Dual Frobenius manifolds of minimal gravity on disk

Liouville field theory approach to 2-dimensional gravity possesses the duality ($b \leftrightarrow b^{-1}$). The matrix counterpart of minimal gravity $\mathcal{M}(q,p)$ ($q<p$ co-prime) is effectively described on $A_{q-1}$ Frobenius manifold, which may exhibit a similar duality $p\leftrightarrow q$, and allow a description on $A_{p-1}$ Frobenius manifold. We have positive results from the bulk one-point and the bulk-boundary two-point correlations on disk that the dual description of the Frobenius manifold works for the unitary series $\mathcal{M}(q, q+1)$. However, for the Lee-Yang series $\mathcal{M}(2, 2q+1)$ on disk the duality is checked only partially. The main difficulty lies in the absence of a canonical description of trace in the continuum limit.


Introduction
The Liouville field theory shows that there is a weak-strong coupling constant duality b ↔ b −1 in correlation functions. This is demonstrated in DOZZ 3-point correlation on sphere [1][2][3]

which is invariant under
where µ is the cosmological constant and γ(x) = Γ(x)/Γ(1− x). The same duality holds for the one-point correlation on disk [4,5] with the boundary parameter s unchanged where the boundary cosmological constant µ B is is defined as where κ = µ sin πb 2 . The minimal Liouville gravity M(q, p) with q < p co-prime is also effectively described by A q−1 Frobenius coordinates [6]. The connection with Liouville gravity is given as b 2 = (q/p) < 1. Therefore, one might naturally wonder if the same Liouville gravity is equally described by A p−1 Frobenius coordinates. One may find a brief description of this duality property of matrix model in [7] and a detailed check for Lee-Yang series on sphere [8,9] which shows that careful analysis is needed.
In this paper we concentrate on testing the duality of the minimal gravity on a disk. In section 2, we provide the general structure of 2-dimensional gravity on a sphere and on a disk using the coordinates of Frobenius manifold. In section 3, we check the dual property of unitary models by using bulk one-point correlation and bulk-boundary twopoint correlation on a disk. We find that flat coordinates of the original and its dual Frobenius manifold provide a convenient path for evaluating correlation numbers on a sphere as well as on a disk. In section 4, we check the dual property of Lee-Yang series (nonunitary case) on a disk. However, the duality is confirmed only partially. The difficulty lies in finding the proper contour integration which corresponds to summing up the orthonomal states available in the random hermitian matrix model. Section 5 is the conclusion. The appendix contains useful formulae of the Bessel function and the Jacobi polynomials, and the computation of resonance relations for the original and its dual Frobenius manifolds obtained from the orthogonality of two-point correlations on a sphere.
2 Frobenius manifolds in random matrix model of minimal gravity

