones for spectral networks [32][33][34][35][36]. However spectral networks appear in a limit of large conformal dimensions in CFT formulation [85], or in the limit 1,2 → 0 of the Ω 1 , 2 -background in the class S theory formulation. From the point of view of connection like (3.8) WKB web limit corresponds to ζ → 0 limit while spectral network limit corresponds to large representation spin limit [38]. We construct detours D(℘, ζ) ∈ L depending on oriented path ℘ on C and phase ζ following two rules: Where π −1 implies a lift of path ℘ to all the sheets of the cover Σ.
2. If the path ℘ intersects W ζ along a line in a point p, the point p splits path ℘ into two parts ℘ − and ℘ + . Then new detours are Here η is a formal parameter. The elementary detour d p, for a ij-WKB line is calculated as follows. One considers a line segment¯ going from the source of the line to the point p, then Where¯ −1 implies that we consider the opposite orientation of the segment¯ , and d source is simple for a primary WKB line, it is just a gluing of lifts to i th and j th sheets across the cut, and for a new-born ik line in a generic junction p jun (see figure 4) we have: The system of detours has a natural grading -"detour degree" -weighted by a formal parameter η, generically we imply η = 1 however sometimes we will use this grading denoting it as D (k) : As a result we get an expression for D ∈ L in a form of a formal sum of paths with positive integer coefficients. It is easy to translate each such a formal sum of objects into a set of objects and backwards. We just imply that a positive coefficient defines how many times an object contributes to a set:

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Due to simplicity of this transition we call the latter set a set of detours and denote it by the same notation D(℘, ζ), for example, this allows us to rewrite a formal sum in a tautological form D(℘, ζ) = γ∈D(℘,ζ) γ Having constructed this system one can define an asymptotic solution of (2.7) being a path-oriented exponential as a matrix in coordinates associated to vacua V having the following expansion:  , where s is a map from points on Σ enumerating cover sheets defined after (2.9). And the form ω is defined in the following way (see [39, appendix A]). For each root p (i) we have a one-dimensional null space ψ (i) : Then on the i th sheet of the cover the form ω (i) is defined as We should stress that the path ordered exponent and similarly detour decomposition satisfy traditional evolution composition property:

Thimbles from WKB lines
We have considered a complex line z a : C → P, now we consider a one-dimensional path ℘ ⊂ C, map z a lifts it to some path℘ in P. We can calculate parallel transport in the bundle of the integrals B i along the path℘ using jumps (2.4) and pull it back to ℘, or alternatively we can calculate the same parallel transport using the pulled back connection as in (2.18), the results should coincide. Using this equivalence one can associate detours to intersections of Lefschetz thimbles. Advantage of this approach is two-fold. First of all, an explicit form of the thimbles, a solution to (2.1) with prescribed boundary conditions is hard to calculate even numerically since this is not a canonical Cauchy problem, in the WKB web formalism this problem is mapped to a one-dimensional one that can be easily solved at least numerically. 5 Then one has a simple expression as an integral of form ω for the Maslov index identified with the eta-invariant of the Dirac operator in the soliton background [31,39] that is also hard to calculate from the first principles. 5 Powerful software for constructing spectral networks is available at [63]. Let us be more specific. Suppose our path ℘ intersects the WKB web W ζ in a collection of points p α : Suppose to a point p α we associate an elementary detour d pα in the sandwiching formula (2.13) from intersection with a ij-WKB line. Therefore we claim that at the liftp α of p α to℘ the i th Lefschetz thimble intersects the j th critical value. The corresponding difference of values of W in the critical points and the index read We have not put an equality for the index since generically the integral gives a complex number. However we can rescale an overall phase of the integrals B i , similarly it is reasonable to compare only relative indices for the same boundary vacua values i and j from physical reasons [31]. In this case the ratio of indices is an integer.

Half-supersymmetric interfaces in the Landau-Ginzburg theory
Those data we have used to define Lefshetz thimbles in subsection 2.1 can be applied to define 2d N = (2, 2) Landau-Ginzburg theory. We consider chiral superfields Φ I = φ I +. . ., then the action reads: A detailed description of this theory can be found in [31,48].
Here we just remind some basic properties: 1. The vacua of the theory on the real line are in one-to-one correspondence with the critical points of W we denoted φ i , i ∈ V.
2. Classical finite energy field configurations saturating BPS bound, solitons, are solutions to (2.1) interpolating from vacuum i to vacuum j and with the fixed phase We introduce half-supersymmetric interfaces following [31] by considering a Morse height functional h : Y → R on the space Y = Map(R x → X), where x is a spatial coordinate of Landau-Ginzburg world-sheet (x, t). As a parameter for this height functional one can choose now a real path℘ ⊂ P. Suppose we have chosen some explicit parameterization z a (ρ) ∈ P for℘ where ρ is a real parameter along ℘, then, explicitly, the height functional is given by the following expression:

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Where σ is a 1-form defined locally as dσ = i 2 g IJ dφ I ∧ dφJ . Then the field theory is formulated as supersymmetric quantum mechanics (SQM) with the target space Y . We will discuss the SQM formulation in the next subsection. Here we just review the construction of critical field configurations to the functional h. The interface preserves supercharges in standard notations of [48]. Critical field configurations of the functional h are described as solutions of the following equation: A variation of h with respect to φ I (x) will give a complex conjugated version of this equation.
In an adiabatic limit where the change rate for parameters is very slow |dz a /dx| Λ −1 W , where Λ W is the maximal soliton width, solution descends to two classes.
The first class of solutions -the hovering solutions -are simply reminiscent of the local vacuum solution. They are described by fields which at each x are critical points for W (φ; z(x)) for the same value of x. In equations: if φ I i (x) is a critical field configuration: (where the exterior derivative only takes derivatives with respect to φ I ) then, since the z a (x) vary continuously along some path℘ ⊂ P once we have a chosen critical point i at some x 0 the field φ I i (x) will evolve continuously. (Here we use the assumption that we have a family of Morse superpotentials so that critical points never collide.) We denote this solution Hov℘ ,ζ (i, i).
In addition to the hovering solutions there are also solutions where solitons are localized near binding points. Consider an effective x-dependent central charge for a pair of hovering solutions: Binding points x c are defined by an equation: In the adiabatic limit we may think parameters z a (x c ) are approximately constant. In the vicinity of binding point x c the soliton solution to (2.1) having small width of order Λ W satisfies approximately (2.27) up to corrections of order O dza dx Λ W . This solution interpolates from vacuum i to vacuum j where it may be approximated by the hovering solution. We denote this solution as Slt℘ ,ζ (i, j).
In general, a forced soliton solution defines a function φ I (x) giving a parameterization of a path in the field space X. As to paths it is natural to associate a path algebra to solutions we also associate an algebra. An algebraic element is a formal sum with positive JHEP05(2019)085 integer coefficients. There is a natural bijection between algebraic elements and unordered sets of solutions given by rule (2.17). Multiplication is defined according to standard rules for a pair of simple elements and extended to all elements by linearity: if two solution paths in X are concantenable the result of multiplication is a solution representing concatenated path, otherwise the result is zero. Using our notations we could rewrite this rule in the following compact form: To construct a set of adiabatic solutions, we form rules for corresponding algebraic elements S(℘): 1. If the path℘ does not have binding points then: If the path has a binding point x c it splits the path℘ into two parts℘ − and℘ + , then the solution has a sandwich structure: We decompose this expression by a simple distributive law, and in this decomposition one should match vacua at all the non-loose ends.
3. If the path intersects multiple binding points one applies the rule (2.33) iteratively.
Compare these rules to the rules for constructing detours (2.12) and (2.13). A similarity between them is not occasional. To clarify this let us notice that intersection points (2.22) define exactly the set of critical points (2.30). Assume for a second that x is a complex parameter and a map z a : R → P can be continued analytically to a complex line z a : C → P. It is clear that i th root of the spectral cover (2.9) corresponds to a quasi-classical value of the following operator in the i th vacuum: In an (ij)-branching point i th and j th roots coincide, and i th and j th vacua do the same. So in the branching point the effective central charge (2.29) for ij soliton sector is zero. According to (2.10) along a ij-WKB line we have: In other words WKB lines define loci of complexified x where a condition is satisfied. To give a binding point condition for x c x in this relation should be real. This gives exactly a set of intersection points (2.22) for ℘ = R. Applying this identification we identify detours and contributions of intersecting Lefschetz thimbles discussed in 2.1.3 -solitons in the binding points. We conclude there is an isomorphism ξ: where I is a real interval I ⊂ C, and it is implied that the map z a : R → P can be continued analytically to a complex line z a : C → P.
One of the crucial properties of interfaces is their composability.
If ℘ denotes a particular path in P, or equivalently a path of theories, then reference [31] explains that one can define an object I[℘] in an A ∞ -category of interfaces between the theories associated with the initial and final points of the path. For composable paths ℘ 1 , ℘ 2 one can moreover define a product of interfaces so that where ∼ denotes homotopy equivalence of interfaces.
For adiabatic solutions to the critical field configuration equation we have the same property of composability: following naturally from composability of parallel transports (2.21).

