Testing 5d-6d dualities with fractional D-branes

6d SCFTs compactified on a circle can often be studied from nonperturbative 5d super-Yang-Mills theories, using instanton solitons. However, the 5d Yang-Mills theories with 6d UV fixed points frequently have too many hypermultiplet matters, which makes it difficult to use the ADHM techniques for instantons. With the examples of 6d N=1,0\documentclass[12pt]{minimal} \usepackage{amsmath} \usepackage{wasysym} \usepackage{amsfonts} \usepackage{amssymb} \usepackage{amsbsy} \usepackage{mathrsfs} \usepackage{upgreek} \setlength{\oddsidemargin}{-69pt} \begin{document}$$ \mathcal{N}=\left(1,\ 0\right) $$\end{document} SCFTs with Sp(N) gauge symmetry and 2N + 8 fundamental hypermultiplets, we show that one can still make rigorous studies of these 5d-6d relations in the ‘fractional D-brane sectors’. We test the recently proposed 5d duals given by Sp(N + 1) gauge theories, and compare their instanton partition functions with the elliptic genera of 6d self-dual strings.


Introduction
In this paper we study the recently conjectured 5d gauge theory descriptions of 6d SCFTs compactified on a circle [1]. The 6d N = (1, 0) SCFTs have a tensor multiplet and Sp(N ) gauge symmetry with N f = 2N + 8 fundamental hypermulitplets, and these can be Higgsed [2] to the E-string theory [5][6][7][8]. The 5d N = 1 gauge theories have Sp(N + 1) gauge symmetry and N f = 2N +8 fundamental hypermultiplets. The 5d Sp(N +1) gauge theories at N ≥ 1 with N f ≤ 2N + 6 hypermultiplets are known to have non-trivial 5d UV fixed points [3,4]. If N f ≥ 2N + 7, the theories have Landau pole issues, in that the Coulomb branch moduli spaces are incomplete by having strong coupling singularities. So for such theories to have UV fixed points, there should be physical explanations of these singularities. Since the 5d descriptions suggested in [1] have N f = 2N +8 matters beyond the bound of [3,4], it would be desirable to have a better understanding on how this is happening.
In this paper we test these novel 5d-6d dualities by studying the spectrum of instanton solitons. Instantons in the 5d gauge theories play important roles in studying 5d and 6d SCFTs [9][10][11]. In particular, for 5d gauge theories having 6d UV fixed points, instantons are Kaluza-Klein momenta on the compactified circle. Therefore instantons are crucial objects in 5d to understand the 6d physics.
To study instantons, we use the ADHM construction engineered by string theory brane picture. However, since the ADHM construction embeds the instanton quantum mechanics into string theory, it often contains unwanted extra degrees of freedom which are not included in the QFT that one is interested in. So when we compute instanton partition functions via the string theory engineered ADHM partition functions, the extra contribution part should be subtracted to obtain correct QFT instanton partition functions [12]. For

