Brane webs and O5-planes

We explore the properties of five-dimensional supersymmetric gauge theories living on 5-brane webs in orientifold 5-plane backgrounds. This allows constructing quiver gauge theories with alternating USp(2N) and SO(N) gauge groups with fundamental matter, and thus leads to the existence of new 5d fixed point theories. The web description can be further used to study non-perturbative phenomena such as enhancement of symmetry and duality. We further suggest that one can use these systems to engineer 5d SO group with spinor matter. We present evidence for this claim.


Introduction
Gauge theories in 5d are non-renormalizable and thus are not expected to exist as microscopic theories. For example, maximally supersymmetric Yang-Mills theory is believed to flow to the 6d (2, 0) theory in the UV [1,2], so the microscopic theory is actually 6d. Nevertheless, there is a lot of evidence that in the N = 1 supersymmetic case, corresponding to 8 supercharges, an interacting UV fixed point may exist making the theory UV complete [3][4][5]. The gauge theory can then be realized as the IR limit of such a SCFT under a mass deformation, corresponding to the inverse gauge coupling square which has dimension of mass in 5d. An interesting question then is how can we study these 5d SCFT's. One way is to embed them in string theory. A convenient embedding is given by 5-brane webs in type II B string theory [6,7]. This realizes the 5d SCFT as an intersection of 5-branes at a point. The moduli and mass parameters of the SCFT are then realized as motions of the internal and external 5-branes respectively. In particular, the 5d SCFT may posses a deformation leading to a low-energy gauge theory.
Thus, 5-brane webs can be used to study various properties of these theories. First of all they give support for the existence of fixed points for various gauge theories. Not JHEP03(2016)109 every 5d gauge theory flows to a 5d SCFT, and the demand that such a SCFT exists is expected to constrain the matter content of the theory. If a gauge theory can be realized as the IR theory in a brane web then this strongly suggests that it flows to a UV fixed point described by the collapsed web. Therefore, brane webs can be used to study the conditions for the existence of fixed points.
Another useful application of brane webs is to study 5d dualities. A single SCFT may have more than one gauge theory deformation, in which case these different IR gauge theories are said to be dual. This is somewhat similar to Seiberg duality in 4d, except that in this case there are several different IR gauge theories all going to the same UV SCFT. This is nicely realized in brane webs, where a SCFT can be deformed in different ways leading to different IR gauge theories [6]. This usually involves an SL(2, Z) transformation in the brane web. Thus, brane webs provide a useful way to motivate these kind of dualities.
Brane webs can also be used to study symmetry enhancement in 5d gauge theories [13,14]. They can be used to calculate the 5d superconformal index of a SCFT using the methods of topological strings [15]. Even when calculating the 5d superconformal index for a gauge theory using localization [16], brane webs are very useful for evaluating the instanton contribution [9,17,18]. They can also realize 5d versions of A type class S theories [19], and thus can be used to study them, and there are many other applications.
The purpose of this article is to study brane webs in the presence of an orientifold 5plane. First, this allows constructing SO(N ) and USp(2N ) gauge theories with fundamental matter, as first done in [20]. This can then be used to study these gauge theories. These systems can also be realized using an orientifold 7-planes, as done in [12], and our results agree with their finds.
More interestingly we can use this to realize more elaborate theories. First, we can realize a linear quiver of alternating SO and USp groups connected by half-bifundamentals. This then provides evidence that these theories exist as fixed points, and allows us to study some of their properties. Second, a subset of these theories are closely related to quivers of SU group in the shape of the Dynkin diagram of type D (henceforward referred to as D shaped quiver), so these methods can be used to study these theories as well. We also argue that these can even be used to engineer SO(N ) gauge theories with spinor matter for N ≤ 12.
The structure of this article is as follows. Section 2 introduces the general construction in the more simplified case realizing a single gauge group. In section 3 we consider the general case giving a linear quiver with alternating SO and USp groups. We also consider the S-dual system leading to a D shaped quiver of SU gauge groups. Section 4 deals with describing SO gauge groups with spinor matter. We end with some conclusions. The appendix provides a short review of index calculations and instanton counting.

The general construction
The starting point is the ordinary brane webs used to describe N = 1 supersymmetric SU groups and their quivers [6,7]. The supersymmetry permits adding an O5-plane parallel JHEP03(2016)109 to the D5-branes. This should lead to orthogonal or sympletic groups and their quivers (such a system was previously considered in [20]). Specifically, the construction involves an O5-plane with several parallel D5-brane crossed by NS5-branes. The orientifold enforces an orbifolding on the transverse coordinates which must be respected by the web.
Next, we wish to recall several properties of O5-planes that will play an important role in what follows. There are 4 different variants of O5-planes denoted as O5 + , O5 − ,Õ5 − andÕ5 + [21]. Putting N D5-branes on top of an O5 + ,Õ5 + results in a USp(2N ) gauge theory on them while putting them on top of an O5 − results in an SO(2N ) gauge group. TheÕ5 − is an O5 − plane with a stuck D5-brane and so putting N D5-branes on top of it results in an SO(2N + 1) group. The O5-planes carry D5-brane charge: the O5 + andÕ5 + carry charge +1, the O5 − carries charge −1 and theÕ5 − carries charge − 1 2 . When a stuck NS5-brane crosses the O5-plane, in a way preserving N = 1 supersymmetry, it partitions the O5-plane into two parts of differing types: O5 + (Õ5 + ) changes to O5 − (Õ5 − ). Likewise a stuck D7-brane also has a similar effect, now changing an O5 + (O5 − ) into anÕ5 and vice versa. The change in the type of O5-plane when crossing an NS5-brane has important implications once quantum effects are taken into account. For example, let's consider a system consisting of an O5 + with a stuck NS5-brane that changes it to an O5 − . Because of the type change, there is a jump in the D5-brane charge across the NS5-brane which should cause the NS5-brane to bend. Then taking into account charge conservation, sypersymmetry and invariance under the orbifolding, one concludes that the correct configuration should be a (2, −1)-brane crossing the O5-plane and becoming an (2, 1)-brane. This is exhibited in figure 1.
Next we explore the implications for the simplest cases of N D5-branes stretched between two NS5-branes in the presence of one of the O5-plane types.