Spectral analysis of instantons in supersymmetric quantum mechanics
Let us briefly review Witten's setup [76] of the supersymmetric quantum mechanics for the needs of the Morse theory. Consider a real n-dimensional Riemannian manifold Y R with coordinates u I , I = 1, . . . , N , metric g IJ (u) and Morse height function h : Y R → R.
One promotes coordinates u I to superfields U I = u I + θψ I +θψ I + θθD I then the action of the supersymetric quantum mechanics (SQM) reads [31]: The corresponding Morse-Smale-Witten (MSW) complex is defined as a vector space spanned by perturbative ground state wave functions with the differential defined by the action of supercharge Q. 6 If we integrate over auxiliary fields in the SQM action (2.39), the resulting field potential is proportional to (∂h) 2 , therefore perturbative vacua in the theory are labelled by 6 In LG cohomology construction the role of Q is played by Q ζ . In principle, one may be interested in considering the whole family of Q ζ parameterized by ζ. In our setup we are interested in one fixed value of ζ, thus we do not distinguish Q ζ and Q from now on. This complex has a natural grading by the fermion number F p = 1 2 (n − (p) − n + (p)), a half-difference of positive and negative eigen values of the Hessian of h in the critical point p.
To define non-perturbative vacua we should take into account non-perturbative corrections due to instantons. Instantons are defined as real action (2.39) saddle points, solutions to the steepest ascend flow (function h increases along the flow) equation: interpolating between critical point of h. Let us denote the space of solutions to (2.41) interpolating from a to b as I R a,b , then the action of the supercharge Q on the complex E reads: where ∇ / i is the corresponding Dirac operator on the instanton background [48]. The Hilbert space of ground states is defined non-perturbatively as cohomology: Obviously, the supercharge shifts the fermion degree by one, so the fermion grading coincides with the cohomological grading of the complex.
To study instantons with the use of proposed spectral analysis techniques we should identify somehow this problem to the construction of Picard-Lefschetz monodromies. We are going to propose a complexified version of the height function, then use it as a new superpotenial. In this setup instanton transitions would appear similar to soliton transitions in the interface background when we perturb our system a little bit like induced boiling of overheated liquid.
Steepest ascend equation (2.41) is the special case of the thimble equation (2.1), however the crucial difference is that the quantum mechanics target space Y R in comparison to X does not have a complex structure. A rather generic complexification continuation of the quantum mechanics was exploited in [81] to relate integration cycles with branes in a two-dimensional A-model. We will follow the easiest way. Define an n-dimensional complex manifold Y C = Y R × R n , with coordinates v I on R n . We introduce complex coordinates Z I = u I + iv I on Y C . We pull back the metric and extend analytically the Morse height 7 Naively, the complex should inherit a complex structure form the quantum mechanics Hilbert space, therefore from this point of view the complex should be a module over C. However we should stress that both the Morse theory and the Khovanov theory imply naturally an integer structure, so we trade our underlying ring for Z, and all our rules will make sense as well.
And consider new integrals: Behavior of these integrals is identical to discussed in subsection 2.1.
We can consider Lefschetz thimbles in this setup, in real coordinates it is given by the following equation, we call "complex" instantons I C : The space of instanton solutions I R is a subspace of complex instanton solutions I C specified to ζ = −1, v I = 0. To filter out real instantons from generically complex ones we notice that in the case ζ = −1 equation (2.47) admits a complex conjugation mapping a solution to a new solution. Therefore the complex conjugation induces a Z 2 -action on I C , and truly real instantons are the only fixed points of this action. Hence we use the proposed spectral analysis technique to construct the space I C and define I R as its conjugation-invariant subspace. Suppose we consider a family of models with height functions h(u I |t a ), by analogy we construct a family of complex models with superpotentials H(Z I |z a ) depending now on generically complex parameters z a covering some parameter space P. We are interested in a study of instantons in some specific real point z (0) of the parameter space. Let us choose some holomorphic map C → P mapping {0} to z (0) and R s ⊂ C to a subspace of P. Then we can construct a spectral cover for this map using H(Z I |z a ) as a superpotential. Having done so, we consider a small path ℘ 0 going from −0i to +0i. As we have discussed in the previous subsection the space of solutions to (2.47) for ζ = −1 is counted by detours, we conclude: where we used η-grading to stress only a subset of single detours. The η-grading defines how many solitons stacked together on an interface (that will become instantons in the supersymmetric quantum mechanics) contribute to a detour, each soliton position after lifting up ζ-and complexification deformations will become an instanton modulus. The number of instanton fermion zero modes defines a homological degree of operator Q, by a supersymmetry transform these modes are in one-to-one correspondence with instanton moduli. Therefore we cut out just one-instanton sector by considering paths of η-grading 1 for Q to be of homological degree 1. As we have discussed the space of "complex" instantons admits an action of complex conjugation, under this action the spectral cover is conjugated as well (p, x) → (p * , x * ). Some of the detours are fixed points of this action we denote them D R , therefore we conclude: 8 Figure 5. Schematic example of a spectral network for instanton calculus. Here we have not depicted all the WKB lines, only those that flow to point 0 are shown, they are terminated at 0. We expect that WKB lines starting from branching points 1, 3, 4, 8 do not contribute as they are not symmetric with respect to reflection. WKB lines emanated from 2 and 6 are obviously symmetric with respect to reflection therefore they may contribute. Primary WKB lines emanated from 5 and 7 are not flowing to 0, however they may create a secondary line in intersection that will flow to 0, and together they form a WKB subnetwork that is reflection-invariant and may contribute too. Let us propose an example of such WKB web in figure 5. We have depicted only those parts of the spectral network giving detours. Those WKB lines that give rise to detours fixed under conjugation are marked by red. For a simple example of this calculation see appendix B.1.
A tricky problem we may attempt to solve in this approach is the sign of the instanton contribution to the supercharge Q matrix element (2.42). Naively, one has to calculate either the determinant (actually determinant bundle) of the Dirac operator in the instanton background or parallel transport of the differential form along the instanton path in the target space (see [48] and discussion in [31, appendix F]). In our case the corresponding sign can be easily derived from integral ω. However in our formulation we substitute a free problem by an interface. Due to the interface all the eigenvalues of the Dirac operator are shifted by some small amount. In particular, a zero eigen mode of the Dirac operator is assigned to each solution modulus by the supersymmetry. However, in the interface background a BPS solution is bound to certain binding point x c and has no moduli. Consequently, the zero mode of the Dirac operator gets shifted to either positive or negative bulk of eigenvalues. We can estimate this shift using the conventional perturbation theory [58,59]: the first order correction to the eigen value reads: where we have expanded the dependence of the parameters z a in orders of |x − x c | since beyond the strip of soliton width Λ W the solution is exponentially close to the vacuum one. From this formula it is obvious that if we change dz a /dx to the opposite, i.e. if we cross by ℘ 0 the WKB line in the opposite direction, the correction to the Dirac operator zero eigen value also changes sign. For example for these two paths ℘ + and ℘ − we have the fermion numbers in the presence of the interface differing by 1: To get the contribution of only Det where the zero mode contribution is stripped off rather than Det we subtract contribution of the zero mode, or alternatively, multiply Det by the difference where ξ(i) is the detour on the spectral cover corresponding the given instanton solution intersecting the WKB line in either transverse direction and θ is a formal Grassman variable corresponding to the instanton zero mode. For a simple example of this calculation see appendix B.2. Finally, in this subsection let us discuss another aspect of the spectral analysis of the instantons. When choosing the map z : C → P one sees there is too much freedom in this choice. Apparently there may be "good" and "bad" choices. To discuss them and a possible way out let us consider branching points of would-be spectral cover for some choice of map z.
The roots of the spectral curve are in one-to-one correspondence with vacua V of the theory. Therefore branching points correspond to singularities where some vacua become degenerate.
Consider a space of real parameters P R of a family of height functions h. P R is just a real slice of P when we promote height function h to superpotential H. Let us choose an open chart U ⊂ P R , such that one can define an ordering of vacua V on the whole U . The boundary of closureŪ can contain singular loci where i th and j th vacua collide. Denote these loci σ U (i, j) .
We call map z : C → P "good" if in addition to this map we can choose such a neighbourhood U 0 of 0, and a real segment I R containing 0 such that For a "good" map we have following properties: 1. There is an (ij)-branching point on the spectral curve given by the map z. The branching point is projected to R.
The first statement just follows from the fact that branching points appear when vacua collide. The second statement was proposed in [31, section 12.4]. Indeed in the neighbourhood of a branching point one can approximate the theory by the Airy cubic model (see appendix B.1), there is an instanton between two real vacua, and we assume it is not spoiled when we go far away from the branching point. In terms of WKB webs this situation looks like a contribution from the branching point in the left in figure 5, the WKB line from the branching point goes along the real line.

