On genus expansion of superpolynomials

# On genus expansion of superpolynomials

Andrei Mironov111mironov@itep.ru; mironov@lpi.ru, Alexei Morozov, Alexei Sleptsov  and Andrey Smirnov morozov@itep.rusleptsov@itep.ruasmirnov@math.columbia.edu
###### Abstract

Recently it was shown that the (Ooguri-Vafa) generating function of HOMFLY polynomials is the Hurwitz partition function, i.e. that the dependence of the HOMFLY polynomials on representation is naturally captured by symmetric group characters (cut-and-join eigenvalues). The genus expansion and expansion through Vassiliev invariants explicitly demonstrate this phenomenon. In the present letter we claim that the superpolynomials are not functions of such a type: symmetric group characters do not provide an adequate linear basis for their expansions. Deformation to superpolynomials is, however, straightforward in the multiplicative basis: the Casimir operators are -deformed to Hamiltonians of the Calogero-Moser-Sutherland system. Applying this trick to the genus and Vassiliev expansions, we observe that the deformation is fully straightforward only for the thin knots. Beyond the family of thin knots additional algebraically independent terms appear in the Vassiliev and genus expansions. This can suggest that the superpolynomials do in fact contain more information about knots than the colored HOMFLY and Kauffman polynomials. However, even for the thin knots the beta-deformation is non-innocent: already in the simplest examples it seems inconsistent with the postivity of colored superpolynomials in non-(anti)symmetric representations, which also happens in I.Cherednik’s (DAHA-based) approach to the torus knots.

FIAN/TD-14/13

ITEP/TH-41/13

Lebedev Physics Institute, Moscow 119991, Russia

ITEP, Moscow 117218, Russia

Moscow Physical Engineering Institute, Moscow 115409, Russia

Laboratory of Quantum Topology, Chelyabinsk State University, Chelyabinsk 454001, Russia

KdVI, University of Amsterdam, the Netherlands

Columbia University, Department of Mathematics and ITEP, Moscow, Russia

## 1 Introduction

In [1, 2] we started a study of the ’t Hooft genus expansion for colored knot polynomials [3]. There are at least five immediate subjects of interest about it:

• a realization of the AMM/EO topological recursion of [4], which was investigated for a couple of simplest examples in [5];

• integrability properties of generating functions like the Ooguri-Vafa partition function [6]; this includes their expansion over the symmetric group characters [1, 2] and representation as Hurwitz [7, 8] and ordinary KP/Toda -functions [9, 2], relation between these two representations being familiar from the old theory of renormalization group flows [10];

• differential and difference equations [11, 12, 13] satisfied by the colored knot polynomials as functions of their representation indices;

• relation between the genus and ordinary loop expansions, where the latter is related to the Vassiliev invariants [14, 15] and the Kontsevich integrals [16];

• the double-scaling large representation limit, where the knot polynomials acquire interpretation in terms of the hyperbolic volumes via the volume conjecture [17] and possess interesting -matrix representations [18] based on the theory of cluster mutations [19].

Only a partial progress along these directions was achieved in [1, 2] and the entire story requires much more attention than it received so far. Still, in this letter we proceed in a somewhat different direction: we consider the genus expansion of the superpolynomials [20, 21, 22, 23, 25, 12, 24, 26]. It involves a number of new elements:

1. the expansion can no longer be in the symmetric group characters, and their adequate MacDonald deformation is still unknown;

2. because of this, one can not yet provide a proper modification of the Hurwitz partition functions; however, the -deformation of the narrower class of Casimir characters is straightforward, and thus the KP/Toda-like representation is readily available;

3. the loop expansion of superpolynomials can and does (as we demonstrate) possess more terms than that of HOMFLY, i.e. at , what can be a signal that the set of Vassiliev invariants is enlarged by consideration of the superpolynomials;

4. this observation makes even more important study of the loop expansion of the Khovanov-Rozansky (KR) polynomials [27], to which the superpolynomials are related in a somewhat non-trivial fashion[20]; this poses new puzzling questions about the relation between the genus and loop expansions in generic cohomological theories and also calls for a better understanding of the colored KR polynomials, which can hopefully be achieved by unification of modern alternatives to the cabling method [28, 29] and to the KR calculus [30].