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various models one could separately compute these extra contributions from string theory considerations [12]. Unfortunatley we don't know how to compute these extra contributions for the 5d Sp(N + 1) gauge theories with N f = 2N + 8 hypermultiplets. Nonetheless one can compute one-instaton function exactly. Brane system for the 5d gauge theories have an O7 − -plane, and one-instanton sector is described by the half-D1-brane localized at the O7 − -plane. One expect that there is no extra degrees of freedom in one-instanton sector. See section 2.2 and figure 3.
Instanton partition functions compute the BPS spectrum of instantons bound to Wbosons in the Coulomb phase. Part of 5d W-bosons uplift to 6d self-dual strings wrapping the circle, and instantons are KK momenta on these strings. So one can study the same physics from the elliptic genera of 6d self-dual strings. We compute these elliptic genera, and compared them with the one-instanton partition function of the 5d gauge theories. We find perfect agreements, which provide nontrival supports of the proposal made in [1]. In particular, our test clarifies the physical setting of the 5d-6d dualities, by emphasizing the roles of background Wilson lines, and also by explicitly showing the relations between various 5d and 6d parameters.
This paper is organized as follows. In section 2, we will briefly review the E-string theory and Sp(N ) generalizations. In both cases, it is crucial to consider the effects of background Wilson lines for the flavor symmetries. We compare the E-strings' elliptic genera and the 5d instanton partition functions combined with perturbative index, and show the fugacity map of the two indices. In section 3, we compute elliptic genera for self-dual strings in the 6d SCFT with Sp(1) gauge symmetry and 10 hypermultiplets using 2d gauge theory description. We compare this result with the one-instanton partition functions of the 5d Sp(2) gauge theory with 10 fundamental hypermultiplets. In section 4, we will generalize our result to 6d Sp(N ) gauge theories. We can see that 5d Sp(N + 1) gauge group can be decomposed into the Sp(1) × Sp(N ), and the former Sp(1) gives the 6d self-string structure as E-string theory and the latter Sp(N ) gives 6d gauge group. In section 5, we will conclude with some remarks on the future direction.
First consider type IIA brane description of the 6d N = (1, 0) SCFT with Sp(N ) gauge symmetry and N f = 2N + 8 hypermultiplets. The case with N = 0 engineers the E-string theory. Brane system is given in figure 1 [14,15], and this theory is also known as (D N +4 , D N +4 ) minimal conformal matter theory [16][17][18][19]. We focus on the self dual-strings which couple to the tensor multiplet in the 6d SCFT. The self-dual strings are instanton soliton strings in 6d gauge theory, and it is realized as D2-branes living on D6-branes. The quiver diagram for the 2d N = (0, 4) gauge theory living on D2-branes is given in figure 2. Their SUSY and Lagrangian are studied in [2,13]   and symmetric hypermultiplet come from the strings stretch between D2-D2 branes with appropriate boundary conditions in the presence of O8 − -plane. Hypermultiplets whose representation is (n, 2N ) come from D2-D6 strings, and Fermi multiplets whose representation is (n, 4N + 16) come from D2-D8 strings and D2-D6 strings across NS5 brane. We circle compactify the theory along x 1 direction.

The elliptic genera of self-dual strings
We focus on elliptic genera of the self-dual strings of the 6d Sp(N ) theories where w is the fugacity for the string winding number. The elliptic genus of the 2d gauge theory on a tours is The elliptic genus of the 2d gauge theory (2.2) was studied in [20][21][22], and the E-string case(or O(n) gauge group) was further studied in [2,13]. The elliptic genus is given by an integral over the O(n) flat connections on T 2 . O(n) gauge group has two disconnected parts O(n) ± . So the Wilson lines U 1 , U 2 along the temporal and spatial circle have two disconnected sector. The discrete holonomy sectors for O(n) gauge group on T 2 are listed in section 3 of [13]. Usually elliptic genus is given by sum of 8 discrete sectors for a given n. But n = 1 and n = 2 cases are special, and they are given by sum of 4 and 7 sectors respectively.
The elliptic genus (2.2) is given by [13,21] Z 6d,Sp(N ) 3) The 1-loop determinant for the 2d multiplets are given by where ± ≡ 1 ± 2 2 and r is the rank of the gauge group O(n). η ≡ η(τ ) is the Dedekind eta function and θ i (z) ≡ θ i (τ, z) are the Jacobi theta functions. 'I' refers the disconnected holonomy sectors and u i are zero modes of 2d gauge fields along the torus. |W I | is order of Weyl group of O(n) I for each sector 'I' [13]. For later convenience, we will use following fugacity notation t ≡ e 2πi + , u ≡ e 2πi − , v i ≡ e 2πiα i , y l ≡ e 2πim l . The elliptic genus contains contour integral of u i , which is a residue sum given by Jeffrey-Kirwan residue(JK-residue) prescription [20,21].
The E-string elliptic genus has manifest E 8 global symmetry. One should turn on the E 8 Wilson line on a circle to obtain 5d SYM description of E-string theory [13].