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We call map z "bad" when for any choice of U 0 z(I R ) ∩ σ U 0 (i, j) = ∅. In this case even if ij-instanton exists we can not connect 0 and the branching point by a simple WKB line, since there is no (ij)-branching point projected to the real line. The situation is more cumbersome, and the instanton WKB line is "glued" from several descendant WKB lines from other vacua degeneration loci like a contribution from 3 branching points on the right in figure 5. We propose an illustrative example of "good" and "bad" choices of z in appendix B.3. Now let us suppose that the "good" choice of the map z can always be made. Then instead of searching for a solution to a gradient flow (2.41) between vacua i and j we can search for a point s ij on the real parameter space P R where these two vacua collide. We make the following Proposition 1. The Q-matrix element between i th and j th vacua is counted by possible homotopy classes of real paths from z(0) to s ij .

Landau-Ginzburg cohomology and WKB web degeneration
A construction of Hilbert spaces of ground states in the Landau-Ginzburg model involves a spectral analysis we have performed on two stages: 1. Critical points of the height functional are counted by combinatorics of binding points -parameter values along a path℘ in the parameter space when Lefschetz thimbles intersect.
2. Instantons are counted by intersecting real Lefschetz thimbles, generated by real gradient flows, on the space Map(R → X) with respect to the height functional h.
To construct the MSW complex we should take the space of solutions to (2.27) and promote it to a complex. To construct this space of solutions we can apply equivalence map ξ (2.36) to a detour element associated to path ℘. The result is a functor: By a ket-vector | here we imply a vector of a Hilbert space of perturbative ground states that corresponds to a critical field configuration ξ −1 ( ) as in (2.40). The second part is much more subtle since one should construct complexification of the space Map(R → X) and define corresponding chiral ring, etc. Instead we use the idea presented in Proposition 1. We consider a family of interfaces given by functions z a (x|σ) with a homotopy parameter σ and search for a map z a (x|σ 0 ) when two critical field configurations, say, ξ −1 ( i ) and ξ −1 ( j ) coincide. However despite homotopic equivalence of ξ −1 ( i ) and ξ −1 ( j ) the very paths i and j are not homotopic equivalent, rather during a homotopy movie a WKB web will undergo a singular transformation through a frame containing a special degenerate kind of a WKB web we call null-web W ζ ( j , i ), so that for the Q-matrix element one has:

Instantons and null-webs
Generically instantons solve the differential equation: In the limit τ → ±∞ the solution should approach either solution of (2.27). A method to solve the instanton equation is proposed in [31]. One should consider so called boosted solitons. Indeed under the boost -a rotation in the Euclidean space-time to angle ϕ -equation (2.56) transforms covariantly with a shift ζ → ζe −iϕ . One considers the solitons bound to the interface as 2d quasi-particles, then they can migrate with the boost velocity so that supersymmetry is preserved. The world-line of such quasi-particle is given by the following equation: where we used the effective central charge definition (2.29). This approach gives a rise to a natural definition of the future and past stable binding points. In the neighborhood of the binding point real and imaginary parts of the central charge have the following behavior: Then asymptotic solution to (2.57) has the following form in the neighbourhood of the binding point: is always positive one has two following possibilities: It is simple to define if the binding point is future or past from the form of the WKB web. Notice that in the intersection point p 0 of path ℘ and ij-WKB line . Moreover equation (2.10) implies So the angle between tangent vectors ∂ t to and to ℘ define the type of the binding point:

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For example, ℘ future past Now let us construct a simple example of a null-web. Suppose there is an instanton connecting future and past binding points: Notice that finiteness of the instanton action implies that the field configuration tends to some vacua at spatial infinities x → ±∞ common for all values of τ . In other words there are no boundary instanton emission vertices at spatial infinities. It is simple to construct corresponding spectral cover and corresponding detours as it is depicted in the left frame of the following diagram: Both detours d 1 and d 2 are of type ij: they both start on the i th sheet and end on the j th sheet. Following our paradigm we put in Proposition 1 there should be an interface map z (0) such that forced soliton solutions ξ −1 (d 1 ) and ξ −1 (d 2 ) coincide, i.e. intersection points of WKB lines with the path ℘ should coincide as in the right frame of diagram (2.63). The path 2 is a closed cycle on Σ we denoted γ. Since according to (2.23): one sees easily that γ λ = 0 (2.65) 8 Let us stress here that diagrammatic notations for null-webs should not be confused with diagrams we used in section 2.3 to count instantons. If we were following literally recipes of section 2.3, we had to use functions za(x) defining interfaces as parameters, thus parameter space P would be an infinite-dimensional space of functions za(x). To avoid this complication we count null-webs appearing as singular transitions between detours parameterizing homotopic critical field configurations.
-20 - Figure 6. Typical form of an instanton in 2d LG model.
For this value of the contour integral we call this asymptotic state of the WKB web null- Let us argue that condition (2.65) is common for all instanton configurations. A common form of an instanton (a curved web in the language of [31]) is a horizontal "caterpillar" (see figure 6). The "body" consists of short curved domain walls and bulk joint vertices we will discuss in the next subsection. Legs are domain walls approaching asymptotically binding points. The collection of vacua at the top (infinite future) and at the bottom (infinite past) are denoted correspondingly as i 1 , . . . , i t and j 1 , . . . , j b . Vacua l and r at the most left and at the most right are common for past and future states. Indeed, the instanton action is proportional [76] to the difference ∆h of the values of the height function for two critical field configurations. The major contribution to this difference from spatial infinities is given by Im ζ −1 ∆W dx. For the instanton contribution to be finite difference ∆W at spatial infinities should be zero, therefore in a generic case corresponding vacua should be common for top and bottom critical field configurations. Consequently paths t and b corresponding to top and bottom critical field configurations start on the sheet corresponding to vacuum l and go to the sheet corresponding to vacuum r, moreover We can form a cycle γ = t • −1 b closed on cover Σ and satisfying (2.65).
Definition 1. Generically, we define a null-web W ζ ( j , i ) for a pair of detour paths i and j as an asymptotic state of the WKB web, such that a part of the web giving contribution to these detours lifts to a finite closed cycle γ on Σ, moreover This definition might seem somewhat paradoxical. It is different form a usual triangulation flip used to discuss cluster transformations in the spectral network literature [32-37, 46, 62]. Flips appear when ij-WKB line starting from a ramification point p 1 hits another ramification point p 2 , at the same parameter setting there is ji-WKB line solution going from p 2 to p 1 . Unlike flips null-webs appear from junctions of pairs of WKB lines of the same type. In the junction point they form a cross-like structure (see an example in -21 -JHEP05(2019)085 figure 10 on page 34). Actually, the cross-like junction corresponds to a "fake" branching point. The fake branching point is a point p 0 where the discriminant of the spectral cover Σ has a double zero, so the sheets of the cover only touch each other without forming a cut. The contour γ is pinched in the fake branching point and can be divided in two closed cycles γ 1 and γ 2 projected to paths connecting p 1 to p 0 and p 0 to p 2 correspondingly: We will consider more illustrative examples of null-webs in what follows and will comment more on this matter.
Null-web W ζ (d j , d i ) corresponds to an instanton connecting two critical values of the height functional corresponding to detours d i and d j , so we propose to count instanton contributions as null-webs, see (2.55).
Actually, the condition of a null-web is a priori stronger than needed for existence of an instanton. In practice, the null-web guarantees the existence of a hovering solution to a "forced" instanton equation: Here σ is a continuous homotopy parameter interpolating between two interfaces corresponding to paths℘ (1) and℘ (2) . As explained in [31, section 10.7] (and was heavily exploited in [39] to argue interface homotopy invariance) counting rigid "forced" σζ-instantons produces a chain map that preserves bi-gradings up to an overall shift and moreover (anti)-commutes with the differentials U Q (1) To establish an isomorphism of cohomologies H * (E (1) , Q ζ ) one must find a chain map U in the opposite direction: that graded commutes with the differentials and moreover satisfies for some maps T i . Apparently, inverted interface homotopy gives U . It is enough to have this map to establish an isomorphism: And the presence of null-web W ζ (d 1 , d 2 ) implies that critical field configurations corresponding to d 1 and d 2 emerge or merge by pairs like in the famous illustration (see, for of the MSW complex invariance on a two-sphere under homotopy. This pair represents a "fake" pair of BPS ground states lifted non-perturbatively. Statement (2.72) implies that we can form a subcomplex containing these two states and cancel it as cohomologous to zero. In what follows we will refer to this argument as a fake pair argument.
Let us complete this subsection by the simplest example of a null-web: just a single branching point. Suppose we have a path ℘ intersecting two of WKB lines emanated from a single branching point as it is depicted in the following diagram (left): Here we compare a path constructed from two consequent detours d 1 and d 2 and an "empty" path corresponding to lift of ℘ to i th sheet. When we shrink the arc of the path ℘, so that path ℘ crosses the ramification point, path γ = d 1 • d −1 2 can be projects to a loop encircling the ramification point twice, obviously, this gives a null-web W ζ (d 1 d 2 , ∅), the corresponding instanton representing merging of an instanton-anti-instanton pair is depicted at the right part of diagram (2.73).