The goal of the present letter is to begin investigation of these issues.

## 2 Hurwitz exponentials

### 2.1 Hurwitz partition function

Consider a function given on the space of irreducible representations, which are labeled by the Young diagram . In this section we discuss conditions when this -dependent function can be expanded into the symmetric group characters .

Let us introduce variables and assume that is a power series in all variables , and, moreover, is a symmetric function in . It is well-known that the eigenvalues of Casimir operators for : , are symmetric polynomials in [32]. Moreover, the first Casimir operators are algebraically independent and one can easily check that their eigenvalues form a multiplicative basis of symmetric functions of degree not higher than . Allowing to be arbitrarily large, one can conclude that can be expanded in the basis of the eigenvalues of Casimir operators.

Let us make the argument more explicit. Consider an irreducible representation of labeled by the Young diagram , then, the Casimir operator is proportional to the identity operator in accordance with the Schur lemma222The shift can be replaced with any other constant, this induces a linear transformation of the set of Casimir operators, the particular choice of being more convenient for many purposes, including application to the genus expansion.:

 ^C(k) = CR(k)^I, (1) CR(k) = l(R)∑j=1(Rj−j+1/2)k−(−j+1/2)k. (2)

In particular, it follows from the Schur lemma that for the Casimir operator the prime character of the linear group is its eigenfunction:

 ^C(k)χR=CR(k)χR. (3)

It is convenient to introduce multiplicative combinations of Casimir operators labeled by partitions (Young diagrams) :

 ^C(Δ) = l(Δ)∏j=1^C(δi), (4) ^C(Δ)χR = CR(Δ)χR. (5)

The symmetric polynomials of evidently form a linear basis in the space of all symmetric polynomials of degree not higher than . Then, each concrete term of the power series can be expanded in this basis, choosing each time large enough , i.e. any symmetric power series in is expanded in the basis of .

Note that, in accordance with the Frobenius theorem, the linear group character is a symmetric polynomial of the monomials :

 pδ=∑ixδi,  pΔ=∏ipδi, (6) χR=∑|Δ|=|R|z−1(Δ)ΦΔRpΔ, (7)

where counts the order of the automorphism group of the Young diagram and the transition matrix is the character of the symmetric group [33, 34]. We use, however, differently normalized characters so that

 χR(p)=∑|Δ|=|R|dRφR(Δ)pΔ (8)

where is dimension of the irreducible representation of symmetric group [8].

These symmetric group characters are eigenvalues of the cut-and-join operators [8]

 ^WΔχR=φR(Δ)χR. (9)

and the operators form a basis related with that of by a linear transformation [8]. Therefore, due to (4) and (9), the eigenvalues of and are also related by a linear transformation. Note that the operators and can be represented by differential operators in time variables . Their explicit form also can be found in [8].

This claim that the multiplicative combinations of eigenvalues of the Casimir operators (4) are linear combinations of the symmetric group characters can be considered as one of the corollaries of the Schur-Weyl duality.

To summarize aforesaid, one concludes that the function can be expanded in if and only if is a symmetric power series in :

 SymmPowSer(Ri−i)=Ser{φR(Δ)} (10)

As is well-known [35] the characters are related by the Frobenius formula with the Hurwitz numbers

 Covn(Δ1,…,Δk)=∑Rd2RφR(Δ1)…φR(Δk)δ|R|,n, (11)

which counts the number of -sheet coverings of the Riemann sphere with ramification points of given ramification types. The type of ramification at the point characterizes the way in which the sheets are glued, and is labeled by the Young diagram (integer partition of ) of weight . The generating function of the Hurwitz numbers which depends on infinite sets of variables , and on an infinite set of variables is given by

 Z(p(i)|wΔ)=∑Rd2RK∏i=1χR(p(i))dRexp{∑ΔwΔφR(Δ)}=exp(∑ΔwΔ^WΔ)Z(p,p′,p′′,…|0), (12)

where acts on any set of variables , i.e. on any of the linear characters in the product. In the case of this partition function becomes a KP tau-function, see [36].