O5 + and USp groups
The classical picture consists of an O5 + -plane with N D5-branes suspended between two stuck NS5-branes resulting in a USp(2N ) gauge theory. Taking into account the bending caused by the D5-branes and the O5-plane results in the web shown in figure 2. It is now straightforward to generalize to cases with fundamental flavor by adding (1, 0) 7-JHEP03(2016)109 branes on top of the D5-branes. These can then be pulled through the external 5-branes, accompanied by Hanany-Witten transitions resulting in webs with semi-infinte external D5-branes. Examples of these are shown in figure 3. Note that the gauge symmetry on N f external D5-branes is SO(2N f ), since these sit on top of an O5 − , which is the correct global symmetry of USp(2N ) + N f F . These webs can now be used to study a variety of issues in 5d gauge theories, notably, the existence of fixed point, identifying decoupled states in index calculations and motivating dualities. Such a thing was done for a different realization of this theory using O7-planes in [12]. One can see that the webs in the reduced space in these systems are similar to the ones, in the reduced space, with the O5 + -plane. Thus, most of the results found using the construction with the O7-plane are also true in this case, and we will not repeat them.
We do wish to discuss the manifestation of the Higgs branch in this web, as this is different from the O7-plane construction. In brane webs, the Higgs branch consists of all the possible motions of the 5-branes along the 7-branes. Uniquely for 5d, at the fixed point there can be additional Higgs branch directions besides the ones visible in the perturbative gauge theory [22]. Figure 4 (a) illustrates an example of this for the case of the E 1 theory: the fixed point has a one dimensional Higgs branch corresponding to separating the (1, 1) 5-brane from the (1, −1) 5-brane. This theory can also be constructed using an O5 + -plane, as shown in figure 4 (c). This also exhibits the 1-dimensional Higgs branch, now given by pulling the (3, 1) and (3, −1) 5-branes out of the O5-plane.
The addition of fundamental flavor is done by adding (1, 0) 7-branes, which we pull out, resulting in N f semi-infinte D5-branes all in the same direction, as shown in figure 5 (a). To enter the Higgs branch we go to the origin of the Coulomb branch and set the masses of the JHEP03(2016)109 Figure 4. (a) The brane web for SU 0 (2), also known as the E 1 theory, at a generic coupling and at a generic point on the Coulomb branch (on the left), and at the origin of the Coulomb branch and taking the bare coupling to infinity (on the right), describing the fixed point. We have also explicitly drawn the 7-branes, shown as black circles. These span the 8 directions coming out of the picture. (b) The brane web for SU π (2), also known as theẼ 1 theory. The web on the left is for a generic coupling and at a generic point on the Coulomb branch, and the the web on the right is at the origin of the Coulomb branch and taking the bare coupling to infinity. One note that there is no Higgs branch in this case. (c) The web of figure 2 (a) at the origin of the Coulomb branch and infinite coupling constant. flavors to zero by coalescing all the D5-branes on the O5-plane. Furthermore, we separate the D7-branes along the O5 − -plane. When the O5 − -plane is crossed by a D7-brane it changes into anÕ5 − which is an O5 − -plane with a stuck D5-brane. We thus conclude that upon each crossing one 5-brane must end on a D7-brane resulting in the picture shown in figure 5 (b).
The Higgs branch now consists of breaking the 5-branes on the 7-branes as shown in figure 5 (c). The possible breakings are limited by the S-rule, which necessitates that at most one 5-brane can be stretched between any given NS5-brane and D7-brane. When JHEP03(2016)109  Finally we take the fixed point limit by collapsing the gauge D5-branes. In this limit additional directions become available. First there is the 1 dimension given by detaching the 5-branes from the O5-plane, similarly to the one in the E 1 theory. This exists for any number of flavors. When N f > 2N there are further additional directions. It appears that when the NS5-branes touch, a D7-brane can always be connected to the other NS5-brane. This eases the constraints imposed by the S-rule and allows additional directions. As we shall soon show this is necessary in order to recover the correct Higgs branch dimensions of known theories, like the rank 1 E 6 theory. When N f = 2N + 4 the two external NS5branes become parallel and there is an additional direction given by breaking one of them on a (0, 1) 7-brane. Finally, when N f = 2N + 5 there are intersecting external legs, where resolving the interaction leads to one of these external legs becoming a D5-brane due to passing thorough the monodromy of the other (see [12] for the details). At the fixed point, one can then also break this D5-brane on the 7-branes leading to additional directions.
We can count the dimension of the Higgs branch for these theories and compare it with the one found using a different realization of these theories, for example using ordinary webs, finding complete agreement. As an example, consider SU(2) with five flavors, the rank 1 E 6 theory. As shown in figure 6 (a) the perturbative Higgs branch is 7 dimensional, which is indeed the gauge theory result. An important limitation here is that there are only two gauge D5-branes so only two D7-branes can be connected to the other NS5-brane. This makes the constraint imposed by the S-rule more stringent. We have argued that this constraint should be relaxed at the fixed point, where the two NS5-branes coalesce. Indeed, without this constraint we would get a 10 dimensional Higgs branch, as can be seen by comparing with the perturbative component of the Higgs branch for a different theory with the same number of flavors but with 2N > N f like the USp(6) + 5F theory in figure 6 (b). Thus, the non-perturbative Higgs branch has 10 + 1 = 11 (remember there JHEP03(2016)109 Figure 6. (a) The web at a generic point in the Higgs branch for USp(2) + 5F . The numbers next to the O5-plane represent the number of D5-branes stuck on it. The Higgs branch is given by detaching a D5-branes and its image from the O5-plane. One can see that the Higgs branch is 7 dimensional (quaternionic) in accordance with the gauge theory result. (b) The web at a generic point in the Higgs branch for USp(6) + 5F . The Higgs branch for this theory is 10 dimensional, again in accordance with the gauge theory result. Note that this differs from the case of (a) only by the number of color branes which is large enough so that every D7-brane can be connected to the other NS5-brane.