Bulk vertices and wall-crossing
The boosted soliton solutions can scatter during migration through bulk vertices [31]: The bulk vertex β {i 1 ,...,ip} [z a ] is given by the instanton solution at certain point z a of parameter space P and with boundary conditions given at infinity by a fan of vacua {i 1 , . . . , i p }.
In target space X the situation is somewhat dual. Vacua i k from the boundary condition fan are points in the target space, boosted solitons are paths in X connecting vacua and forming a closed curve in X, and the instanton (a map R 2 → X) is a disk stretched on this curve as it is depicted in the right part of diagram (2.74). The instanton solution is differentiable, hence the disk should be a differential contractible manifold.
In [31] rich algebraic A ∞ -and L ∞ -structures hidden in the soliton scattering processes were discovered. In particular, a generating function of bulk vertices satisfies the Maurer-Cartan equation. This generates a set of mutual relations between bulk vertices, -23 -JHEP05(2019)085 however these relations are not defining, so we are not able to fix all the bulk vertices from these constraints.
However an explicit value of the bulk vertex is irrelevant in our consideration since the action of the whole instanton is given by the change of the height function. Nevertheless we are interested if a certain bulk vertex is zero or not. In the case the vertex is zero there is no solution to the instanton equation with prescribed boundary conditions, for example if X has a non-trivial homology H 1 (X, Z) the curve formed by boundary solitons in X may have a non-zero homology class, then a smooth instanton disk is unable to be stretched to this boundary.
We will try to solve the problem of defining necessary bulk vertices from a different perspective: we use consistency conditions with wall-crossing, or, equivalently, homotopy invariance of interfaces. Indeed, the same bulk vertices contribute to the hovering solution of "forced" σζ-instanton equation (2.67) counting chain maps for interface homotopy. A hovering solution including vertex β {i 1 ,...,ip} [z a ] implies that this vertex is non-zero. The interface homotopy is naturally implemented in the WKB web formalism, hence it will be not difficult to implement bulk vertex definition in the null-web formalism.
Let us illustrate this idea in the simplest example when ij and jk solitons scatter into a ik soliton. We construct corresponding diagrams following approaches we mentioned: a contribution of bulk vertices to the "forced" instanton equation, descendant WKB line creation, disk in the target space: The wall-crossing formulas in this formulation explicitly correspond to a statement of invariance of the Euler characteristic of interfaces under homotopy, this statement is replicated by equivalence of detours: However if we restrict ourselves to ik sector then the complexes are one-dimensional and equivalence of Euler characteristics implies an isomorphism, therefore there is a corresponding invertible chain map U represented by a hovering "forced" instanton solution containing bulk vertex β ijk as it is depicted in diagram (2.75(a)). Surely, this reasoning can be generalized to more complicated bulk vertices.
-24 -JHEP05(2019)085 Figure 7. A tangle embedded in a three-manifold M 3 . Transverse slices to the x-plane are a Riemann surface C so the tangle is described by an evolving set of points z a (x) in C. In this paper we will take C to be the complex plane so that M 3 is just C × R = R 3 .
Notice that counting bulk vertices through descendant WKB lines is implemented intrinsically in the formulation of the null-webs. The peculiarity of the null-web in this case is that it includes descendant WKB lines rather than only primary ones.
However the reader should be warned that the proposed reasoning fails in the case when the target space has a non-trivial fundamental group. In this case the boundary of implied instanton disk solution depicted in diagram (2.75(c)) may encircle some defects in the target space, and hence there is no smooth disk instanton solution. And this is exactly a discrepancy between so called Yang-Yang and monopole LG models proposed in [39], we will also mention this situation in what follows. So while applying methods from this section we always imply π 1 (X) = {1}. An accompanying interpretation in terms of wallcrossing formulas is the following: punctures of X give rise to purely "flavor" solitons (see [39, section 7.1]) that spoils the wall-crossing formulas. 3 Landau-Ginzburg su 2 link cohomology

Tangle interfaces in the Landau-Ginzburg model
Let us briefly recall a few points from section 18.4 of [31]. The link L whose link-homology we wish to formulate will be presented as a tangle, that is, as set of distinct points z a in the complex plane continuously evolving with a parameter x. The points are allowed to be created or annihilated in pairs at critical values of x but otherwise cannot collide. 9 See figure 7.
In link-homology the strands of the tangle, and hence the points z a are labeled by irreducible representations R a of some compact simple Lie group G. And indeed the Chern-Simons invariant associated to the Euler character of the link homology will be that for gauge group G with Wilson lines in irreducible representations R a . Actually this 9 In principle one could consider punctures on a general Riemann surface C, and hence discuss links in C × R. However, in this paper we will strictly limit ourselves to the case where C is the complex plane. formulation allows one to calculate invariants of an oriented link. So if the orientation of the strand in the tangle coincides with the evolution direction x orientation we mark this strand by the original representation R a , however if it is opposite the strand should be marked by the conjugate representationR a .
In the Landau-Ginzburg approach to link homology collection {z a , R a } parameterizes a family of massive 1 + 1 dimensional quantum field theories with (2, 2) supersymmetry, T (z a , R a ). The spatial axis of the "worldsheet" on which the quantum field theory is defined is to be identified with the x axis in figure 7, and the time axis is not shown in that figure. Parameters z a ∈ C span superpotential parameter space P of the quantum field theory. In a tangle the z a 's vary as a function of x, and therefore the parameters of the quantum field theory vary as functions of x. This defines what is known as a "Janus wall" or an "interface." As shown in [31], interfaces define a notion of parallel transport of the category of branes over the parameter space of the quantum field theory. Moreover, suitably interpreted, the parallel transport is given by a "flat connection." Therefore we can hope that homotopic deformations of the path of parameters {z a (x)} will lead to chain homotopic complexes. Therefore, this is a natural setting for the formulation of link homology.

Review of LG su 2 link cohomology construction
We follow [31] and consider Landau-Ginzburg model of [29] on the monopole moduli space. The target space of this model is the universal cover of the moduli space of m magnetic monopoles in SU(2) Yang-Mills-Higgs theory on R 3 . The moduli space has the form R 4 × M 0 where M 0 is the simply-connected strongly-centered moduli space. The most natural metric would be the hyperkähler metric, although fortunately we will not need to know any details of this metric.
In order to describe the superpotential we use the identification of the moduli space with a space of rational maps CP 1 → CP 1 of degree m and preserving the point at infinity [7,18,[49][50][51]. Thus the rational map can be taken to be u → P (u)/Q(u) where Q is a monic polynomial of degree m and P has degree m − 1 with nonvanishing leading coefficient. The polynomials P, Q are relatively prime so P never vanishes at the roots of Q. We will denote those roots (which need not be distinct) by w i : The superpotential is Here k a is a charge of a singular monopole located at z a , it is given by the highest weight of su 2 irreducible representation R a . This superpotential is multivalued on the monopole moduli space but single valued on a cyclic cover. This cyclic cover coincides with the simply connected cover of monopole moduli space.