Frobenius manifold and Liouville correlation numbers
The matrix degree of freedom of random matrix model is represented by an operator Q in the continuum limit. It is defined as a differential operator [10], whose Fourier transform reads where some terms irrelevant for our purpose (i.e., calculations on the sphere and disk) are dropped. Here y stands for the Fourier space coordinate and u i 's form a system of co-ordinates for a (q − 1)-dimensional Frobenius manifold A q−1 . Details may be found in [6,11] and some are summarized in appendix A. The flat co-ordinates on A q−1 are defined by v i = θ i,0 with where k ∈ {0} ∪ N and (a) n = Γ(a + n)/Γ(a) is the Pochhammer symbol. Minimal Liouville gravity M(q, p) is specified by two co-prime integers p and q (q < p), where q is identical to the order of Q. Q and its conjugate P = Q p/q + . . . are required to satisfy the Douglas string equation [P, Q] = 1 which is effectively described in terms of an action principle [7] where the action is given by S q/p (v) = Res y=∞ Q (p+q)/q + m,n t m,n Q |pm−qn|/q , where 1 ≤ m < q and 1 ≤ n < p. Each KdV parameter t m,n has Z 2 symmetry and is identified with t q−m,p−n and is only defined up to a normalization factor. The number of these parameters is equal to the number of allowable operators in the minimal model. The string equation reduces to the equation of motion, which establishes a relation between v i 's and t m,n 's. The KdV parameters t m,n can be identified with the coupling constants λ m,n of the Liouville gravity, up to resonance terms in general. The gravitational scaling dimension (powers of the cosmological constant µ) is assigned to the coupling constants as [12] [t m,n ] = [λ m,n ] = p + q − |mp − nq| 2q . (2.5) Note that [λ 1,1 ] = 1, and therefore λ 1,1 can be identified with the cosmological constant µ.
The assignment implies that the identification of the coupling constants can involve higher order corrections, so that resonance transformation has non-linear terms [13] t m,n = λ m,n + A m 1 ,n 1 ,m 2 ,n 2 λ m 1 ,n 1 λ m 2 ,n 2 + · · · , (2.6) where [λ m,n ] = [λ m 1 ,n 1 ]+[λ m 2 ,n 2 ] and the numerical factors A m 1 ,n 1 ,m 2 ,n 2 can be determined by an order-by-order calculation. The bulk correlation numbers on a sphere are generated from the free energy [6,13] where C a bc = η ad C dbc is the structure constant of the Frobenius manifold in the flat coordinate basis. The two-point correlations and their dual descriptions are summarized in appendix C.
The correlation numbers on a disk is simply given in terms of the generating function [14] F disk = − tr log C(Q) , (2.8) where the trace is to be replaced by the integration of a continuous variable x, which has the highest gravitational scaling dimension. C(Q) is a polynomial of the operator Q and can be extended to be matrix valued depending on the insertion of boundary operators.
The degree of C(Q) in Q fixes the boundary condition. The simplest boundary condition corresponding to an insertion of the identity operator on the disk boundary is obtained by taking a first order polynomial C(Q) in Q, denoted by C(Q) = µ B − Q. Here µ B is a parameter corresponding to the boundary cosmological constant. In this case, the generating function reads where we introduce a subscript to indicate the order of C(Q) and the trace is to be replaced by the contour integration over x with the highest gravitational scaling dimension. The variable x corresponds to the continuum limit of the orthonormal states available in the hermitian matrix model. A derivative of the generating function with respect to a coupling constant λ m,n yields a bulk one-point correlation number with (1, 1) boundary condition: The subscript * denotes the on-shell values which turn off all coupling constants except λ 1,1 and use the Frobenius coordinates as the solution of the Douglas string equation. The correlation number (2.10) has an equivalent but alternative expression in terms of a function W(l) introduced in the following. A derivative of F (1) with respect to µ B gives where W(l) is defined by Here x 1 is identified with the coupling constant λ m 1 ,n 1 of the highest scaling dimension. By definition, ω(µ B ) is the Laplace transform of W(l) where its integration contour of l from 0 to infinity is to be properly defined so that the Laplace transformation is convergent. Using this object W(l), an alternative expression for the correlation number is obtained by (2.14) Therefore W(l) plays the role of generating function with a given boundary length l. Thus we may refer to W(l) as generating function, as long as no confusion arises. Accordingly, we will also call the objects like (2.14) correlation numbers hereafter. The bulk-boundary two-point correlation with (1, 1) boundary condition is obtained by taking the derivative of F (1) with respective to µ B in addition to λ m,n : where B is identified with the boundary operator B 1,1 . Other boundary conditions are obtained when C(Q) is properly defined. For example, let us take a second order polynomial in Q: where we have expanded 1/C(Q) in partial fractions and have used ω(x ±1 ) = − tr(x ±1 − Q) −1 .
Its on-shell value, which is to be identified with the one-point correlation number for the boundary operator B 1,2 , is required to vanish. This imposes a condition [14] on the boundary parameters x ±1 = κ cosh πbs ±1 : The on-shell value of the derivative of F (2) with respect to λ m,n reads (2.17) which is identified with the bulk one-point correlation with (1,2) boundary O m,n (1,2) (s).
One may extend the process to the (1, k) boundary One may compute the bulk-boundary two-point correlation for (1, 2) boundary condition as: An extension to the (1, k) boundary condition is straightforward when α 's are rational functions of x α = κ cosh(πbs α ) given by Note that the one-point correlation (k = 1) vanishes because s α = s + iαb.
The results of bulk-boundary two-point correlations (2.22) can be compared with their counterparts of field theoretic approach. The point of our interest is whether matrix model approach reproduces their s-dependent part (up to normalization) [16,17] (2.25) with P m,n = b 2 |mp−nq| q and the boundary operator B is identified with B 1,k .