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is an additional direction given by taking the web off the O5-plane) which is indeed the Higgs branch dimension of the rank 1 E 6 theory. Similarly, one also get from the web the correct dimensions of both the perturbative and non-perturbative Higgs branches for the E 7 and E 8 theories.

O5 − and SO groups
Changing the O5 + to an O5 − leads to an SO(2N ) gauge theory, an example of which is shown in figure 7. The major difference in the web is that the bending caused by the O5-plane is in the opposite direction. This results in different bounds for fixed points, so for example one cannot draw a web for pure SO(2), while one existed for the O5 + case, pure USp(2). This is in accordance with the expected UV incompleteness of 5d U(1) gauge theories. The generalization by the addition of fundamental (in the vector representation) flavors is straightforward, examples shown in figure 8. Now, the flavor D5-branes sit on top of an O5 + -plane resulting in a USp(2N f ) global symmetry again in accordance with the gauge theory expectation.
An alternative realization of SO(2N ) + N f F using an O7-plane also exists, and again the reduced space webs of these two constructions are similar. Thus, all the results seen from that construction are also valid in this one and we will not repeat them here. We do wish to describe the manifestation of the Higgs branch in this case. In the pure case, exactly as in the O5 + case, one finds a 1-dimensional Higgs branch that opens at the fixed point. This agrees with the results seen also from the O7-plane constructions as well as other constructions when these are available (such as pure SO(6) = SU(4)).  . Separating a D7-brane and its image across an O5 − -plane, and then moving them past the (2, 1) 5-brane. This leads to the configuration identical to separating a D7-brane and its image, each with a D5-brane ending on it, across an O5 + -plane.

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Next we discuss the generalization when flavors are present, starting with the case of one flavor. We can again go to the origin of the Coulomb branch and the limit of zero mass. The major difference from the USp case is encountered when separating a 7-brane from it's mirror image, since now there is anÕ5 + between them. One cannot have a stuck D5-brane on anÕ5 + , so we conclude that when separating the 7-branes the two D5-branes must end on the same 7-brane. 1 The resulting construction is shown in figure 9. The implication of this is that now there is a 1-dimensional Higgs branch where the gauge theory is broken to SO(2N − 1), in accordance with the gauge theory expectation. The generalization to more than one flavor is now straightforward. There are now 2N f 7-branes stuck on the O5-plane which come in alternating pairs with one with no 5-branes ending on it and the other with two 5-branes ending on it. Breaking the 5-branes on the 7-branes, while taking due care of the S-rule, correctly reproduces the breaking pattern and the dimension of the Higgs branch as expected from the gauge theory.
Finally, we take the fixed point limit and consider non-perturbative Higgs branch directions. Like in the USp case, there is always the direction given by separating the JHEP03(2016)109

