Phenomenology of unusual top partners in composite Higgs models

We consider a particular composite Higgs model which contains SU(3) color octet top partners besides the usually considered triplet representations. Moreover, color singlet top partners are present as well which can in principle serve as dark matter candidates. We investigate the LHC phenomenology of these unusual top partners. Some of these states could be confused with gluinos predicted in supersymmetric models at first glance.

The discovery of a Higgs-like scalar resonance at the LHC [1,2] has materialized longstanding questions on the Standard Model (SM) as the ultimate theory of particle interactions. Why is the Higgs boson mass insensitive to the scale of new physics (Planck mass)? Is there a dynamical origin for the spontaneous breaking of the electroweak (EW) symmetry?
Do elementary scalar particles really exist?
The two time-honored avenues addressing the above questions are supersymmetry (SUSY) and compositeness. In the former, scalars are associated with fermions via a new symmetry extending Poincaré invariance of particle interactions. In the latter, scalars emerge as resonances of underlying bound fermions. In both cases, the solution involves tying the properties of the Higgs-like scalar to those of fundamental fermionic states, which do not suffer from the quantum sensitivity to large scales. In this work we will focus on the composite avenue, which was proposed as an alternative to the SM Higgs mechanism shortly after the SM itself was established [3,4]. While the first incarnations, inspired by Quantum Chromo Dynamics (QCD), were essentially Higgsless [5][6][7], it was later realized that a SM-like limit could be achieved by extending the global symmetry of the condensing theory to allow for a misaligned vacuum [8]. At the price of a moderate tuning, this class of models features a limit where a light Higgs-like state emerges as a pseudo-Nambu-Goldstone boson (pNGB).
This idea was revved up in the early 2000s, thanks to the holographic principle [9], which links near-conformal theories in 4 dimensions to gauge/gravity theories in 5 dimensions on a warped background. A 'minimal' model emerged [10,11], based on the symmetry breaking pattern SO(5)/SO (4), where the only pNGBs match the 4 degrees of freedom of the SM Higgs doublet field. The phenomenology of this model has been widely explored, and we refer the interested reader to the excellent reviews [12][13][14].
While the minimal model, and variations thereof, can be considered as a useful template to understand the phenomenology of a composite pNGB Higgs, models in this class are not UV complete and its UV embeddings contain additional BSM states which are relevant at colliders, like the LHC. From the holographic point of view, a 5-dimensional model is consistent only if it includes all the operators of the corresponding 4-dimensional conformal field theory: in models with top partial compositeness [15], for instance, this implies the inevitable presence of QCD-charged bosonic operators, corresponding to two-point functions we present the current bounds on scenarios with a dark matter candidate, before offering our conclusions and outlook in Section V.

II. MODEL ASPECTS
We consider an Sp(2N c ) hyper-color gauge theory with 5 Weyl fermions ψ i in the antisymmetric and 6 Weyl fermions χ j in the fundamental representation as an underlying model of the composite sector. The fermion sector exhibits an SU(5)×SU(6)×U(1) global symmetry.
It has been named M5 in [38] and its EW sector has been investigated in [49]. The chiral condensates ψψ and χχ spontaneously break the global symmetry to the stability group SO(5) × Sp (6). The SM color group SU(3) c is realized as a gauged SU(3) subgroup of Sp (6), while the weak gauge group SU(2) L is a gauged subgroup of SO (5), which also contains a custodial subgroup SO(4) ∼ SU(2) L × SU(2) R . The U(1) Y hypercharge Y = T 3 R + X is a gauged linear combination of the diagonal generator of SU(2) R ⊂ SO(5) and U(1) X ⊂ Sp (6).
In addition, the model contains two global abelian symmetries U(1) χ and U(1) ψ , acting independently on the two hyper-fermion species. One linear combination of these U(1) factors is Sp(2N c ) anomaly free, and the spontaneous breaking by the condensates yields a pNGB, while the would-be pNGB associated to the orthogonal U(1) combination is expected to receive a mass through the Sp(2N c ) anomaly. We summarize the microscopic field content that replaces the Higgs sector of the SM in Tab. I.