Now we return to the function . It can be re-expanded to the following form:

 (13)

with being complicated combinations of the expansion coefficients of in the basis of . Functions of such a type we call Hurwitz exponential since these are exactly the exponentials entering the Hurwitz partition functions (12).

### 2.2 From Hurwitz to KP partition functions and renormalization group

Let us comment more on the two bases, multiplicative and additive . Note that the generic Hurwitz exponential spanned by the additive basis (13) gives rise to the generating function which is not a KP -function [36]. However, if the exponential is spanned by the linear basis (2),

 FR=exp{∑ktkCR(k)} (14)

(12) at is the Toda lattice -function [36, 37] with respect to times . Moreover, it is also the Toda chain -function at [36] with respect to times .

When dealing with these Hurwitz exponentials, one may keep in mind the following analogy with the renormalization group (RG) and completeness of basis [10]. Let us consider a quantum field theory partition function

 Z(G;φ0;t)=∫A;φ0Dϕexp(12ϕGϕ+A(t;ϕ)) (15)

which depends on: (a) the background fields ; (b) the coupling constants and (c) the metric .

The coupling constants parameterize the shape of the action

 A(t;ϕ)=∑n∈Bt(n)On(ϕ), (16)

where the sum goes over some complete set of functions , not obligatory finite or even discrete. The space of actions parameterized by the coupling constants , is referred to as the moduli space of theories. The actions usually take values in numbers or, more generally, in certain rings, perhaps, non-commutative. The space of all functions of is always a ring, but this needs not be true about the moduli space , which could be as small a subset as one likes. However, the interesting notion of partition function arises only if the completeness requirement is imposed on . There are two different degrees of completeness, relevant for discussions of partition functions. In the first case (strong completeness), the functions form a linear basis in , then is essentially the same as itself. In the second case (weak completeness), the functions generate as a ring, i.e. an arbitrary function of can be decomposed into a sum of multiplicative combinations of ’s. In the case of strong completeness, the notion of RG is absolutely straightforward, but there is no clear idea how RG can be formulated in the case of weak completeness (which is more relevant for most modern considerations).

In the strongly complete case, the non-linear (in coupling derivatives) equation, even if occurs, can be always rewritten as a linear equation. In fact, one can easily make a weakly complete model strongly complete, by adding all the newly emerging operators to the action , then, if the product is added with the coefficient , one has an identity .

The core of the analogy is that (linear basis) corresponds to a strongly complete set and (multiplicative basis) corresponds to a weakly complete set of operators. Moreover, as we saw one can lift the multiplicative basis to the linear basis as the weak completeness lift to the strong completeness, i.e. via introducing new operators (4).

### 2.3 HOMFLY polynomial as Hurwitz exponential [1, 2]

In s.2.1 we outlined the necessary and sufficient conditions for to be a Hurwitz exponential. Here we explain why the HOMFLY polynomials are the Hurwitz exponentials. This fact was realized in [1] by explicit calculations.

We need to check that the HOMFLY polynomials are symmetric functions in and power series in . The first property follows from the fact that the HOMFLY polynomial is the vacuum expectation value of the Wilson loop in Chern-Simons theory with the gauge group [38]:

 HR=⟨TrR(U)⟩CS=⟨χR(U)⟩CS, (17)

where is the Wilson loop which is a group element of and the Chern-Simons averaging goes over the gauge field . The HOMFLY polynomial defined in a such way for any knot is actually not a polynomial but a rational function. To get a polynomial, one needs to normalize dividing it by the HOMFLY polynomial of unknot, which is equal to the Schur function , calculated at the special point (topological locus)

 p∗k=Ak−A−kqk−q−k. (18)

Therefore, the normalized HOMFLY polynomial is

 HKR=⟨χR(U)⟩CSχR(p∗). (19)

Using formula (8) in this case, one gets that

 (20)

Since form a linear basis in the algebra of polynomials symmetric in [31], it is clear from (20) that is a symmetric function in . Moreover, the numerator is a symmetric polynomial and the denominator is a symmetric polynomial. Let us show that the denominator has a constant term as a function of variables . To this end, we rewrite the denominator as