2.3Õ5
Finally we want to consider the case of anÕ5 plane. At first one encounters a problem with the fractional NS5-brane on it. This leads to a change between anÕ5 + and anÕ5 − , resulting in a jump in the D5-brane charge. However this jump is now fractional, and it does not appear to be possible to reconcile the bending required by charge conservation with the reflection symmetry implied by the orientifold. One approach to realizing these theories, in the case of anÕ5 − , is to use the construction for SO(2N +2)+1F and go on the Higgs branch leading to SO(2N + 1). An example of this is shown in figure 11. We can now transform to a description with anÕ5 − by moving the stuck D7-brane though the external 5-branes to the other end of the O5-plane, while taking due care of the monodromy of the 7-brane. Now, the resolution of the above issue is clear: there is also a half monodromy on the O5-plane which corrects the bending so as to be consistent with the orbifolding.
One can now use this construction to realize SO(2N + 1) + N f F gauge theories. Once again the reduced space web matches the one using an O7-plane and the results found from this description also apply to this case. The Higgs branch is realized exactly as in the SO(2N ) case.
Finally, we can inquire about the web with anÕ5 + . A natural guess is that this describes the USp theory with θ = π. 2 Indeed, we expect such theories to exist yet there are no discrete choices in the web save for this. Furthermore, such a thing occurs for example in the construction of the maximally supersymmetric 5d USp(2N ) gauge theory using O4-planes [23,24]. However, the web for USp(2N ) using anÕ5 + , an example of which is shown in figure 12, appears to be identical to USp(2N ) + 1F and does not describe a new theory. Thus, it appears that there is no difference between using an O5 + and anÕ5 + .
JHEP03(2016)109   (6) where a half-bifundamental is understood to exist whenever an × is used between an SO and USp groups.
As a result, there does not appear to be a way to describe USp π (2N ) with an O5-plane. One can set out to get such a web by starting with the E 2 web and giving a mass to a flavor. Then depending on the mass sign one gets either the E 1 orẼ 1 theories. This indeed works for ordinary webs and ones with an O7-plane, but not for this case. The problem is that in this case the flavor can only be integrated in one direction. It is interesting whether there is a fundamental reason why θ = π cannot be accommodated in this construction, or alternatively if it is possible to incorporate it in the web in a more intricate way.

SO × USp quivers
So far we considered a system with just two external NS5-branes. The web can be generalized to an arbitrary number of such branes which leads to a long quiver with alternating SO and USp groups connected by half-hypers in the bifundamental representation. Two examples of this are shown in figures 13 and 14. The quiver can contain both SO(2N ) and SO(2N + 1) gauge groups which can be achieved by adding a stuck D7-brane. This can also lead to an half-hyper in the fundamental for USp(2N ) which appears in the web as a stuck D7-brane or a stuck external D5-brane. Note that due to a global gauge anomaly, the 5d version of [25], a USp(2N ) gauge theory must have an even number of fundamental half-hypers [5]. This is indeed respected by the web.
These webs have several interesting implications. First, they point to the existence of fixed point theories for these quiver theories. This can also be generalized by adding flavors and the web can be used to argue the limit beyond which a fixed point does not exist. The web can also be used to study the Higgs branch, both the perturbative component and the non-perturbative component, as in the previous examples. It can also be used to identify decoupled states in index calculations using the SO × USp formalism, as done for other systems in [9,12,17,18]. Figure 14. The web for 3HF + USp(2) × SO(7) × USp(2) + 1HF where HF stands for a halffundamental. Note that the total number of half-fundamentals is even for each USp(2) so there is no gauge anomaly.

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Yet another application is to study symmetry enhancement in such theories. In brane webs this is manifested by some of the external legs becoming parallel. For example, consider a linear quiver consisting of n G groups of ranks N i , for i = 1, 2 . . . , n G , with F i fundamental hypers under the i'th group. By inspecting the D5-charges of the NS5-charge carrying external branes, one can see that these are neither parallel nor intersecting as long where the + sign is for USp groups and the − sign is for SO groups, and we take for some series of adjacent groups then a group of NS5-charge carrying external branes become parallel, signaling an enhancement of the topological symmetries associated with these groups. In particular, if all the groups obey then all these external branes become parallel, suggesting an enhancement of U(1) n G → SU(n G + 1) (see figure 15 (a) for an example). If occures for one of the groups then the NS5-charge carrying external branes associated with that group intersect (see figure 15 (b) for an example). The intersecting branes can be continued past one another accompanied with a Hanany-Witten transition. If this process terminates after a finite number of such transitions then this 5d gauge theory go to a 5d fixed point described by the collapsed web (see figure 15 (c) for an example). One can now use this brane web to try and read the global symmetry of the fixed point theory.
For example, consider the previously considered class of theories, where every group Say we now add one more flavor to one of the edge groups, say for i = 1. As seen in figure 15 (b), this leads to a configuration with the leftmost NS5charge carrying external brane intersecting the n G other NS5-charge carrying branes. This can be resolved by continuing them past one another, accompanied with a Hanany-Witten transition, leading to a configuration with no intersection (see figure 15 (c) for an example) so we conclude that this class of theories go to a 5d fixed point. Inspecting the web one sees that this configuration as F 1 + n G D5-branes on the left side and F n G D5-branes on the right side. Thus, we conclude that in this case there should be an enhancement of U(1) n G × SO(2F 1 ) → SO(2F 1 + 2n G ) or U(1) n G × USp(2F 1 ) → USp(2F 1 + 2n G ) depending on whether the i = 1 group is of type USp or SO respectively.
In the rest of this section we concentrate on one further application which is motivating 5d dualities. These are manifested by a different gauge theory description, of the same web, generically in a different SL(2, Z) frame. We can first start by generalizing the dualities of [12] also to the quiver case. As a simple example consider the web shown in figure 16 JHEP03(2016)109