Dual Frobenius manifold
We can equivalently describe the M(q, p) (still q < p) minimal gravity on a A p−1 Frobenius manifold (instead of A q−1 Frobenius manifold) with Q(y) = y p + p−1 i=1 y p−1−i u i . In this case the Douglas action in (2.3) is replaced by the dual action where, as before, t m,n = t q−m,p−n . Note that for q < p we use the notation S p/q for the dual action and S q/p for the original action. The scaling dimension (denoted by curly brackets to distinguish from the A q−1 case) of the KdV parameters in this dual action is given by which represents the power ofμ. Note that {t m,n } = q p [t n,m ]. In particular, {λ 1,1 } = q/p measured in units ofμ and therefore, λ 1,1 in this dual description can be identified with the cosmological constant µ.
The bulk generating function on a sphere is similar to (2.7), with S q/p replaced by S p/q . The duality has been tested for the Lee-Yang series in [8,9]. One may use the disk generating function analogous to (2.8) with Q of order q replaced by that of order p.
The resolvents in (2.11) in both descriptions should be equal, but it is emphasized that the inverse Laplace transforms W(l) will be different from each other. This is because the boundary coupling constant µ B ∝ √ µ cosh(πsb) is replaced by the dual boundary coupling The bulk one-point correlations on disk with (1, 1) boundary in (2.13) and (2.14) are expected to behave similarly. To be precise, one finds where K ν (z) is the Bessel function. Here we use the notation O (q−1) m,n to stand for the expectation value of the (m, n) operator using the original (A q−1 ) action. In the dual (A p−1 ) description we find Both should result in the same FZZ one-point correlation: We can compute dual expectation values with (k, 1) boundary if we use the boundary free energyF (k) obtained in the dual A p−1 description. For example, the bulk one-point correlation corresponding to (2.18) for the case of (k, 1) boundary is given by and In addition, as a counterpart of (2.22), the bulk-boundary two point correlation with (k, 1) boundary condition is expected to have the form The boundary one-point correlations B (k,1) have a form analogous to (2.24) and therefore vanish when k = 1.

Frobenius manifold A 2
We recapitulate the calculations presented in [18], denoting Q 3 as Q of degree 3: The flat co-ordinates are v i = θ i,0 = u i (i = 1, 2) using (2.2). The Douglas action is given by a linear combination of θ 1,0 , θ 2,0 , θ 2,1 and θ 1,2 : The scaling dimensions of the KdV parameters are We do not need the correction terms in the resonance transformation since t 1,n = λ 1,n + O(λ 3 ). The derivatives of S 3/4 are given by The Douglas equations are defined by setting (∂S 3/4 /∂v i ) = 0. We choose the following solution to define the on-shell conditions: The generating function for correlation numbers on a disk is given by The one-point correlation O 1,n (1,1) l on a disk can be obtained by differentiating W(l) with respect to λ 1,n and evaluating the result on-shell. For example, see the formulae in appendices A and B, This gives the desired µ and s dependence as given in (2.28). Strictly speaking, the argument of the Bessel function differs by a numerical factor. However it can be eliminated by an appropriate rescaling of l.
The correlator O 1,2 (1,1) l is slightly more involved, since we need to perform the x integral including an additional factor (∂Q 3 /∂λ 1,2 ) which is obtained by a variation of the Douglas equations with respect to λ 1,2 . That reads Similarly, Making use of Laplace transformation (2.13), we see that the bulk-one point correlation numbers with (1, 1) boundary condition reads for n = 1, 2, 3, which reproduces the known result (2.30).

Dual Frobenius manifold A 3
Let us now instead take Q to be of degree 4: We find that the flat co-ordinates v i in this case are related with u i 's by The Douglas action is given by a linear combination of θ 1,0 , θ 2,0 , θ 1,1 and θ 3,1 : The dual scaling dimensions of the KdV parameters are Since the ratios of the scaling dimensions is the same as in the A 2 description, there continues to be no non-trivial resonance transformation up to the order we need. The derivatives of S 4/3 are given by (3.10) We choose the following solution to define the on-shell conditions: As before, the correlation number O n,1 (1,1) l is obtained by differentiating the generating function with respect to λ n,1 : These results are consistent with the duality as suggested in (2.28)-(2.30). After Laplace transformation (2.13), we see that the bulk-one point correlation numbers with (1, 1) boundary condition reads . We note that (∂Q/∂t 21 ) * = y/v 1 , which makes the integrand for the y-integral an odd function, incorrectly giving O 2,1 (1,1) l = 0. This is another instance of a problem that has been pointed out in [18]. This happens in general when the degree of Q is even and the m in O m,n (1,1) l is even. We will continue to see instances of this in the general case that we deal with in the subsequent sections.
The bulk one-point correlation numbers O n,1 (k,1) (s) with (k, 1) boundary (k = 2, 3) reduces to a sum of O n,1 (1,1) (s α ) as in (2.31). The bulk-boundary two-point correlation (2.34): is proportional to R(P n,1 , kb, s) with P n,1 =b 2 3 , which is the same as P 1,n of A 2 description as mentioned below (3.7). Here B = B k,1 and the matrix model approach reproduces the s-dependent part of the bulk-boundary two-point correlation.