 ∑|Δ|=|R|φR(Δ)p∗Δ=χR(p∗)dR. (21)

The dimension is given by the following formula:

 dR=|R|∏1=i

The character can be expressed through the eigenvalues of matrix by the second Weyl determinant formula

 χR[X]=deti,jxmjideti,jx−ji. (23)

From this formula it is obvious that has zeros at the points , furthermore, the multiplicities of zeros equal to (take the corresponding derivative). Expanding the function as series in it is easy to prove by induction that the lowest term has exactly the same degree as Vandermond, hence, it is proportional to , which cancels with a similar product in . Thus, one would expect that the denominator does not have a pole at the point and the HOMFLY polynomial (20) is a power series in .

In other words, we claim that the HOMFLY polynomial is a symmetric function of and can be regarded as a power series in these variables. Therefore, taking into account (10), one can conclude that the HOMFLY polynomial can be expanded into basis of :

 HKR=exp{∑ΔwKΔ⋅φR(Δ)} (24)

with some coefficients . This means that the -dependence is fully concentrated in , while the coefficients encode the information about the knot .

Now one can naturally consider the generating function of the non-normalized HOMFLY polynomials, i.e. their sums with the Schur functions depending on the source variables :

 ZH=∑RχR(¯p)HR=⟨exp(∑n1k¯pkTrUk)⟩CS=∑RχR(¯p)χR(p∗)HR (25)

where the trace is taken over the fundamental representation. On one hand, this is exactly the Ooguri-Vafa partition function which was considered in [6] in the context of duality of the Chern-Simons theory and topological string on the resolved conifold. On the other hand, this is the Hurwitz partition function (12) with : the case, when the Hurwitz partition function celebrates its most interesting properties, in particular, integrability [36]. Note that the Hurwitz form (24) of the HOMFLY polynomial is essential not only for studying its integrable properties [2], it also provides a link to the open Gromov-Witten invariants etc [39].

In the next two sections we consider two particular expansions of into perturbative series, which are induced by two important expansions of the HOMFLY polynomials.

## 3 Two important expansions involving Hurwitz structure

There are several important perturbative expansions of the HOMFLY polynomials. These are: the ”volume”  expansion, genus expansion, Vassiliev expansion, all of them giving rise to very interesting invariants. We do not consider the ”volume”  expansion here, because it deals with the limit , and we are going to study the -dependence. Hence, we consider in this section the two other expansions. For each expansion, we specify the coefficients .

### 3.1 Genus expansion [1]

The genus expansion (’t Hooft limit) of HOMFLY polynomials is a perturbative expansion of correlation function commonly used in matrix model and QFT, which is also known as large expansion. It corresponds to coupling constant of the theory going to zero and the parameter of the gauge group going to infinity, with their product kept constant. In [1] it was demonstrated that the genus expansion for the HOMFLY polynomials gets natural form of a Hurwitz exponential (24) with particular values of constants naturally scaled with :

 HKR(q=eℏ/2,A)=exp{∑Δℏ|Δ|+l(Δ)−2⋅SKΔ(ℏ2,A)⋅φR(Δ)} (26)

i.e.

 wKΔ=ℏ|Δ|+l(Δ)−2⋅SKΔ(ℏ2,A). (27)

The rescaled coefficients are series in with coefficients depending on the knot but not on the representation . Actually, they also depend on the group, e.g. for the Kauffman polynomials ( group), they are different.

### 3.2 Vassiliev expansion

Though the dependence of HOMFLY polynomials on is completely captured by , in there is still a dependence on the group, hidden in the parameter . Therefore, one may ask how to separate in this dependence from the dependence on the knot. To answer this question, one has to construct a perturbative expansion of , keeping finite in (26), i.e. putting . This leads to the Vassiliev invariants. In fact, what one obtains in this way is nothing but the Kontsevich integral, which is a perturbative series in with coefficients given by the trivalent diagrams and Vassiliev invariants [40, 42]:

 HKR(A=eNℏ2,q=eℏ2)=∞∑i=0ℏiNi∑j=1r(R)i,jvKi,j (28)

Here denote the trivalent diagrams, is dimension of the vector space formed by the trivalent diagrams, and are the invariants of finite type (Vassiliev invariants) of knot .