S-duality and O5 0 -plane
In order to make further progress one must do an SL(2, Z) transformation on the entire system, including the O5-plane. This requires understanding the behavior of the O5-plane under these transformations, in particular S-duality. There is one case where this is actually known which is an O5 − -plane with a full D5-brane. In that case the total D5-brane charge of the system is zero, and its strong coupling behavior is of the perturbative orbifold R 4 /Z 2 , the Z 2 being a reflection in the four directions combined with (−1) F L [21,26]. Thus, in this case we might be able to say something explicit about the S-dual theory.
The simplest thing to start with is an O5 − -plane with N parallel D5-branes crossed by 2k NS5-branes, where an even number is necessary so that asymptotically we still have an O5 − -plane so that we can apply S-duality. Doing S-duality on this configuration results in the web shown in figure 18 (b). This clearly shows a long SU(2k) linear quiver where at its end there are the branes connecting the NS5-brane with the orbifold fixed plane. The gauge theory existing on such a system is known to be an SU(n 1 ) × SU(n 2 ) gauge theory with n 1 + n 2 = 2k. The numbers n 1 , n 2 arise as there are two different types of 5-branes ending on the orbifold fixed plane differing by their charge under the twisted field living at the fixed plane. In the present case, one can see an SU(k) × SU(k) gauge theory. The matter content supplied by the crossed NS5-brane is a bifundamental hyper between each SU(k) and the adjacent SU(2k) so we conclude the duality shown in figure 19. The Chern-Simons levels are all 0 as the web is invariant under reflection which is the brane web analogue of charge conjugation in the gauge theory.
One can now inquire whether we can find additional evidence for this duality. First, we can do several simple checks such as comparing the dimension of the Coulomb branch and the number of mass parameters. A short counting shows that they are equal. Matching the global symmetries is harder as not all are classically apparent. The theory with the O5 − plane classically has an U(1) 2k−1 × SO(2N ) 2 which, as suggested by the web, is enhanced to SO(2N ) 2 × SU(2k). However, on the dual side, the classical global symmetry is U(1) 2N × SU(2k), which the duality suggests should enhance to SO(2N ) 2 × SU(2k). Indeed this is supported by the instanton analysis of [27,28].
Both theories also have discrete global symmetries. The D-shaped quiver theory has a Z 2 × Z 2 symmetry given by charge conjugation and exchanging the two SU(k) groups. The SO × USp quiver theory as a Z 2 reflection symmetry, which the web suggests matches charge conjugation in the dual theory. The duality suggests that there should be another JHEP03(2016)109  Z 2 that matches the exchange of the two SU(k) groups. There is indeed an extra Z 2 on the SO × USp quiver theory, exchanging the two spinor representations of all the SO groups. We expect this to match the exchange of the two SU(k) groups. Note that this operation on the Dynkin diagram of type D indeed corresponds to exchanging the two spinor representations. This matches similar results in the linear A type quiver [9].
Another check that can be done on this duality is comparing their superconformal indices (see the appendix for a review of the 5d superconformal index). As a starting point we can take the simplest example illustrated in figure    theory as an SU(4) 3 global symmetry where one is visible perturbativly and the others are brought by instantonic enhancement. Indeed by an index calculation we verified that such an enhancement is present.
Unfortunately, calculating all of these contributions is technically demanding so it is worthwhile to look at a simpler example. Particularly, we can consider integrating out flavors so as to reduce the degree of enhancement. This is done by taking an external D5-branes to infinity. Note that for the two edge flavors this is identical to pulling an NS5-brane to infinity, and thus to also integrating out a flavor in the dual theory. Thus, we arrive at the duality shown in figure 21 which is the one we shall check using the superconformal index.
The theory on the right of figure 21 is SU(2)×SU(4)×SU(2) gauge theory with 2 flavors for the SU(4). The classical global symmetry is SU(2) × U(1) 6 . The fugacity allocation is shown in figure 22. We work to order x 5 which requires the contributions of the (1,0,0) JHEP03(2016)109 where we have only displayed terms up to order x 3 even though the calculation was done up to order x 5 .
From the x 2 terms we see that the (0,1,0) instantons bring about an enhancement of U(1) → SU(2) so that the quantum symmetry is SU(2) 5 ×U(1) 2 in accordance with the dual JHEP03(2016)109 theory. Further comparing the two we find that taking: t render the two equal. From the matching we see that the enhanced SU(2) global symmetry of the SO × USp quiver matches the perturbative SU(2) global symmetry of the D shaped quiver theory and vice versa, as expected from the web.
The index also makes manifest the Z 2 × Z 2 global symmetry. It acts on the theory by permutating the 4 SU(2) global symmetry groups, perturbativly realized in the SO × USp quiver, similar to its action on the 4 vertices of a rectangle whose symmetry group is also Z 2 × Z 2 . The matching of fugacities is consistent with charge conjugation of the D-shaped quiver mapped to reflecting the SO × USp quiver, while exchanging the two SU(2) groups is mapped to charge conjugation of the SO × USp quiver (which exchanges the two spinor representations of SO (6)).
The index can be written in characters of the SU(2) 5 × U(1) 2 global symmetry where it reads:

Spinor matter
In this section we discuss the addition of matter in a spinor representation of an SO gauge group. It is well known that there is no perturbative way to add matter in spinor representations through D-brane constructions in string theory. However, we claim that there is a way to do so for webs in the presence of O5-planes, in a non perturbative manner. We first present our conjecture for how this is done, and present our argument for why this gives spinor matter. We then proceed to give evidence for this conjecture. We claim that the configuration shown in figure 24, in which we add a stuck NS5brane to an SO(2N ) gauge theory, corresponds to adding a single hyper in the spinor representation of that group. Our motivation for this is as follows. First, consider the system in figure 25, describing an 1F +SU(2)×SO(2N +2)+1F gauge theory. Starting from this system, we can get to the the one in figure 24 by going on the Higgs branch described in the web by separating a full D5-brane. In the gauge theory this describes giving a vev to the operator qBQ where q is the SU(2) fundamental, B the half bifundamental, and Q the vector of SO(2N + 2).
Perturbativly, this completely breaks the SU(2) gauge group. However, the web suggests that in this limit we do remain with additional degrees of freedom. Thus, these can only come from instantons of the SU(2). It is well known that the 1 instanton of SU (2) with N f flavors carries charges in the spinor representation of SO(2N f ). Therefore, we conjecture that the remaining state can be described by an hypermultiplet in the spinor of SO(2N ) whose origin is non-perturbative in the brane web. Although we have used SO(2N ) in this example, the same reasoning can also be carried out for the SO(2N + 1) case.
Before giving support for our claim, we wish to state some further implications of it. First, we can consider what happens when we attach further D5-branes as shown in figure 26. We can answer this question by again starting with the system of figure 25 where adding the D5-brane corresponds to adding a flavor for the SU(2). The instanton is again in the spinor of SO(2N f ) which decomposes to two spinors of opposite chirality under SO (2N f − 2). We thus conclude that we now get two hypermultiplets both spinors of SO(2N ), but of opposite chirality. Finally, we wish to consider what happens if we JHEP03(2016)109 Figure 26. The matter contribution associated with a single stuck NS5-brane found using the preceding argument. similarly add a (2, 1) 5-brane in the other direction. Particularly, we still expect a spinor hyper, but we inquire whether it has the same chirality or not as it opposing friend. We can answer this by considering the appropriate equivalence of the system in 25, where the spinor should appear as the instanton of the SU(2) gauge group. The chirality of this spinor is determined by the SU(2) θ angle, and as this is identical in the two constructions, we conclude that the two spinors have the same chirality. To change the chirality between the two spinors, one would have to switch the θ angles of one of the SU(2)'s. As previously mentioned, we do not know if this can be done.
We can now proceed to give evidence for our conjecture. First, we look at the Higgs branch. In figures 27 and 28 we show the webs for a variety of SO groups with two spinors of the same chirality. These theories then have a Higgs branch breaking them to an SU group. We show that the web correctly reproduces this branch, giving the expected theory. Furthermore, this branch can only be accessed when the spinor is effectively massless which in the web corresponds to the point where the would be SU(2) instanton is massless as expected from our interpretation.
Note that we are essentially limited by the requirement that the would be SU(2) gauge group sees less than 8 flavors. Naively, this would imply the we cannot get spinors of SO(N ) for N > 10. However, we can by a slight generalization get one also for N = 11, 12. In these theories, the spinors are pseudo-real, so a half-hyper is possible. Figure 29 shows the webs we conjecture for SO (11) and SO(12) with one half or full hyper in the spinor representation. One can see that the Higgs branch of these webs agrees with what expected from the gauge theory. One issue with the webs for the full spinor cases is that they have only one mass deformation, in contrary to the two expected from the gauge theory. This is reminiscent of the web for USp(2N ) + AS which also has just one mass deformation. In that case the web is for a massless antisymmetric. Likewise this web appears to have a massless spinor.
Using these webs we can look at the existence of fixed points for SO groups with both vector and spinor matter. First, holding the spinor matter fixed, we can use the web to determine what is the maximal number of vectors one can add while still having a 5d fixed point. We generally find agreement with the expectations from [29].
We can also ask what this implies about the limit of spinor matter. As mentioned, we are limited by the requirement that the would be SU(2) gauge group sees less than 8 flavors. Yet, we argue that this does not represent a limitation on spinor matter for SO gauge theories, rather a breakdown of the interpretation of these webs. A limitation on JHEP03(2016)109 Figure 27. Several examples of the Higgs branch for theories of the form SO(2N ) + 2S for N = 3, 4, 5. Starting from the initial web on the right, we take the massless spinor limit, corresponding to taking the distance between the two pairs of NS5-branes to zero. Then a Higgs branch opens up given in the web by detaching the web from the orientifold. This is shown on the right where for ease of presentation we have shown only half the web. (a) The case of N = 3. We know from the gauge theory that there is a Higgs branch breaking the theory to SU(3). (b) The case of N = 4. We know from the gauge theory that there is a Higgs branch breaking the theory to SU(4). (c) The case of N = 5. We know from the gauge theory that there is a Higgs branch breaking the theory to SU(5) + 2F . In all 3 cases the Higgs branch is correctly reproduced in the web. the matter content due to a lack of 5d fixed point manifests as a lack of a brane web when taking the Yang-Mills coupling to infinity, generally due to intersecting legs that cannot be resolved by a finite number of HW transitions. This is not the case here, rather the intersection arises when we take the massless spinor limit indicating that there are in fact additional states in this case. Therefore, we do not think this gives a limit on spinor matter for SO gauge theories, rather being a limitation of the method.