A. pNGBs
The condensates ψψ and χχ break the global group SU(5) × SU(6) × U(1) to SO(5) × Sp (6). This will give rise to three classes of pNGBs in this model: 1. A SM singlet pNGB a from the Sp(2N c ) anomaly-free spontaneously broken U(1). It is expected to be light and with couplings of an axion-like particle (see [38,39,50] for studies of collider bounds and projections for the pNGB a of the model considered here, as well as for other composite axion-like particles).
3. 14 pNGBs in the color sector in the 14 of Sp (6), which decomposes into 8 0 +3 −2x +3 2x under SU(3) c × U(1) Y . They play a central role in the phenomenology we discuss here, hence we provide more details below as they have not been discussed elsewhere in the literature.
The pNGB sector of SU(6)/Sp(6) can be parameterized by a scalar field Σ χ in the antisymmetric 2-tensor representation 15 of SU(6), transforming like gΣ χ g T where g ∈ SU(6). 1 The vacuum, which respects the stability group Sp(6), can be written as where 1 3 is a 3 × 3 identity matrix. Hence, within Sp(6), the QCD SU(3) c subgroup is defined by the following 8 generators where λ a are the Gell-Mann matrices corresponding to the usual SU(3) c generators, normalized as tr(λ a λ b ) = 2δ ab . In addition, there is a U(1) X subgroup of Sp(6) needed to assign the correct hypercharge to the composite colored states: the SM hyper- (5) in the EW coset. Choosing x = −1/3 yields the correct hypercharge for the top partners, as we will show below.
The pNGB matrix can be written as where X I are the 14 generators broken by the vacuum in Eq. (2.1). It transforms as U χ → gU χ h † with g ∈ SU(6), h ∈ Sp(6). In terms of SU(3) c , the 14 degrees of freedom decompose into a color octet π 8 and a complex color triplet π 3 , where π 8 has charge 0 with respect to the U(1) X subgroup and the triplet 2/3. As these are SU(2) L singlets, these numbers correspond automatically to their hypercharges and consequently also to their electric charges. The explicit decomposition of Π χ in terms of these fields reads In the following we will refer to π 8 and π 3 as octet and triplet pNGBs, respectively.
The π 8 couples via the Wess-Zumino-Witten term to two gluons. The corresponding coupling is proportional to f −1 χ and, thus, one could get in principle contraints on the decay constant f χ from existing LHC data [40]. These bounds depend on the π 8 mass m π 8 and vanish for m π 8 > ∼ 1.1 TeV. However, we note for completeness that one has in addition a decay constant f ψ in the electroweak sector beside f χ . One expects that both have the same size. It is well known, that electroweak precision data give constraints on f ψ , see e.g. [16] and references therein. One finds that the ratio v/f < ∼ 0.25, where v is electroweak vaccum expection value. This implies f χ f ψ > ∼ 1 TeV.

B. Chimera hyper-baryons
In the confined phase, the model contains fermionic resonances (chimera hyper-baryons) corresponding to composite operators made of one ψ and two χ hyper-fermions. They can be classified in terms of their transformation properties under the stability group SO(5)×Sp (6) Hence, it is the 14 that contains color-triplets that can mix with the SM elementary top fields to generate partial compositeness for the top quark mass origin. In terms of Sp (6), the components of the 14 are embedded in the anti-symmetric matrix 3,k gives correct transformations for the SU(3) c generator embedding (i.e. the diagonals transform like 3 × 3 ⊃3 and3 ×3 ⊃ 3 while the off-diagonals transform like octets). Each component Q 3 and Q 8 also transform as a fundamental of SO (5): where we have fixed x = −1/3 in order to have the correct hypercharges for the color triplets that will mix with the top quark. The first four components transform as two doublets of SU(2) L (and a bi-doublet of SU(2) L × SU(2) R ), while the fifth is a singlet.
The couplings of the top fields to the hyper-baryons depend on the choice of three-hyperfermion operator. In fact, the partial compositeness couplings for the left-handed top (in the doublet q L,3 ) and right-handed top t c R are assumed to originate from a four-fermion interaction. The simplest possibility is with the appropriate components of the hyper-fermions. Here we have chosen to couple them to the operator ψχχ in the channel (5,15), see Tab. II. This implies the presence of the singlet baryons as well: Octoni (Dirac): The choice of the names is motivated by the fact that the statesh,B andg have the same quantum numbers as the higgsino, bino, and gluino in supersymmetric extensions of the SM.
Their embedding in the global symmetries are schematically shown in Fig. 1, together with that of the colored pNGBs.