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If monopole centers are widely separated we can define e Y i := P (w i ) then evaluation of the residue in (3.2) gives a new superpotential: Now coordinates (w i , Y i ) on the target space have a nice quasi-classical interpretation: for a single monopole we could write: w = x 2 + ix 3 and Y = µy + iϑ where (y, x 2 , x 3 ) denote the center of mass of a monopole in R + × R 2 and ϑ denotes the electric phase. All the monopoles are placed in a half-space y > 0 and singular monopoles are sitting at the plane y = 0 (a tip of a "cigar" in the M5-brane formulation of [82]). We can go further and integrate over fields Y i , the resulting superpotential -called Yang-Yang superpotential -reads: From this point of view W YY can be considered as a low energy effective superpotential for the monopole Landau-Ginzburg model, from the point of view of manipulations with the chiral ring we have assigned to some of the operators their classical expectation values. This procedure does not change asymptotic behavior of the connection (2.7), and therefore it does not affect the spectral curve. However the resulting model is different in a crucial way as it was demonstrated in [39]. As the result of integration the target space acquires singularities and a non-trivial fundamental group, this breaks flatness of the parallel transport and invariance of the Hilbert spaces of ground states under link regular homotopic transforms. In particular, the wall-crossing arguments for constructing instanton bulk amplitudes fail due to extra flavour wall-crossing that is not captured by the usual wall-crossing formula (see [39]).
Notice that the Yang-Yang superpotential (3.4) substituted in the integral (2.3) gives a description of conformal blocks in the free field fomalism [40]. And it is well-known that monodromies of the conformal blocks are braid invariants and after braid closure become link invariants. The asymptotic monodromy of the integral is given by the Euler characteristic of the corresponding MSW complex, hence the Euler characteristic of the MSW complex is a link invariant by construction, it is not complicated to check that it coincides with the link Jones polynomial.
In the remaining part of this section we are going to apply methods of spectral analysis from the previous section, for this purpose the superpotential W Y Y is suitable, however as we mentioned we imply that the target space has a trivial fundamental group, there are no wall-crossings involving purely flavour solitons. Thus secretly we work with W monopole . Therefore it is enough to study the vacua for a single puncture. For a single puncture we have a single vacuum (see appendix A)

Spectral curve and classification of vacua
where v α is a vector of weight α. Generally we can identify all the basis vectors of a representation of the highest weight k with vacua for all admissible values of m = 0, . . . , k.
We will consider the simplest case of the fundamental representations, in the su 2 case representations are isomorphic to complex conjugate ones, then it is enough to consider just the case of k a = 1. There are just two possible solutions for a single puncture -V(z; 1; 0) and V(z; 1; 1) -we denote as (−) and (+) spin projections correspondingly.
The next basic example is two punctures, correspondingly we have: The spectral curve in this case for two punctures z a and z b can be easily constructed (see [39, appendix A]). However in a more generic situation this construction is technically involved. The major difficulty on this route is to find a suitably "nice" basis in the chiral ring. Such a basis was found in [66] (see also [1,2,26,65,68,71,86]) in a more generic case -it is called a stable envelope basis -of "quantized" or Jackson integrals and it does not seem to have a single line formulation in our framework. However we get used to the quantum q-Langlands correspondence This theorem is important for us since conformal blocks of W q,t (g) have a nice representation in terms of Jackson type integrals generalizing (2.3), on the other hand conformal blocks of U L g satisfy q-Knizhnik-Zamolodchikov difference equations. The only thing we should do now is to adopt this result to our non-quantized case, in this case we get a Theorem 2. There exists a basis in the chiral ring such that connection (2.7) has the following form: Only a mutual positioning of the punctures matters, so we take z a = z, z b = −z. Then the space of parameters P ∼ = C and we choose a trivial map z(x) = x, then the spectral curve reads: The two roots coincide with two vacua (+, −) and (−, +) and we construct easily the WKB web (see figure 8).

Braiding, fusion/defusion interfaces
Composability property of interfaces (2.38) allows one not to construct a new interface for a new link each time, instead we can decompose any interface into a product of elementary interfaces similarly to Kirillov-Reshetikhin-Turaev (see e.g. [57,74]) U q (su 2 ) formulation of link invariants. Such basic interfaces are braiding interfaces analogous to generators of the braid group -we call them R and R −1 -interfaces by analogy to R-matricesand caps/cups, or fusion/defusion interfaces joining/creating a pair of strands into/from a closure. The latter are analogs of q-Clebsh-Gordan coefficients. Without loss of generality we can choose parameters to be real c > 0, ζ < 0. Then it is natural to associate a collection of constant braids in the diagram to a collection of constant trajectories z a lying on the imaginary axis:

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Then two braiding elements are given by the following plate diagrams: To assign corresponding interfaces one should choose complex paths z a : C → P such that z a (R) will give desired strand trajectories. For example, for two strands we could choose z 1 = z, z 2 = −z, and a complexifiable trajectory function for R ±1 reads: Indeed, as x flows from −∞ to +∞ in the complex plain points z 1,2 will make either a clockwise or a counterclockwise twist correspondingly. However, as we have explained in section 2.4.1 the soliton content depends only on a homotopy class of path ℘, therefore we can choose a simpler map z(x) = x we used to construct a spectral cover and choose corresponding paths ℘ in the complexified x-plane. Choices corresponding to clockwise and counterclockwise twists are depicted in figure 8. Calculating detours and taking into account the hovering solutions in vacua (−, −) and (+, +) we derive the following expressions for the interfaces (to compare to [39, eq. (4.5), (4.7)] one should switch (q, t)-gradings to opposite ones):

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In [39] it was argued that the fusion/defusion interfaces can be thought of as certain half-twist also depicted in figure 8. The resulting expressions are: Here we used grading q P t F for all the solutions: By horizontal lines we have depicted soliton solutions bound to the interface, they are labelled by indices of corresponding WKB lines. We splitted these indices into ones without a prime and ones with a prime. The reason for that is that soliton paths in the target space X have different topology for prime and non-prime binding points. We will not comment here on this point, however this fact can be easily seen from comparing P degrees of solutions, also one can think of a path in P corresponding to R −1 -twist as a path corresponding to R-twist flowing in the opposite direction. If we reverse the path corresponding to R we see that it first intersects the primed WKB line then non-primed one.

Null-web examples
We will not re-cite all the arguments of link invariance under the Reidemeister moves listed in [39, section 6], let us consider here just the Reidemeister move II and show how the corresponding complex contributions cancel due to presence of null-webs.
The Reidemeister move II implies that two following links are equivalent: However expanding the complex in the left hand side one derives the following contributions: Terms in brackets cancel due to instantons and we present corresponding null-webs, it is simple to construct them since as one moves apart the strands the intersection points on the link diagram move towards each other, and soliton binding points move with them. So we can choose the following path℘ family: In a diagram drawn in figure 9 we present corresponding link diagrams and WKB webs. We have marked null-webs corresponding to instantons cancelling contributions of Pdegrees −1 and +1 as W (−1) and W (+1) and by a blue marker correspondingly. At this point let us stress again that a null-web does not represent a cluster mutation mapping an ideal triangulation to an ideal triangulation, and the situation in question is rather illustrative. In this case the spectral cover is two-fold, usually one assigns to a WKB web an ideal triangulation of the base curve C according to three rules [32][33][34][35][36]: WKB lines play the role of "medians" of triangles, branching points correspond to "centers" of faces of -32 -

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triangles, punctures correspond to vertices of triangles. And triangulation is ideal if all the edges of triangulation have triangle faces on both sides. We have depicted a what-wouldit-be trangulation according to this rules at r = 0 by dashed red lines. Obviously, in the middle we get some rhombus rather than an ideal triangulation.
A generic strategy to construct a null-web is the following. Solitons are usually bound to certain elements like intersections, or caps/cups. We can move them homotopically in the link diagram so solitons (intersection points of WKB webs with path ℘) move as well. Null-webs appear near configurations corresponding to shrinking diagram resolutions as in the previous example. However, this strategy may fail when applied to multiple twists, like in the following diagram: If one naively shrinks a double twist (moving to the left in the diagram) to a point the WKB web becomes too singular. To resolve this singularity we use Reidemeister move I (move to the right in the diagram), then in this spider-like diagram the intersection can be shrinked painlessly. For example, let us show that indeed 12 and 12 solitons form an soliton-anti-soliton pair, therefore they can be canceled. This is hardly seen from the simple double twist diagrams. We should squeeze branching points so we denote corresponding null-web as merge of two branching points: By this null-web we imply a resolution by a spider like move: Let us put here an explicit example of a null-web governing an instanton canceling two following terms required for validity of Reidemeister III move: We have chosen a configuration with a single smooth monopole since it is simpler to analyze the spectral curve in this case. In particular, the locus of branching points is given by the discriminant of vacuum equation ∂ φ I W = 0 that is a cubic polynomial in this case. The corresponding null-web is depicted in figure 10.