Frobenius manifold A q−1
The Douglas action for the unitary model M(q, q + 1) is given by We define x by On-shell, when all couplings besides λ 1,1 vanish, we have In order to compute the bulk one-point correlation on the disk O m,n (1,1) l , we need to evaluate (∂Q/∂λ m,n ), which can be computed as follows: Using (3.16), we can expand the Douglas action as a series in λ: where S m,n = θ m,m−n + (terms containing µ).
By demanding the vanishing of the variation of the string equation with respect to λ's, we find that ∂v a ∂λ m,n = − where [(∂ 2 S 0 /∂v 2 ) −1 ] a,b stands for the inverse of the Hessian matrix ∂ 2 S 0 /∂v a ∂v b . In this case, (3.20) Using orthogonality of the two-point correlations on the sphere [19] we find where P (α,β) n (z) stands for the Jacobi polynomial. The derivation of this is summarized in appendix C.1. Note that the on-shell value of the derivative (∂Q q /∂v a ) reads  In order for the integral to converge, l is properly chosen. In addition, we note that the integral identically vanishes when both q and n are even, since the integrand is an odd function of y in this case. This was also noted in [18]. In every other case, after performing the y-integration and up to normalization factors, we obtain The final step to compute the bulk one-point correlation O m,n (1,1) l is performing the x-integration of (3.25) from µ to ∞. This was done case-by-case in [18], and it was verified that it yields the expected answer in all those cases. We fill this gap by proving an integration formula (B.5), whose proof is summarized in appendix B. Using this integration formula, we obtain O m,n (m ≥ n) and B = B 1,k , which is proportional to R(P m,n , kb, s).

Dual Frobenius manifold A q
The dual action for M(q, q + 1) is Note that the v's and θ's used in A q description are distinct from those in A q−1 description, since these are derived from Q of order (q + 1), while the ones in the previous subsection were derived from Q of order q.
The number of operators in the M(q, q + 1) model in A q description is the same as in A q−1 description. We label operators with indices (n, m), where the two indices related as (n, m) ↔ (q + 1 − n, q − m) denote the same operator. We chose a set with m ≥ n, i.e., the entries on and above the diagonal in the matrix below: The gravitational scaling dimensions associated with these operators are where they are understood as the power ofμ ∝ µ q+1 q . The derivative of the action S (q+1)/q with respect to v 1 defines x by The on-shell value of x reads It is convenient to definex such thatx =μ x µ q+1 q . (3.32) We observe thatx ∝ v q+1 1 . Using the orthogonality of the two-point correlator on a sphere in the dual description (derived in appendix C.2), we find that The analogue of (3.20) in this case is  ∂λn,m exp(lQ q+1 ). Now, the only anomalous case is when q is odd and n is even, in which case the integrand is an odd function of y and the integral identically vanishes. In every other case, the result of this integration up to normalization factors is The earlier remarks about the normalization of l and a minor abuse of notation apply. As a final step, we need to integrate this over x as  The Lee-Yang model is the simplest for the Lee-Yang series M(2, 2q + 1) on disk. The one-dimensional coordinate v of the Frobenius manifold A 1 describes the Lee-Yang series [6]. We summarize the original Frobenius manifold description in this subsection.
The second order polynomial Q 2 = y 2 +v is used to find the Douglas action for M(2, 5) where the KdV parameters have the scaling dimensions [t 1,1 ] = 1 and [t 1,2 ] = 3/2. There is no resonance term between the two couplings up to the order of our interest, so that the KdV parameter t 1,n is identical to the Liouville coupling constant λ 1,n . A derivative of the action S 2/5 with respect to v gives where v is defined as the function of x. The generating function W(l) is given in terms of integration over x whose lower limit of integration range is identified as λ 1,2 3) The bulk one-point correlation numbers on disk with (1, 1) boundary condition are given as After Laplace transform we have the correlation numbers reads in agreement with (2.30). In addition, the resolvent ω(x ± ) reads where x ± = κ cosh(πbs ± ) and s ± = s ± ib. Therefore, the one-point boundary correlation number B (1,2) = 0 according to (2.24). For the (1, 2) boundary, one has the bulk onepoint correlation numbers O 1,n (1,2) (s) = ± O 1,n (1,1) (s ± ). Finally, the bulk-boundary two-point correlation (2.22) with P 1,n = b 2 5−2n 2 shows that B = B 1,2 .