Dualities
As our final piece of evidence, we examine dualities between systems involving SO groups with spinor matter. The idea is to use the webs to motivate dualities and then test them using the superconformal index. This then provides independent evidence for the duality and thus also for the original identification leading to it. There is one limitation in this test as instanton counting for SO groups with spinor matter is currently unknown. Thus, we are limited to comparing the perturbative parts. JHEP03(2016)109 Figure 28. Several examples of the Higgs branch for theories of the form SO(2N + 1) + 2S for N = 2, 3, 4. Starting from the initial web on the right, we take the massless spinor limit, corresponding to taking the distance between the two pairs of NS5-branes to zero. Then a Higgs branch opens up given in the web by detaching the web from the orientifold. This is shown on the right where for ease of presentation we have shown only half the web. (a) The case of N = 2. We know from the gauge theory that there is a Higgs branch breaking the theory to SU(2). (b) The case of N = 3. We know from the gauge theory that there is a Higgs branch breaking the theory to SU(3). (c) The case of N = 4. We know from the gauge theory that there is a Higgs branch breaking the theory to SU(4) + 2F . In all 3 cases the Higgs branch is correctly reproduced in the web. The S-dual of the web in (a). It describes an SU 0 (2) × USp π (4) × SU 0 (2) gauge theory. The USp π (4) group can be seen by pulling the (1, 1) and (1, −1) 7-branes through the 5-branes, and merging them to an O7 − plane (see [12]).

Example 1
As our first example, consider the theory shown in figure 30 (a). From figure 26, we claim that this describes an SO(8)+2S +2C gauge theory where we use S and C for the two Weyl spinor representations of SO (8). We can take the S-dual description leading, as shown in figure 30 (b), to the quiver theory SU(2) × USp(4) × SU(2). Thus we conjecture that these two theories are dual. We want to also check this using the superconformal index.
We start with the SO(8) theory. The classical global symmetry is U(1) × USp(4) 2 coming from the topological and flavor symmetries. There is also a Z 2 discrete symmetry coming from exchanging the two spinor representations. The analysis of [29] suggests that there is no enhanced symmetry so it seems to also be the quantum symmetry.
We preform the calculation up to order x 5 finding: where we use χ[d 1 , d 2 ] for the representation of dimension d 1 (d 2 ) under the first (second) USp(4) symmetry. Since USp(4) has two 35 dimensional representations, both appearing in the index, we have also written their Cartan weight to distinguish between them. Note that the index is symmetric under the exchange of the two global USp(4)'s which is the manifestation of the discrete Z 2 symmetry. Next we move to the SU 0 (2)×USp π (4)×SU 0 (2) theory. The classical global symmetry is U(1) 3 × SU(2) 2 , but as we will show this is enhanced at least to U(1) × USp(4) 2 by the JHEP03(2016)109 Figure 32. The fugacity spanning for the SU 0 (2) × USp π (4) × SU 0 (2) theory. SU(2)'s 1-instanton. There is also a discrete Z 2 symmetry of exchanging the two SU (2) groups that matches the corresponding one in the SO(8) theory. Next, we evaluate the index of this theory to order x 5 . To that order we have contributions from the (1,0,0) + (0,0,1) + (1,0,1) + (2,0,0) + (0,0,2) -instantons. Using the fugacity spanning shown in figure 32, we find: Although we evaluated the index to order x 5 , we have written it only up to x 3 to avoid over-clutter. From the x 2 terms one can see the conserved currents of the classical global symmetry as well as ones provided by the (1,0,0) + (0,0,1) -instantons results in the enhancement of U(1) 2 × SU(2) 2 → USp(4) 2 . This matches the global symmetries of the two theories and one can see that also the indices match to order x 3 . We have also confirmed that the matching persists up to order x 5 .