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So it gives following shift of the theta functions where we have (−) sign for i = 1, 4 and (+) sign for i = 2, 3. The overall factor shifts by y 8 q can be absorbed by the redefinition of the string winding fugacity w → wqy −1 8 [13]. We shall observe later that the E 8 Wilson line effect continues to be crucial for the 6d Sp(N ) generalizations of the E-string theory.
One-string. With the effect of E 8 Wilson line, one-string elliptic genus is given by the sum of 4 discrete sectors where Z 1,[I] for I = 1, 2, 3, 4 are given by In order to compare this result with the 5d instanton partition functions, we expand this result in terms of q Two-strings. At n = 2, the elliptic genus is given by the sum of 7 sectors. We skip the details of the calculation here, because we shall see the calculation with Sp(N ) generalizations in section 3. We just report the q-expanded two-strings result in the presence of E 8 Wilson line (2.12)

5d SYM and instanton partition functions
Non-perturbative effect of the 5d gauge theory is essential for the duality. We first consider the general 5d N = 1 Sp(N + 1) gauge theories with N f = 2N + 8 fundamental hypermultiplets. Type IIB brane diagram for N = 1 case is given in figure 3. Instantons are realized by the D1 branes living on the D5 branes. One should carefully use the string theory engineered ADHM construction. It contains unwanted extra degrees of freedoms [12]. For JHEP12(2016)016 O7-D7 0 1 2 3 4 5 6 7 8 9 • -----• --- example, figure 4 shows the brane diagram for Sp(N + 1) gauge theory with N f = 2N + 6 matters at N = 1, which was considered in [3]. In this case D1 branes which can escape to infinity provide extra degrees of freedom. Their contribution to the instanton partition function can be computed separately. To obtain correct instanton partition function, one should subtract this extra contribution from the ADHM quantum mechanical index. However, for 5d Sp(N + 1) gauge theory with N f = 2N + 8 matters, we don't know how to identify the contribution of the extra degrees of freedom to the index. 3 The extra states are supposed to be provided by the D1 branes moving vertically away from the D5 branes. We currently do not have technical controls of such extra states. However one-instanton sector is special, because this sector is realized by the half-D1 brane stuck to O7 − plane. The half-D1 brane can not escape to infinity, so it does not contains any extra degrees. For this reason, we expect that one can study the oneinstanton sector of the general 5d Sp(N + 1) gauge theories with N f = 2N + 8 fundamental hypermultiplets using the ADHM description. 5d index has the perturbative part and the instanton part Z 5d = Z 5d pert Z 5d inst . The 5d Instanton partition functions for the Sp(N + 1) gauge group with matters are wellstudied in [12,23]. As we explained above, naive instanton partition functions can contain unwanted degrees freedom, so one should subtract this factor q is instanton fugacity and k is instanton number. There is no Z extra factor for the oneinstanton sector. Z 5d,Sp(N +1) k is given by  Q, Q † are two of the (0,4) supercharges of the ADHM QM system [12]. J 1 and J 2 are the Cartan generators of SO(4) which rotating the R 4 . J R is the Cartan of SU(2) R R-symmetry. G i and F l are Cartans of Sp(N + 1) gauge group and SO(4N + 16) flavor symmetry group, and their conjugate chemical potentials are α i and m l . We will use the following fugacities If one set k = 2n + χ where χ = 0 or 1, Z ± k is given by where Weyl factor |W | is given by R l denotes the representation of hypermultipet matters. See [12] for the details. 4 Actually Sp(N + 1) gauge theory has Z2 valued θ angle because π4(Sp(N + 1)) = Z2, so its index is given by But in our case, θ is not important. Its effect can be absorbed by redefinition of the flavor chemical potential.

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Vector multiplet part for O(k) + sector is given by and for O(k) − sector is given by for χ = 0. Here and below, repeated ± signs in the argument of the sinh functions mean multiplying all such functions. For instance, (2.21) Fundamental hypermultiplets index contribution for O(k) + sector is given by and for O(k) − sector is given by for χ = 1, and for χ = 0.