Dual Frobenius manifold A 4 and its problem
The dual description is given by the four-dimensional Frobenius manifold A 4 with Q 5 = y 5 + u 1 y 3 + u 2 y 2 + u 3 y + u 4 . The relation between u i 's and the flat coordinates v i 's is given by The dual Douglas action reads whose derivatives with respect to v i give (4.10) These equations imply that v 2 and v 4 should be irrelevant and thus they will be omitted hereafter. Then x is reduced to The KdV parameters has no resonance up to the order of our interest, so that we have t n,1 = λ n,1 . We choose the on-shell value of v i as (1,1) l ∝κ 1/5 K 1/5 (κl), (4.14) whereκ ∝ µ 5/4 ∝ κ 5/2 . After Laplace tranformation, we can easily check that O 2,1 (1,1) in A 4 description has the same value O 1,2 (1,1) in A 1 description.
However, a troublesome issue arises in other correlation numbers. For example, O 1,1 (1,1) l is given as a derivative of W(l) with respect to λ 1,1 . with The relation among v 1 , v 3 and x is given by (4.11). The result depends on how to perform the x-integration. If one performs x-integration in terms of v 1 , dx = (v 3 /5)dv 1 while maintaining v 3 = 0, then the final result is proportional to v 3 and vanishes. If one fixes the x-integral as dx = (v 1 /5)dv 3 , the integral does neither vanish nor agrees with the b ↔ b −1 duality. The absence of the canonical description of x-integration is carried over into Lee-Yang series M(2, 2q + 1). It should be noted that similar problem already appeared in non-unitary series [18]. Therefore, one has to devise a proper way to perform x-integration to understand the duality for non-unitary series. Suppose we compute the resolvent To perform x-integration to find W(l) in the dual picture one may perform v 3 -integral from 0 to −∞, regarding v 1 and v 3 as independent of each other and get the following result.
where x ± =κ cosh(πbs ± ). The first term is what we want from the perspective of b ↔ b −1 duality. This shows that one needs to find a way to compensate the unpreferable second term by properly choosing the x-integration.

Conclusion
The b ↔ b −1 duality of the minimal Liouville gravity M(q, p) was examined in the matrix model approach using the original and its dual Frobenius manifolds A q−1 and A p−1 . We calculate the bulk one-point and bulk-boundary two point correlation numbers on a disk and found that the duality holds for the unitary series M(q, q + 1). The (1, k) boundary condition in the original picture corresponds to the (k, 1) boundary in the dual picture. The resonance transformation in the dual picture is also used. In contrast, for non-unitary series the duality is not easy to check. The correlation numbers without x-integration show the duality. However, the correlations with the presence of the x-integration depends on the choice of the integration path. This shows that one has to find a canonical prescription of contour integrations in the non-unitary series.
In the paper, we consider the boundary conditions of the type (1, k) in the original and (k, 1) in the dual descriptions. One may wonder if one can extend the results with mixed boundary conditions of the type (k, l) since according to the brane picture in [15] one has |(k, l); s = with s α 1 ,α 2 = s+iα 1b +iα 2 b. This is expected to appear after an extension of the formalism by combining both the original and dual Frobenius descriptions, which will be presented in the near future.
Acknowledgements. The work was partially supported by National Research Foundation of Korea grant 2017R1A2A2A05001164.