Representation (28) separates the information about the knot and the (gauge) group. The knot information is given by the Vassiliev invariants which are nothing but the integrals (combinatorial sums) over the given knot [40, 42, 41]. They are rational numbers. The group (and the representation) information is given by the trivalent diagrams which are generated by the Casimir operators of the corresponding algebra.

The trivalent diagrams are represented by the polynomials of degree in . Thus, (28) is the double series in powers of and such that the degree of is larger or equals to that of . As follows from (26), the coefficients of these polynomials can be expressed in terms of (see Appendix A for some examples):

 r(R)i,j = i∑k=0c(R)i,j,kNk, c(R)i,j,k = ∑|Δ|+l(Δ)−2≤i−kcΔi,j,kφR(Δ), (29)

where . Representation (29) for the trivalent diagrams can be evaluated using paper [1] or by direct calculations. At the moment, it seems that concrete have no any particular sense: since there is no a canonical choice of the basis in the space of trivalent diagrams, one would associate concrete with a particular choice of the basis.

Thus, taking into account formulas (3.2), one gets

 HKR(ℏ,N)=∑i,j,k∑|Δ|+l(Δ)−2≤i−kℏivKi,jNkcΔi,j,kφR(Δ) (30)

## 4 Superpolynomial deformation of the Hurwitz exponential

Superpolynomials are also polynomial invariants depending on the representation , with one additional variable as compared with the HOMFLY polynomials. Hence, there is a question of describing the -dependence of superpolynomials, of extrapolating a Hurwitz exponential pattern. In this section, we discuss this question.

### 4.1 Superpolynomials are not Hurwitz partition function

In order to prove that the HOMFLY polynomials are Hurwitz exponentials we used the symmetry property, which follows from the fact that the HOMFLY polynomials are averages of the characters, that is, of the Schur polynomials. For the superpolynomials, the Schur polynomials are replaced with the MacDonald polynomials [25]. However, these latter are not antisymmetric functions in , i.e. it is impossible to expand the superpolynomial in the basis of .

Consider, for instance, the MacDonald polynomials at the special points . Then, they are manifestly given by

 M∗R=β−1∏k=0∏1≤j

Put . Then, it is clear from this formula that the MacDonald polynomials are antisymmetric in rather than . Moreover, they are uniquely defined as a common system of eigenfunctions of the commuting set of operators generalizing the Casimir operators, which are nothing but the Ruijsenaars Hamiltonians [43]:

 ^Hk=∑i1<...

where the Van-der-Monde determinant and the shift operators are defined as:

 ^Pk=qβxk∂xk,   ^Qk=q(1−β)xk∂xk (33)

The spectrum of (32) can be defined from the eigenvalues of spectral operator:

 (n∑k=0zk^Hk)MR(x1,...,xn)=∞∏i=1(1+zqRi+β(n−i))MR(x1,...,xn) (34)

Thus, the eigenvalues are symmetric in . This appeals to construct a full set of symmetric polynomials in . Unfortunately, in this case there is no a counterpart of the Schur-Weyl duality known, and the MacDonald polynomials are not simple characters. Hence, there is no a distinguished set of symmetric functions of , and we construct the full sets of symmetric polynomials in in two ways in order to present the superpolynomial as a deformed Hurwitz exponential.

### 4.2 Beta-deformation of Casimir operators

As a simplest deformation, one may consider a very naive -deformation of the Casimirs eigenvalues:

 CβR(k)=∑i(Ri−βi+12)k−(βi+12)k. (35)

It is clear that for they are equal to (2). They are also clearly symmetric in . Hence, one can use them to construct a full set of symmetric polynomials in analogy with formula (4):

 ^Cβ(Δ) = l(Δ)∏j=1^Cβ(δi). (36)

However, any interpretation of this set neither from mathematical nor from physical point of view is known. For this reason, we suggest another construction.