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One-instanton: N = 0. One can see that there is no contour integral for one-instanton sector. The one-instanton partition function for Sp(1) gauge group with 8 fundamental matters is given by the sum of Z ± 1 Z 5d,Sp(1) k=1 . (2.25) It shows SO(16) global symmetry.
Perturbative part: N = 0. To obtain full 6d degrees of freedom, we must include the perturebative partition function (1) adj,+ + χ Sp (1) fund,+ χ SO (16) 16 where χ Sp (1) R,+ denotes the Sp(1) character of the representation R, but only sums over positive weights. This is because our index acquires contribution only from quarks, W-bosons, and their superpartners, but not from anti-quarks or anti-W-bosons. We will use this notation throughout the paper. Plethystic exponetial of f (x) is defined by where x collectively denotes all the fugacities. If we expand the 5d index Z 5d = Z 5d pert Z 5d inst in terms of Sp(1) fugacity v, it is exactly same as the E-strings elliptic genera in the sense of double expansion of the instanton fugacity q and the string winding fugacity w. 5 The 5d Coulomb vev fugacity v is identified the 6d string winding number fugacity w, and the instanton fugacity q becomes the string momentum fugacity q. Keeping in mind the 5d-6d fugacity relations and the E 8 Wilson line effect, we will study in the next two sections the 6d Sp(N ) gauge theories and their 5d Sp(N + 1) gauge theory descriptions.

6d SCFT with Sp(1) gauge symmetry
In this section, we will study the circle compactified 6d SCFT with Sp(1) gauge symmetry and its 5d Sp(2) gauge theory description. Both theories have N f = 10 fundamental hypermultiplets. We confirm the duality by comparing the 5d instanton partition function and the elliptic genera of the self-dual strings in the 6d theory. The elliptic genera for the 6d Sp(1) gauge theory are partially studied in [2]. Main difference between [ (20) Wilson line will induce a shift y 8 → y 8 q −2 , while leaving other y l unchanged. Indeed, we will show that the 5d and 6d indices agree with each other after this shift.

6d index
To study full structure of the 6d index, we include not only the instanton soliton strings(or self-dual strings) part but also the 6d perturbative part Z 6d = Z 6d pert Z 6d s.d. . The elliptic genus for self-dual strings is given by where Z 6d,Sp(1) n is given in (2.2). The matter contents of the 2d gauge theory description for the self-dual strings are given in figure 2. We are considering N = 1 case, so there is an additional fundamental hypermultiplet contribution compared to the E-string theory. To compare the 6d index with the 5d index, we will study the q-expanded form of the elliptic genera finally.
One-string. One-string elliptic genus is similar with E-string case where Z 1,[I] are given by again after redefining the string winding fugacity w → wqy −1 8 . The q expansion of this index is given by where f 1 and Z inst 1 are defined by where Z 2,[I] are given by , , for I = 1, . . . , 6. , . (3.12) Finally q-expanded form of the two-string elliptic genus (3.10) is where f 2 (t, u, v, y i ) and Z inst 2 are defined by

(3.23)
Perturbative index. The perturbative index of the theory on a circle is given by where PE is defined in (2.27). First term of the index comes from the 6d W-bosons and second term comes from the 6d fundamental quarks. The background SO (20) Wilson line has no effect on the fields in the SO(20) fundamental representation, and only affects spinor representation. So the perturbative index is unaffected by this Wilson line. In the exponent, we have only kept the contributions from BPS states with positive central charges in the regime q v y ±1 l .

5d index
Everything is same with Sp(1) case. We only increase the gauge group rank by 1 and add two more fundamental hypermultiplets. So the index is generalization of (2.25) and (2.26) (20) fund (y i ) . Here v i are defined below (2.14), and we chose our Sp(2) positive roots by 2e 1 , 2e 2 , e 1 + e 2 and e 2 − e 1 where e 1 and e 2 are orthogonal unit vectors.

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One-instanton. One-instanton partition function is If we set v 1 = v, v 2 = w and expand Z 5d = Z 5d pert Z 5d inst in terms of w, it gives the same result as the 6d index Z 6d . Namely we checked that the w expansion of Z 5d completely argrees with (3.4), (3.13) and (3.22).