Example 2
Our next examples involves SO(N ) groups with N odd. As the webs for these theories involves anÕ5 − plane with a stuck monodromy, performing S-duality is difficult. However, we can still overcome this by simply considering the guage theory on the NS5-branes. For example, consider the web of figure 33 (a) describing SO(7)+1V +2S. We can mass deform it as shown in figure 33 (b). From the point of view of the NS5-branes, this describes an SU 0 (2) gauging of the SCFT described by USp(4) + 1AS + 2F (see figure 33 (c)). The gauging is done into the topological symmetry of the USp(4) gauge theory, but as this theory has an enhancement of symmetry to SU(3) [5], we can rotate it so as to sit in the flavor sector. So we conclude that the dual is AS + USp(4) × SU 0 (2) where all that's left is to determine the θ angle of USp (4). Comparing global symmetries, we see that they match: the SO(7) theory having a U T (1) × SU V (2) × USp S (4) global symmetry while the quiver having a U T (1) × SU AS (2) × USp(4) one (here we have used the enhancement of U(1) × SU BF (2) → USp(4) coming from the 1-instanton of the gauge SU(2) seen in the previous JHEP03(2016)109 example). We thus see that the dual must be AS + USp π (4) × SU 0 (2), as otherwise there would be an additional enhancement not expected in the SO(7) theory. 3 We want to further test this duality by comparing the superconformal index. There are two problems with this calculation. One, due to the presence of the spinor matter, we cannot calculate the SO(7) instanton contribution so we can only calculate the perturbative part. Two, there is a problem calculating di-group instantons in the AS +USp π (4)×SU 0 (2) theory. Calculating instantons in USp + AS requires removing decoupled states where the full instanton partition function, Z, contains extraneous contributions that must be removed by hand. This case is well understood, and the form of the decoupled states was worked out in [30]. Defining Z c for the full instanton partition function with the extraneous contributions removed, we find: where c stands for the antisymmetric SU(2) fugacity, a for the USp(4) instanton fugacity, and χ SU(2) [2] is the character for the fundamental of the gauge SU(2) (which is a global symmetry from the USp(4) point of view). We also use P E[x] for the plethystic exponent of x, and this term in (4.3) gives the contribution of the decoupled states. One notes that they carry gauge charges under the SU(2) gauge group. These are responsible for the lack of enhancement, but also imply non-trivial interaction between these decoupled states and the SU(2) gauge group degrees of freedom. Therefore, while Z c should properly capture USp(4) or SU(2) instantons, we expect additional extraneous contributions for di-group instantons making these calculations unreliable.
Bearing this in mind, we next state our result. We start with the SO(7) + 1V + 2S theory. The classical global symmetry consists of a topological U(1), an SU(2) associated JHEP03(2016)109 the USp(4) + 1AS + 4F theory as an enhancement of U T (1) × SO F (8) → SO(10) [5] which we can use to rotate the gauging to the flavor symmetry. Thus, we conclude that the dual is USp π (4) × USp 0 (4) + AS where the last θ angle was chosen so that the global symmetries match.
Particularly, the SO(9) theory as a classical symmetry given by U T (1) × SU V (2) × USp S (4) while the USp quiver as a classical U T (1) 2 × SU BF (2) × SU AS (2) global symmetry. However we find that when θ = 0, for the USp group with the antisymmetric, there is an additional enhancement of U T (1) × SU BF (2) → USp(4). Thus, with this choice of θ angle, the global symmetries of the two theories agree again up to additional enhancements on either side. 4 We next test this by calculating and comparing the superconformal index. There are two major limitations in this calculation. First we cannot calculate the SO(9) instanton contribution due to the presence of spinor matter. Second, we cannot reliably calculate di-group instantons for the USp 2 theory. The reasons are the same as before: instanton counting for USp(4) + AS requires removing the contributions of decoupled states. The precise form of these decoupled states was worked out in [30], and in our case the removal is done by: where c is the antisymmetric fugacity, z the bifundamental, q the topological one for the group with the antisymmetric and χ USp(4) [5] is the character for the antisymmetric of the gauge USp π (4) (which is a global symmetry from the USp(4) + AS point of view). Again The gauge charges imply additional corrections for di-group instantons are expected so (4.7) is insufficient for the evaluation of di-group instanton contributions.

A Index computation
This appendix provides a brief review of the 5d superconformal index, and it's calculation using localization. The superconformal index is a sum of the BPS operators of a theory where if two or more operators can merge to form a non-BPS multiplet, they sum to zero. This is a useful quantity as it is invariant under continuous deformations since the spectrum of BPS operators can only change via this merging. Specifically for the case of 5d N = 1 SCFT, the representations of the superconformal group are labeled by the highest weight of its SO L (5) × SU R (2) subgroup. We will call the two weights of SO L (5) as j 1 , j 2 and those of SU R (2) as R. Then following [16] the index is: where x, y are the fugacities associated with the superconformal group, while the fugacities collectively denoted by q correspond to other commuting charges Q, generally flavor and topological symmetries. For a 5d gauge theory the index can be evaluated by localization where it is given by [16]: where the integral is over the Cartan subalgebra of the gauge group. The terms Z pert and Z Nek are the contributions of the perturbative and instanton sectors respectively. The perturbative contribution, Z pert , can be easily evaluated using the results of [16]. The instanton contribution, also known as the 5d Nekrasov partition function [36], is harder to evaluate. In general Z pert is expanded in a power series in the instanton fugacity, each term providing the contribution of the associated instantons. These terms can in turn be evaluated by a contour integral where the integrand receiving contributions from the various matter and gauge content of the theory. The expressions for most of these contributions that we need have appeared elsewhere, notably [9,11,12,16,30], and we won't repeat them here. The only exception being the SO × USp bifundamental and half-bifundamental whose expressions we provide below. In addition one also has to supplement this with a pole prescription detailing which poles are inside the contour. A good review of these is given in [30].
Finally, the evaluation of the Nekrasov partition function is sometimes plagued with the contributions of extraneous degrees of freedom that must be removed by hand. These can materialize in the partition function as a breakdown of x → 1 x invariance, which must be obeyed as it is part of the superconformal algebra. Another way these can appear in the partition function is as an infinite tower with representations of increasing dimension for the O − part and even K.
In some cases the contributions add additional poles to the integrand, and the prescription then follows from the previous case where one defines p = 1 x in the denominators of (A.7)-(A.8). The prescription is then to assume x, p 1, and set p = 1 x only at the end of the calculation.
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