### 4.3 Operators ^Tk

Since we are interested in a basis symmetric in , it is allowed not to depend on at all. Indeed, there are ”intermediate” symmetric functions, which generalize the Schur functions but still solve the (trigonometric) Calogero-Moser system. These are the Jack polynomials [34]. They are obtained from the MacDonald polynomials just in the limit of . Since the Jack polynomials are defined to be eigenvalues of the trigonometric Calogero-Moser Hamiltonians , one can consider their generating function:

 (u|R|∞∑i=0u−i^Hi)JR=T(u)JR (37)

the generating function for the eigenvalues being

 T(u)=∏(i,j)∈λ(u−(i−1)β+(j−1)) (38)

Then, it is natural to define the operators such that

 ^TβkJR = Tβk(R)JR, Tβk(R) = ∑i,j((j−1)−β(i−1))k−1, (39)

These operators play an important role in the theory of Jack polynomials, the latter being somewhat mysteriously connected [44] with the AGT relations [45]. It is possible to express through linear combinations of .

The full set of functions is then given in complete analogy with (4):

 TβΔ(R):=l(Δ)∏i=1Tβδi(R). (40)

For explicit calculations we used exactly this basis. Thus, one can write the most general form of the -deformation of the Hurwitz exponential (24) for the superpolynomial:

 PKR=exp{∑ΔωKΔ⋅TβΔ(R)} (41)

Particular values of constants can be dealt with by particular perturbative expansions, similarly to the HOMFLY case. We again consider the two particular examples: the genus expansion and the Vassiliev expansion.

### 4.4 Genus expansion of superpolynomials

The genus expansion of the superpolynomial is given by , , (i.e. const), is arbitrary and is a more or less straightforward generalization of the Hurwitz exponential at , that is, and :

 PKR(q=eℏ/2,t=eβℏ/2,A) = exp{∑Δℏ|Δ|+l(Δ)−2⋅SKΔ(ℏ2,β,A)⋅TβΔ(R)} (42)

i.e.

 ωKΔ=ℏ|Δ|+l(Δ)−2⋅SKΔ(ℏ2,β,A). (43)

Why do we think that this definition makes sense? First of all, making computational experiments with particular superpolynomials, we observe that their expansions are very similar to expansions of the HOMFLY polynomials (26). By this reason we suggest that the definition of superpolynomial expansion has same structure. Second, we may expect that the dependence on the representation should be described by nice enough understandable functions. Actually, they should be -deformed counterparts of symmetric group characters, but at the present moment we are not aware of such a deformation. In the previous subsections, basing on symmetric properties of the Macdonald polynomials, we gave our arguments why we consider just as a full basis. Third, we expect that in the order of the expansion only the diagrams satisfing the condition

 |Δ|+l(Δ)≤n+2

can contribute. Our definition (42) is based on these three points.

Originally, there was a hope that the coefficients of the expansion could be independent on so that the full -dependence would be hidden in the group factors . However, it seems not to be the case. Instead, the coefficients are deformations of arising in the HOMFLY case, where they are generating functions of the higher special polynomials

 SKΔ(ℏ2,A)=∞∑n=0ℏ2nσKΔ(n).

One can proceed similarly in the superpolynomial case (42)

 SKΔ(ℏ2,β,A)=∞∑n=0ℏ2nsKΔ(n)

Here are polynomials in and . In Appendix A, we give a few explicit examples.

At the zero and the first orders our definition is agreed with the expansion from [24]:

 PR(A,q,t)q=eℏ/2, t=eβℏ/2=P|R|□+ℏ(νRt−βνR)σ|R|−2□σ2+…, (44)

where is the special polynomial, is the higher special polynomial of the first order (see [1] for details), .

Equation (42) is far from being tautological: it implies non-trivial relations between superpolynomials in different representations. In particular, it restricts the shape of superpolynomial for the hook Young diagrams, as soon as one knows it in all symmetric and antisymmetric representations. As we are going to demonstrate, this restriction is quite severe: it can even imply that generic colored superpolynomials are non-positive! Whether this is a drawback or an advantage of our postulate (41) remains to be understood.