A Frobenius structure
We recall some facts and collecting some useful quantities about A q−1 Frobenius manifold. The reader is referred to the appendix A.1. of [6] for a detailed summary of these notions.
In the flat co-ordinates of A q−1 Frobenius manifold, the metric takes the form where the metric is used to raise and lower these indices (v a = v q−a for instance). The Frobenius algebra structure constants in these co-ordinates are given by The structure constants are symmetric under all permutation of indices and are defined in such a way that C 1ab = η ab = δ a+b,q . For our purposes it suffices to know the structure constants and various other quantities only along the line v k = 0 (k > 1). All quantities evaluated on this line will be indicated by a subscript v. The structure constants on this line are Particularly useful is On the line v k = 0 (k > 1), Q and its derivative with respect to the flat co-ordinates are given by where T n (z) is the Chebyshev polynomial. Finally, we note the derivatives of θ i,k respect to the flat co-ordinates on v: if k is even, (A.6)

B Bessel function and Jacobi polynomial
First we note the following facts about Chebyshev polynomials: Consider the following integral Let q be even. If m is even, then T ′ m (y) is an odd polynomial, making the integrand an odd function, thus causing the integral to vanish. If m is odd, then the integrand is an even function, and after a substition y = i sinh x and using (B.1), I can be evaluated using the following integral representation of the modified Bessel function of the second kind: Now let q be odd. We again substitute y = i sinh x. We can then use the integral representations To perform the x-integration when one computes the correlation numbers, the following integration formula is essential: where 0 < |ν| < 1 for our purposes, and we recall that K ν (x) = K −ν (x). To prove this formula, we first observe that the Jacobi polynomial appearing above can be written as a polynomial in (x − µ) as follows: We now perform the x-integration term by term, using which is proved by using the identity ∂ x K ν (x) = −K ν−1 (x) − (ν/x)K ν (x) recursively. Finally, the linear combination of Bessel functions thus obtained can be summed using the following identity: which is proved by using the identity K ν (x) + 2(ν+1) x K ν+1 (x) = K ν+2 (x) recursively. To summarize the derivation of (B.5): Finally, we note the following identity, which appears when we perform the Laplace transform (l-integration), with t = arccosh(α/β). Differentiating with respect to α gives ν sinh(νt) β sinh(t) = sin(νπ) π ∞ 0 dl e −αl K ν (βl). (B.10) C Orthogonality of two-point correlators on the sphere The first part of this section is largely a summary (with some notations modified for convenience) of section 3.2 of [19], where the two-point correlator on a sphere was calculated, and the resonance transformations were found for unitary models M(q, q + 1). We refer the reader to that paper for further explanations. In the second part, we do a similar calculation for M(q + 1, q).

C.1 A q−1 description
The two-point correlator on a sphere is given by where using S q/(q+1) = S 0 + m,n λ m,n S m,n + O(λ 2 ), we see that the dotted terms contain positive integer exponents of the cosmological constant µ.
There are three cases to be considered: (m 1 −n 1 ) and (m 2 −n 2 ) are both even, they are both odd and they have opposite parity. It can be easily checked by dimensional analysis that when (m 1 − n 1 ) and (m 2 − n 2 ) have opposite parity the two-point correlator is analytic (i.e., a non-negative integer power) in µ, and must thus be discarded as non-universal [6]. The only non-trivial constraints then arise from demanding the orthogonality of the twopoint correlator in the cases when (m 1 − n 1 ) and (m 2 − n 2 ) are either both even, or both odd.
First consider the case when m 1 − n 1 and m 2 − n 2 are even. Denote ∂S m,n ∂va = δ m,a f m,n . Then We already see that the two-point correlator vanishes if m 1 = m 2 , but we still need to explicitly require that it vanishes if Orthogonality now forces the f m,n 's to be proportional to a particular class of Jacobi polynomials: f m,n ∝ P (0, m q −1) k(m,n) (t), where k(m, n) is some integer. Knowing that P (0,b) k (t) ∝ t k + (lower-order terms in t), and comparing with (C.1), we see that k(m, n) = m−n 2 . Putting all this together, we find that h m 1 ,n 1 h m 2 ,n 2 dt.
Following a similar line of reasoning as in the even case, we conclude that h m,n ∝ P (0, m q ) m−n−1 2 (t).
Putting it all together, we find that where the dots now denote terms containing positive integer exponents of the dual cosmological constantμ.
When (m 1 − n 1 ) and (m 2 − n 2 ) have opposite parities, we see that n 1 + n 2 = q + 1, and that the the scaling dimension above is an integer. Once again, when the result of an expectation value turns out to be analytic inμ, the result must be discarded as being non-universal. This leaves us with cases where (m 1 − n 1 ) and (m 2 − n 2 ) have the same parities.
Consider the case when (m 1 − n 1 ) and (m 2 − n 2 ) are even. Denote ∂S n,m ∂va = δ n,af n,m . Then