C. Partial compositeness couplings and baryon number
Following the Coleman-Callan-Wess-Zumino (CCWZ) prescription [52,53], the low energy Lagrangian for the hyper-baryons contains three types of couplings [54]: where F L/R and F are functions of the pNGB matrices Π χ and Π ψ . The kinetic term encodes gauge interactions with the SM via the covariant derivative D µ . The second term is generated by the operators in Eq. (2.11) and encodes the mixing between the SM top fields and the hyper-baryons, hence generating a mass for the top quark proportional to the product y L y R . 2 The indices u and d indicate that the corresponding SU(2) L doublets have isospin 1/2 and −1/2, respec- We note that the three-hyper-fermion operator ψχχ must have conformal dimension d 5/2 in order to obtain a top quark mass, since y L/R ∼ (Λ HC /Λ t ) d−5/2 and Λ HC Λ t [14]. Finally, we include derivative couplings of the colored pNGBs in the third term, as they comprise couplings between the octet and singlet baryons, which are of phenomenological relevance for our purposes. These interactions are generated by the strong dynamics itself, and they are suppressed by the compositeness scale f χ .
We first need to embed the SM fields q L,3 and t c R in a representation of SU(5) × SU(6) to write down the couplings to the top, second term in Eq. (2.14). First we define two unique embeddings as5 of SU(5) as follows: Then, we embed them in the 15 (Ā) representation of SU(6) as follows:  (6), they need to be dressed by pion matrices as follows: such that the two operators transform as (5, 15) of SU(5) × SU (6).
Finally, the couplings with the top fields can be written as follows. For the left-handed top field: where i, j are QCD color indices and the SU(5) contractions lead to where, for simplicity, we have set to zero the misalignment angle that breaks the EW symmetry (see Appendix A for more details). We only display couplings involving one colored pNGB. Similarly, for the right-handed top singlet: Alternative top quark embeddings in the global symmetries and couplings to other hyperbaryons, see Tab. II, are reported for completeness in Appendix B. The case of the (5,15) leads to similar couplings to the one presented here, up to signs. The (5,35), instead, is very different, as it involves the 21 of Sp(6) and the partial compositeness couplings always involve a minimum of 2 colored pNGBs. We leave the phenomenology of this case to future work.
The last term in Eq. (2.14) generates derivative couplings between the hyper-baryons and the colored pNGBs. In our case, this only involves the 14 and the singlet of Sp (6), and it can be written as where the trace acts on the Sp(6) indices and Here, Ψ 1 contains the singlet top partners and d µ is a Maurer-Cartan form written in terms of the colored pNGBs. Expanding up to linear order in the pNGB fields, we find where the SO(5) contractions are left understood.
All the couplings stemming from Eq. (2.14) allow to assign SM baryon number charges B to all the top partners, so that B is still preserved in the presence of top partial compositeness.
This results in all the color triplets to carry B = 1/3, like quarks, while color octets and singlets remain neutral. This can be achieved by assigning appropriate baryon number to the hyper-fermions in the underlying theory, see Tab. I: B = 1/6 to χ 4,5,6 transforming as an anti-triplet and B = −1/6 for χ 1,2,3 transforming as a triplet. Hence, This implies that the lightest state among the components of Q 8 , Q 1 and π 3 must be stable in absence of either baryon or lepton number violation, as there is no matching SM final state.  [55]) and a color octet Majorana top partner (at NNLO approx +NNLL from [56]).

III. PHENOMENOLOGY AT HADRON COLLIDERS
The phenomenology of M5 at hadron colliders depends crucially on the mass hierarchy among the QCD-colored baryons, which enjoy the largest production rates due to their QCD interactions. As they all belong to the same baryon multiplet -the 14 of Sp (6)  A typical spectrum for the colored top partners is illustrated in Fig. 3 (left). The triplets that have charges matching the top and bottom quarks, i.e. 2/3 and −1/3, receive large positive corrections due to the mixing with the top fields, which makes them heavier than the octets and of X 5/3 . On the other hand, the mass difference between the octets and X 5/3 is due to QCD corrections. A crude estimate can be obtained starting from the electromagnetic contribution to the mass split between proton and neutron in QCD. We take as a starting point the results of [57] on the electromagnetic contribution to the proton neutron mass difference ∆m em 0.58 MeV, which is also confirmed by lattice studies [58]. This corresponds roughly to a relative mass difference r = 2∆m em /(m P + m N ) 6 · 10 −4 . We then re-scale this by the gauge couplings and the difference of Casimir factors for the two QCD representations, to obtain