### 4.5 Is colored superpolynomial positive?

There is a lack of examples of superpolynomials in non-symmetric representations. Even so, we check all known examples for consistency with expansion (42). That is, we expanded the superpolynomials in symmetric and antisymmetric representations into series of , and then calculated the coefficients in front of the corresponding . For the first and the second orders, it is enough to consider only (anti-)symmetric representations to fix all the coefficients. Thus, the first and the second orders are determined for all other representations. We checked if they coincide with the corresponding orders of known (hypothetical) superpolynomials in non-symmetric representations. We considered the two cases: the trefoil and the figure eight knot. The explicit expressions for the zero, first and second orders are given in Appendix A.

In [24] it was suggested to look for a superpolynomial of the figure eight knot in the form with some coefficient :

 P41[2,1](q,t,A) \lx@stackrel?= 1+(Z(−1|−1)3|3+Z(1|0)1|1+Z(0|1)1|1)+(Z(0|−1)3|3Z(1|0)1|1+Z(−1|0)3|3Z(0|1)1|1+αZ(1|0)1|1Z(0|1)1|1)+Z(0|0)3|3Z(1|0)1|1Z(0|1)1|1 (45) Z(s|σ)I|J(A) = {AqI+st−σ}{Aqst−J−σ},     {q}=q−1q (46)

It was argued that the positivity restricts this coefficient to be :

 P41[2,1]\lx@stackrel?=1a6t10q10(3a10t16q10+5a8t14q12+3a8t16q16+q12t5a2+3a4t10q16+5a4t6q8+q20a4t12+5q12a4t8+ +q20a8t18+2a4t8q14+3q4a4t4+2a6t15q20+2q2a6t6+8q14a6t12+a6t9q6+8q10a4t7+5q14a4t9+ +q2a4t3+q18a8t17+q4a2t+a2t7q16+5q14a8t15+q8a2t3+5a6t7q4+8q8a6t9+a12t20q10+5q16a6t13+ +a10t14q6+a6t13q14+a10t19q16+a2t6q14+a4t2+q10+a4t11q18+5q6a4t5+a8t8+2a6t5+11a6t10q10+ +2q6t4a4+2a8t12q6+2a8t16q14+3a8t10q4+a8t9q2+2a8t12q10+2q18a6t14+q6a2t2+a6t7q6+q14a2t5+ +a10t15q6+2q10t3a2+q6a2t+3a2t4q10+a10t15q8+a6t11q14+5a8t12q8+2a6t9q10+2q10a4t6+ +2a4t8q10+2a8t14q10+5q6a8t11+q14a10t18+a10t19q14+a10t13q4+a10t17q12+2a10t17q10+ +8q10a8t13+8q6a6t8+8a6t11q12+2a6t11q10) (47)

However, this is inconsistent with our expansion, which requires that . This behavior could imply that , which is also symmetric under the permutation (which is expected for such a highly symmetric knot as in representation with symmetric Young diagram). However, such breaks the positivity: not all the coefficients of the superpolynomial enter with positive integer coefficients333The positivity is presented in the homological variables , hence we use them in these examples, while for making expansions we use the Macdonald variables . In order to clarify our notation, we list here the superpolynomial of the trefoil in the fundamental representation: (48) :

 P41[2,1]\lx@stackrel??=1a6t10q10(−a4t10q14+a10t16q10−q10a2t5+a10t17q12+5a8t14q12+3a8t16q16−a4t6q6+3a4t10q16− −a8t14q14+5q12a4t8+q20a8t18+a4t8q14+3q4a4t4+2a6t15q20+8a6t11q12+2q2a6t6+4q14a6t12− −a6t9q6+3q14a4t9+q2a4t3+3q6a8t11+q18a8t17+4q10a8t13+q4a2t+a2t7q16+3q14a8t15+5a6t7q4+ +8q8a6t9+a12t20q10+5q16a6t13+a10t14q6−a6t13q14+a10t17q10+a2t6q14+a4t2+q10+a4t11q18+ +3q6a4t5+a8t8+2a6t5+7a6t10q10+4q6a6t8+q6t4a4+q14a10t18+a8t12q6+a8t16q14+2q18a6t14+ +q6a2t2−a6t7q6+q14a2t5+q10t3a2+a10t13q4+q6a2t+a2t4q10+a10t15q8−a6t11q14−a10t15q10− −a8t10q6+5a8