Sketchy review of Khovanov homology construction
As it was indicated in the introduction our final aim is to compare cohomological theory emerging in the Landau-Ginzburg model description of tangles to Khovanov homology. Let us put here a brief review of the Khovanov homology construction following [8,[15][16][17].
Let us denote by E(L) a complex corresponding to a link L as a vector space. One constructs the complex following simple rules. One puts a resolution in each vertex according -34 -

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to the rule: The complex is bi-graded by P-degree and F-degree (homological degree), we denote their shifts by q P t F . Then the complex corresponding to link L decomposes eventually into a direct sum of complexes corresponding to disjoint sets of cycles with appropriate degree shifts. One maps them to a bi-graded linear spaces according to a rule: Where V is a two-dimensional space spanned by vectors v + and v − with P-degrees +1 and −1 correspondingly. Then one considers a set of differentials d 2 χ = 0 having homological degree 1 and acting in each intersection χ by either: • Joining cycles (multiplication): • Cutting cycles (co-multiplication): The total differential is defined as The multiplication and co-multiplication make from complex elements a Frobenious algebra mimicked by a TQFT, corresponding string diagrams are depicted below equations (3.24) and (3.25). Homotopic equivalence of string diagrams produces corresponding commutativity diagrams for multiplication and co-multiplication. The differential is local in the By definition, the Khovanov homology satisfies a skein exact triangle categorifying the skein relations for the Jones polynomials:

"Isotypical" interface
The structure like in (3.22) is inherited naturally from the isotypical decomposition. One can re-write the R-matrix acting in ⊗ as where P ∅ is a projector to the scalar in the isotypical decomposition. On the other hand the structure like in (3.13b) appears in the natural basis in the tensor product, the Euler characteristic of that complex is just ordinary representation of the Drinfeld universal R-matrix [19]: where σ : a ⊗ b → b ⊗ a is a permutation in the tensor square. The isotypical decomposition of tensor products of irreducible representations reads: where Q are again irreducible representations and D Q are invariant modules, numbers dim D Q are called multiplicities. In this basis the R-matrix has a very simple form since it acts by intertwiners: R =  transition between canonical and isotypical bases in the tensor power of representations. To perform this transition on the level of complexes one should perform an action of a specific interface we call an isotypical interface I. In what follows we will consider a conjugated R-interface: where is a consequent interface ζ-gluing defined in [31], however we will not need the explicit formulation of this operation, instead we will construct direclty the conjugated interfaceR and compare it to Khovanov's construction.
However before following this route one should make a minor change of variables. So far for an unknot we have: LGCoh Actually, these homologies are isomorphic to each other; the only thing we should do is to shift F-degree to F + P, one can achieve the same result if applies a gauge transformation to the form ω → ω + dW , these transforms do not change the complex since the differential (supercharge Q) acts only between subspaces of the same P-degree and F-degrees differing by one. So we change variables (q, t) → (qt, t) and call this construction LGCoh. By construction LGCoh and LGCoh are isomorphic. A construction for an isotypical interface is naturally implemented in the 2d CFT limit of the LG model: integrals (2.3) give a free field representiation of conformal blocks. In the CFT there is a natural operation of vertex operator fusion mimicking isotypical decomposition (3.32). Fusion implies that we break initial assumption |c∆z| 1 when consider vacuum classification (3.5).
One can start following the change of the model behavior from the hovering solution in the case of (+, +) vacua (see figure 11). In this case the only solution is the hovering one.
In figure 11 the red trajectories correspond to hovering solutions for w i while the black trajectories correspond to punctures. It is clear that if one stays above the critical value -37 -

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|c∆z| ∼ 1 the hovering trajectories twist as in (3.13a), and if one moves punctures closer the solution behaves as in identity interface in (3.22).
In the sector for +− and −+ vacua we should deform the path ℘ in such a way that it comes to the puncture closer (notice that during this deformation one slides the path through branching points ∆z = ±ic −1 , so again a fusion transition of the vacua occurs).
Consider the following diagram: We have just redrawn the diagram depicted in figure 8: now the cut is shown explicitly, 12-WKB lines are marked by the red color, 21-WKB lines are marked by the blue one. We consider three homotopic paths ℘ k . Let us schematically write all the detours for those paths. We denote by d (ab) i a detour due to intersection with the corresponding WKB line starting on the a th sheet and ending on the b th sheet. A path on Σ without detours we will denote as (kk) , and the sheet permutation due to going through the cut we will denote as σ (kl) .
Therefore we see that all the three paths give equivalent interfaces: Neither of paths (3.37) gives an interface that coincides with the desired one, so we combine some contributions from paths ℘ 2 and ℘ 3 . We assume that if one starts with the -38 -

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(+, −) vacuum (sheet 1) then one takes detours form ℘ 3 , otherwise from ℘ 2 , and we take one of terms in the brackets: (12) +σ (12) + σ (21) + d (21) 3 σ (12) d For these manipulations to be valid we should switch to an equivalence class of complexes, so we say that this interface corresponds to an abstract path ℘ 0 about what we know only it is homologous to ℘ 1 , ℘ 2 , ℘ 3 . We should notice that here again there are four contributions and two terms in brackets that can be cancelled by the fake pair argument, hence we have not changed cohomology: The definition of the Q-charge action does not change, however the complex does change, and it may happen that for some path choice ℘ 0 the supercharge act locally on the link digram. All the terms contain permutation σ (ij) due to intersection of the cut, this permutation is important since we would like to get an untwisted identity interface like in (3.22), and this permutation exactly undoes the twist for the trajectory of w-field. Taking into account all the contributions, rearranging terms, making a substitution (q, t) → (qt, t) and suppressing an overall q, t-monomial factor we arrive to the following interfaces:

Comparison of Landau-Ginzburg cohomology and Khovanov homology
Now we would like to compare complexes following from (3.22) and (3.41a). We will argue that (3.41a) is equivalent to (3.22) in two steps: 1. We show thatẼ 2. We show that the differential Q can be represented as where χ are intersections in the link diagram, moreover Q χ acts on intersection χ by gluing or cutting cycles in the resolution as in (3.24) and (3.25)

Checking item 1
Obviously, the first four terms in brackets in (3.41a) form an identity interface, so the question is why the next four term in the brackets form a pair of a cup and a cap. Let us for brevity denote these terms as Then one can use a "hump" move: If one considers these contributions closer one observes these are exactly four contributions of an identity interface for (+, +), (−, −), (−, +) and (+, −) vacua correspondingly. One can modify the set of detours in each case to a simple "empty" detour on surface Σ. Let us demonstrate this satement in the case of (+, +) vacuum. We modify the curve and corresponding detours as follows:

Checking item 2
To check the second item in our list we will just construct the action of the local differentials Q χ and compare it with rules (3.24) and (3.25).
The first step one should take is to assign vectors v + and v − to two types of cycles. This can be easily done by consideration of the unknot, it is given exactly by two contributions with P-degrees ±1, using (3.41a) one has Internal relations between link diagrams preserving cohomology: a "hump" move, and a "tri-dent" move: allow one to check (3.24) and (3.25) only for a twist (an inverse twist check follows) and in the simplest setting when cycles are represented by circles. Now we just present a form of the maps in terms of soliton link diagrams and depict null-webs responsible for these maps: • Multiplication: there is no term on the other side of same degree therefore Q = 0 in this situation.
• Co-multiplication: So far we have constructed a system of differentials Q χ acting in diagram intersections. ComplexẼ can be seen as a hypercube of resolutions in the complete analogy to the Khovanov complex: vertices are represented by different resolutions of link diagram intersections χ in (3.41a), edges are Q χ . The action of the supercharge form a Frobenious algebra given by relations (3.24) and (3.25) and satisfying (3.27), therefore for edges supercharges Q χ anti-commute. However to claim (3.27) one should make one more step and argue that there are no differentials other than Q χ .
Suppose there are other types of differentials. Consider a cube of resolutions, for simplicity, let us consider a visualisable 3d cube: The vertices of the cube are marked according to the resolution choice. There are three types of differentials each shifting one of the resolutions: These differentials form edges of the cube. Suppose there is some new type of differential, it gives a new mapQ : Ψ 110 → Ψ 001 marked by the red arrow in the diagram. One can represent it as more elementary moves consequently shifting all the resolutionsQ ∼ Q 2 Q 1 Q −1 3 . This combination can not be considered as a combination of instantons since -43 -