Generalization to the 6d SCFTs with Sp(N ) gauge group
In the previous section, we observed that the 6d string winding fugacity w corresponds to one of the fugacities for the 5d Sp(2) gauge symmetry in the instanton partition function. We can generalize this observation. Sp(N + 1) group can be decomposed into Sp(1) × Sp(N ) ⊂ Sp(N + 1). We expect that the former Sp(1) ∼ SU(2) is responsible for the string winding fugacity, and the latter Sp(N ) gives the 6d gauge symmetry. We will confirm this assertion by comparing the 5d and 6d indices. The 5d index for Sp(N + 1) gauge group and N f = 2N + 8 fundamental hypermultiplets is given by

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Then the perturbative index becomes Z 5d,Sp(N +1) pert where we only keep positive weights(roots) in the plethystic exponential. We can expand the instanton partition function in terms of w Z 5d,Sp(N +1) k=1 (4.5) Now we will compare this with the 6d index. Note that the first line of (4.4) is already same as the 6d perturbative index, so w 0 q 0 orders clearly agree with each other.
One-string. Now we compare the 5d-6d results at w 1 q 0 and w 1 q 1 orders. One-string elliptic genus has following form Z 6d,Sp(N ) n=1 where Z 1,[I] are given by After making q expansion of Z 1,[I] , and after replacing all chemical potential by z → iz 2π (where z denotes 1,2 , α i , m l ), one obtains

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We do not write explicit form of F (m l , α i , i ) which is the coefficient of q in Z 1, [3] and Z 1, [4] , because they are canceled after summation. Then w 1 q 0 term in (4.6) agrees with (4.4). Also we have checked that w 1 q 1 term agrees with the corresponding order of Z 5d .
Two-strings. We compare the 5d-6d results at w 2 q 0 and w 2 q 1 orders. Two-string elliptic genus is given by , , (4.12) where discrete sector I is same as (3.21). There are additional poles from symmetric hypermultiplets, which are given by u * = − + ± α i for all i. Now we can obtain general form of two-strings elliptic genus.

Conclusion
We studied the 6d SCFTs compactified on a circle with Sp(N ) gauge symmetry and N f = 2N + 8 fundamental hypermultiplets. In particular, we tested the 5d Sp(N + 1) gauge theory descriptions of the 6d theories. We compared the Witten indices of the 5d and 6d theories. For the 5d instanton partition function, the usual ADHM construction contains unwanted string theory degrees except in the one-instanton sector. We observe perfect agreement of the two indices in double expansion of the string winding fugacity w and the instanton fugacity q up to w 3 q 1 order. As usual, the 5d instanton charge is mapped to the 6d KK momentum mode. The 5d Sp(N + 1) gauge group is decomposed into the Sp(1) × Sp(N ), and the former Sp(1) charge is mapped the 6d self-dual string winding number. The fugacities for the latter 5d Sp(N ) gauge symmetry and SO(4N + 16) flavor symmetry are mapped to the 6d Sp(N ) gauge symmetry and SO(4N +16) flavor symmetry.
We have also observed that the background SO(4N + 16) Wilson line plays crucial roles in these 5d-6d dualities, similar to the E 8 Wilson line in the E-string theory. These results provide the detailed rules of the dualities proposed by [1].
The natural question is what happens if we naively compute higher instanton partition functions using (2.15). Our naive computation shows disagreements with the result predicted by the ellipitic genus of self-dual strings. Difference between two results must comes from the extra degrees in the string engineered ADHM construction. We hope this result gives the better understanding of the extra degrees in the brane system.
We can also try to check the duality between 5d gauge theory with Sp(2) and SU(3) gauge groups, each having 10 fundamental hypermulitplets [9,10,25,26]. The SU(3) gauge theory is also conjectured to uplift to the same 6d Sp(1) SCFT on a circle. Although the string theory engineered ADHM construction of the SU(3) gauge theories have extra degrees too, we can detour this problem by introducing anti-symmetric hypermultiplets. Antisymmetric representation is same as (anti-)fundamental representation in SU(3) group. So the 5d SU(3) gauge theory with 10 fundamental hypermultiplets can be regarded as the gauge theory with 8 fundamental and 2 anti-symmetric hypermultiplets. This trivial change of viewpoint affects the details of the ADHM construction. Such alternative ADHM descriptions are sometimes shown to provide more useful description of instantons [26]. It is interesting to see if their ideas apply to our system.