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one of them is an anti-instanton Q −1 3 , however there may be present a singe modulus BPS instanton somewhere on the boundary of the moduli space of this configuration. ProductQ ∼ Q 2 Q 1 Q −1 3 is depicted by a blue path in the diagram. There is another path Q 1 Q 2 Q −1 3 connecting Ψ 110 and Ψ 001 marked by the orange color. Then mapQ should get contributions from bothQ In a generic situation all such terms contain numbers of Q's and Q −1 's of opposite parity, therefore they are summed up to a zero. Alternatively, we can consider a matrix element of Q 2 that should be zero, it is given by a sum over all possible paths:

Discussion
So far we have argued that the su 2 Landau-Giunzburg cohomology is equivalent to the Khovanov homology. This statement was not obvious in the initial formulation (3.13a)-(3.13d) since the resulting complexes and differentials acting on them are quite different. However, the Landau-Ginzburg theory proposes not just a single complex rather a family of complexes. The content of bound BPS solitons on an interface given by path℘ in parameter space P depends on a choice of "chambers" (see figure 1). Transformation of the BPS content across the walls separating chambers is widely known as wall-crossing phenomenon. So we just propose a choice of a path defining the supersymmetric interface crossing a sequence of chambers in such a way that the Landau-Ginzburg complex and Khovanov complex become isomorphic rather than just only quasi-isomorphic. A physical meaning of such path choice is to mimic isotypical decomposition of interfaces since the R-interface is supposed to be a categorification of R-matrix that becomes diagonal in the isotypical basis. This choice may seem artificial since it is not presented by a certain path℘ rather by different contributions from different paths. This can be done if one considers an equivalence class of complexes with respect to the wall-crossing morphisms. Despite this artificial flavor the supercharge Q acts locally in link diagram intersections by gluing or cutting cycles analogously to the differential in the Khovanov homology. Consequently we conclude that the su 2 Landau-Ginzburg cohomology also satisfies the skein exact triangle sequence: LGCoh → . . . The superpotential for what one could call a naive monopole model analog, or quasiclassical monopole model, when monopole centers are well-separated, see (3.3), is given in [10]. Here we use a low energy effective description with a su n Yang-Yang superpotential that in terms of integrals (2.3) gives a free field formulation for SU(n) WZW-model with N punctures correspondingly [40]: Here k i,a is a vector of hieghest weight of representation R a inserted in puncture z a .
Let us stress again a peculiarity of the transition from the monopole model to the Yang-Yang model we mentioned in the beginning of section 3. During this transition new singularities are created on the target space: this makes wall-crossing formulas in their initial formulation inapplicable due to purely flavour solitons and eventually breaks the link invariance. Therefore despite we work with the Yang-Yang superpotential (4.1) in actual calculations we imply that the actual model has a target space given by the universal cover of the monopole moduli space with a superpotential without singularities. And it is enough to study only vacua classification of a single puncture model. It is not surprising that we have the following statement:

Classification of vacua
Where v λ is a subspace of weight λ and genrically, where V λ is irreducible su n -representation module of the highest weight λ. This statement follows naturally from the relation between chiral operator basis and stable basis (see [2,66]). Again we will restrict ourselves to links colored by the fundamental representation, however we will have to color strands by both fundamental and anti-fundamental¯ representations. Both representations are n dimensional of heighest weights k = (1, 0, 0, . . .) We will denote them appearing in this order as i andī correspondingly. It is simple to define what these solutions are, especially if one assumes some ordering, say all c i are real and satisfy c 1 c 2 . . . c n−1 : And in a way analogous to su 2 case one arrives to the following Here η is the Killing form on the algebra su n .

Braiding interfaces
We will consider the following types of braiding interfaces (the interface evolution axis x flows in the upward direction in all diagrams, see figure 7): The corresponding strand is marked by the fundamental representation if the arrow on the strand flows in the same direction as the interface "time" x, and by the anti-fundamental one otherwise. Obviously, there are six more possible orientations, however we will not discuss them here since they are related to mentioned two by "tri-dent-like" moves. It is simple to notice that if both strands are marked by the fundamental representation there is a very simple admissible vacua classification. Admissible filling vectors and vacua are:

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Therefore the spectral curve factorizes to polynomials of order two and one according to two possible cases described above: it is not really crucial what are numbers t i , q ij and s ij , a relevant information about this curve is discriminants of polynomials for i ⊗ j pairs: they read D ij = x −2 +c 2 ij , where effective parameterc ij = c ( m i − m j ). Therefore the behavior of i ⊗ j vacuum is analogous to the behavior of +− vacuum in su 2 case discussed in section 3, and similarly forī ⊗j vacua. Therefore without re-derivation we just adopt the results of section 3 and construct following expressions for interfaces: Here solitons are marked by detours analogous to ones depicted in figure 8. Sheets 1 and 2 correspond to vacua j ⊗ i and i ⊗ j.

Fusion/defusion interfaces
A natural place to search for construction of fusion/defusion interfaces is again isotypical decomposition. The product of a representation and its conjugate always contain a trivial representation: The trivial representation in this setting is treated as a wave function of a constant x slice without any punctures (see figure 7). And the Clebsh-Gordan coefficients between R,R and ∅ give expressions for the Euler characteristics of the fusion/defusion interfaces. As we have seen in the previous section the isotypical decomposition can be invoked in the construction of "half"-R-interfaces, therefore it is natural to guess the structure of fusion/defusion interfaces by considering R-interfaces for ⊗¯ and¯ ⊗ vacua. We are interested in the vacuum set (n − 1, n) (n,1) since it has a zero weight k + k¯ − α i ∈∆ + m i α i = 0 as an empty space should have. However this vacuum set does not split and the resulting spectral curve has a rather complicated structure. For example, for su 3 , one has: We depict a generic structure of su n curve for this vacuum in figure 12. We have denoted vacua accordingly j = (j ⊗j) andj = (j ⊗ j) at x → +i∞. We construct fusion/defusion interfaces analogously to [39, section 4.3] as half-twists. However, it is simpler to define different interfaces in different scale orderings: c 1 c 2 . . . c n−1 , or c 1 c 2 . . . c n−1 . So we use both implying that one can change the ordering homotopically, or assume that parameters c i are slightly x-dependent.
Or, diagramatically, we have: The thick horizontal line in all these diagrams is understood as a corresponding D-brane boundary condition. We denoted multiple solitons by a dashed horizontal line, each such soliton represents a migration of a single w i field. This is an incorrect interpretation since in counterclockwise cap and cup interfaces all the field w i migrate simultaneously, they appear from intersections with descendant WKB lines (j, n) and (j,n). However for simplicity we depict and assume that those solitons are a combination of consequent soliton jumps, like in clockwise cup/cap interfaces. This simultaneous/consequent representation switches to an opposite for counterclockwise/clocwise orientation if one chooses the opposite sign of ζ for example.

Link invariant
The remaining R-interfaces can be constructed by suitable coupling to the fusion/defusion interfaces through tri-dent-like moves: = Having all the R-interfaces and fusion/defusion interfaces one can define corresponding complex by simply gluing all the elementary interfaces together. The differential is given by the Q-action (2.55). The resulting su n Landau-Ginzburg cohomology for link L: n LGCoh(L) := H * (E(L), Q) (4.14) is expected to be an invariant of link L. To check this one should check invariance of this construction under three Reidemeister moves and two extra conditions we call "Reidemeister 0" moves ensuring invariance for different interface evolution x-axis direction choices (see figure 7). "Reidemeister 0" moves include hump deletion/creation move and trident-like move depicted in diagrams (3.44) and (3.49) correspondingly. Invariance under all these moves they can be easily checked along the lines of [39, section 6]. Let us remind that discrepancy between Yang-Yang and monopole superpotentials becomes essential in this situation. Similarly, we can argue invariance under Reidemeister II and III using similarity between a pair of fundamental representations in su n and su 2 cases. Reidemeister moves II and III work there as they work in the Khovanov construction, therefore they work here as well.
We will not go into detailed check of all the moves, let us restrict ourselves just to Reidemeister I move as an example.

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Reidemeister I move implies an isomorphism of complexes of links different by a curl up to an overall shift of P-and F-degrees due to the framing anomaly: = q # t # Let us consider a complex appearing in the l.h.s.: Terms in brackets cancel due to corresponding null-webs we can depict schematically as: And remaining terms in (4.15) represent exactly one strand identity interface. This can be easily seen in the explicit detour construction or by an implant argument like in [39]. Actual calculation of link invariants in this setup is still rather involved. We consider an example of such calculation for the Hopf link in su 3 in appendix C. As one sees the resulting cohmology is isomorphic to Khovanov-Rozansky homology in this example [41] and Poincaré polynomials are related by a simple change of variables:

Brief review of Khovanov-Rozansky homology
Here we follow mostly recent review [75]. Generically, R-matrix when both representations are fundamental has a simple decomposition (up to an overall scaling): where P is a projector to the first antisymmetric representation. This projector becomes a projector to a trivial representation in the case of su 2 and is non-trivial for the generic case of su n . So in the resolution of an intersection a new type of diagrams appears. It contains a tri-valent vertices for two incoming or outgoing edges and special edge corresponding to the anti-symmetric representation. So one has the following complex decomposition: Each resolved diagram forms a vertex of the resolution hypercube and it is represented by a tri-valent graph. Khovanov-Rozansky homology theory associates to each graph a q-graded vector space [55]. Technically this space is spanned by elements of a polynomial ring modulo certain ideals so that the elements of the diagram correspond to coloring of the resulting diagram by vectors of corresponding representations. So, for example, one associates variable x i to each oriented edge of the resolved diagram with an ideal x n+1 i = 0 to ensure that the fundamental rep is n-dimensional.
The differential acts by local morphisms d = all χ d χ in intersections χ mapping between two vector spaces corresponding to two resolutions. However, a simple explicit construction of this differential like in the SU(2) case is still missing, one should use a rather intricate matrix factorization theory instead. Similarly to su 2 case one would like to construct some analog of TQFT in terms of invariance of thin film embeddings. In this case one uses two types of films, for example see figure 13 for a film corresponding to a differential morphism. In the literature compositions of these thin films are referred to as (pre-)foams and studies of relations between morphisms are referred to as foam calculus [14,54,60,64]. In particular, one uses foam calculus to show local differential anti-commutativity  In this case we will not argue the whole equivalence of homologies due to complexity of Khovanov-Rozansky homology formulation. Similarly rules for the supercharge Q in the generic su n case are rather involved. In particular, there will be non-trivial instantons changing sheet pairs in decomposition (4.8). So we will only emphasize a similarity between Landau-Ginzburg cohomology and Khovanov-Rozansky homology lying at the top. It follows from the isotypical interface construction. Using the relation between spectral covers in vacua ⊗ in su 2 and su n (see section 3) it is not complicated to construct analogous isotypical interface in the su n case, however in the isotypical decomposition instead of trivial representation appears the first antisymmetric one (that is trivial in the su 2 case). So after shifting the fermion degree F → F + P, or, equivalently, changing variables q → qt one gets: and the corresponding Euler characteristic of this interface is projector P . Here solitons in the interface correspond to detours depicted in diagram (3.36).
For fusion/defusion interfaces we have: Apparently, the cohomology of the unknot is properly normalized: The next step in this construction is to provide operators Q χ acting in each intersection resolution χ locally. An important property of locality is that Q χ and Q χ anti-commute for different intersections χ and χ . In this case we are able to say that

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And a tautological consequence of this construction (see appendix D) is an exact triangle for LG cohomology: LGCoh n LGCoh n LGCoh t (5.12) However let us avoid constructing supercharge action explicitly, instead we propose implicit arguments for local supercharges' anti-commutativity. The fact that local operators Q χ exist is rather obvious. There is always a map between the last element of (5.7) and identity interface corresponding to contraction of solitons d 3 and d 5 . Surely, Q χ contains much more non-trivial elements. They appear due to collision of solitons bound to the intersection and result into emission of different soliton showers that spread across the link interacting with other solitons bound to other intersections and fusion/defusion interfaces.
Let us argue that all the local supercharges Q χ anti-commute. Consider two simple neighboring intersections and apply Reidemeister II move: = = Two new intersections appear, there we apply expansion of the R-interfaces and cancel extra contributions by the fake pair argument. The result is the same link, however the R-interfaces and corresponding local supercharge actions are permuted. This implies that there for any local pair of actions Q 1 and Q 2 there is another pairQ 1 andQ 2 applied in the opposite order so that Q 2 Q 1 = −Q 1Q2 . Other types of two neighbor intersections can be dealt with by auxiliary isotopy moves, then one uses the exchange argument proposed above: Apparently, one can extend these arguments to arbitrary pair of intersections, so all the local supercharges anti-commute.  Now function H can be considered as a superpotential. The chiral ring is spanned by 1, and Z with the following ring relations: The action of the derivative ∂ z acts as a multiplication by Z in the chiral ring. The resulting connection coincides with the Airy connection: Its flat sections are spanned by Airy functions. The spectral curve is very simple: The WKB web W 1 for ζ = 1 have the form depicted in figure 14. Now we construct ℘ 0 around the point s and see that for s ≥ 0 there is an instanton flowing from vacuum −s 1 2 to vacuum s 1 2 , and there is no instanton otherwise.

B.2 Airy 2 model
As an illustrative example of Q-matrix model sign calculation we consider Airy 2 model, just two non-interacting Airy models: The complex in this case is just a tensor product of complexes:

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And the supercharge Q = Q 1 + Q 2 . The condition Q 2 = 0 implies that supercharges Q 1 and Q 2 anti-commute, in terms of matrix elements this statement reads: The corresponding spectral curve is highly degenerate, so we resolve it a little bit: Here we used vacua marking as in subscripts in diagram (B.8). If one takes off the resolution of the spectral curve the encircled branching points collide. Each matrix element corresponds to a detour along a WKB line: If we choose z 1 = a 2 , z 2 = −b 2 for a, b being real the system has four vacua {a, −a, ib, −ib}.
Only two first vacua are real, and there is an instanton connecting them just like in the Airy model example.
It is simple to construct this instanton in terms of WKB webs. For this purpose we make a choice ("good" one) of a map z 1 (x) = x, z 2 (x) = −b 2 . Obviously, the contributing branching point is located at 0, when two first vacua collide. And one gets a detour due to the corresponding WKB line: Re x ℘ a 2 0 (B.14) -58 -

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Here we have splitted projections of the WKB line and marked them with the corresponding color code.
However one can choose a different map: z 1 (x) = a 2 , z 2 (x) = x. This is a "bad" choice of a map since there is no value of parameter x, even complex one, when two first vacua collide, instead there are two values: x = 0 when two last vacua collide, and x = a 2 when the first and last pair of vacua collide. The corresponding instanton is constructed as a descendant combination of WKB lines from these two sources: Generically, calculation of link cohomologies becomes quite involved for more complicated links and higher n. In this section as the first non-trivial but still simple example we construct explicitly cohomology 3 LGCoh(Hopf) for the Hopf link and compare it to the analogous Khovanov-Rozansky homology.
For the link complex we have:

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Supercharge Q does not change P-degree, therefore components of this complex of definite P-degree are honest subcomplexes: Subcomplexes of P-degrees 0, 6, 8, 10 are rather simple, supercharges act there by 0. However complexes of P-degrees 2 and 4 are non-trivial. Let us consider them consequently: first we consider E 2 . We label all the generators of the complex by Ψ i , i = 1, . . . , 5 in the order as they appear in expansion (C.1), then we have: We will draw all the null-webs as in a matrix form as they saturate corresponding matrix elements: Here we denoted corresponding solitons as in expansion (C.1).
The second differential is simply contraction of soliton-anti-soliton pairs: And we have put −1 sign to one of the elements by analogy with the Airy 2 model discussed in appendix B.2, so that Q 2 Q 1 = 0. I this case we derive the following cohomology:

D On exact skein triangle tautology
The statement that the Khovanov (Khovanov-Rozansky) homological construction satisfies the skein exact triangle relation is somewhat tautological since necessary elements are just built in the construction. However this property is not so obvious for other link homology constructions. So let us review what elements of the construction are crucial for the skein exact triangle. We exploit the following Suppose that the composite chain-map f i+1 f i is chain-homotopic to 0, i.e. there are