Octets Triplets
This estimate confirms that the octet top partners are dominantly produced at the LHC compared to the usual triplet top partners. It is also interesting to note that the mass difference between the octonis and the gluoni is generated by EW corrections, which we estimate to be where we included the dominant contribution of SU(2) L . Note, however, that a contribution to this mass difference is also generated by SU(5)-breaking mass differences in the ψ sector, which could go in either direction. Finally, we expect the charged octoni to be slightly heavier than the neutral one due to EW symmetry breaking effects.
The final states resulting from octet top partner decays depend on the mass hierarchy with the singlet top partners and the QCD-colored pNGBs. We reasonably expect the pNGBs to be lighter than the colored hyper-baryons. The singlet top partners, however, receive a mass M 1 = M 14 from the confining strong dynamics, and the precise values can only be obtained from lattice studies. We will explore two different scenarios for M 1 . As discussed in the last section, the lightest state amongB,h 0,± , π 3 is stable, unless additional baryon or lepton number violating interactions are added to the model. If the lightest singlet top partnerB orh 0 is lighter than π 3 , a stableB/h 0 provides potential Dark Matter (DM) candidatescase A. If π 3 is lighter thanB, a stable π 3 is not viable, and new interactions need to be present, which open baryon and/or lepton number violating π 3 decay channels -case B.
Note that case B could also occur if the singlet top partners are the lightest. Both cases carry resemblance with SUSY signatures: gluinos decaying into tops plus missing transverse energy in case A, and R-parity violating decays in case B.

A. Scenarios with a DM candidate
This scenario can occur if the singlet top partners, boni or higgsonis, are lighter than the colored pNGBs, and cannot decay into any SM final state being the lightest hyper-baryons.
We also assume throughout this work that the colored top partners are heavier than the pNGBs. Henceforth, the lightest color-singlet baryon can be a DM candidate or, at least, be detector stable if it decays via higher order operators.
The top partnersh 0 ,h + andB and the pNGB π 3 have quantum numbers resembling the higgsino-bino and right-handed stop sectors of SUSY models, and their phenomenology depends on the mass mixing among them. Considering only the EW interactions, one finds as shown in Fig. 3 (right), with a mass splitting estimated to range around or less than 0.2% of the mass, i.e. below a GeV for masses in the TeV range, see Eq. (3.2). A small mixing is also generated by the EW symmetry breaking. However, the mass difference between the boni and the higgsonis also receives a sizable contribution from the SU(5)-breaking mass differences between the singlet and bi-doublet hyper-fermions ψ, which can go in either direction. The most natural expectation is that the spectrum remains fairly compressed, hence we would expecth + andh 0 to decay into soft leptons and mesons plusB. Thus, all three particles would effectively contribute to the missing transverse momentum as the soft decay products are hardly registered in the detectors. Such a scenario might, therefore, be easily confused with a SUSY model at first glance.
The QCD-colored pNGBs π 3 and π 8 are heavier than the EW ones as their masses receive contributions from QCD loops [37]. As π 3 carries baryon number, its decay modes are strongly constrained: In the scenario under consideration, the only available decay channels are π 3 → tB, th 0 , bh + .
The first one dominates if y R y L , while the decays in the higgsonis dominate for y L y R .
In principle, decays into lighter families, like cB and uB, are also possible, but in the spirit of composite Higgs models we expect those to be strongly suppressed. Hence, π 3 behaves exactly like a right-handed stop in supersymmetry, and LHC bounds from scalar top quark searches can be directly applied [59][60][61]. We will come back to this in Sec. IV.
The color octet π 8 can decay directly into a pair of SM states: with decays into a pair of light jets as subleading channels. We will discuss bounds on π 8 further in Sec. III C.
The octet top partnersG 0,+ andg feature the largest pair-production cross sections at hadron colliders such as the LHC or a prospective 100 TeV pp-collider. In the scenario considered here, their decays lead to final states similar to those of gluinos in SUSY models.
This applies, in particular, to the Majorana gluonig that decays via the following channels depending on the mass spectrum. In all cases the final states contain large missing transverse momentum as we assume theB to be collider stable. This implies that gluino searches at the LHC can be used to constrain these scenarios. A similar comment applies in case of the Dirac statesG 0 andG + , which -depending on the mass spectrum -decay into the following channelsG 0 → π 3t → ttB / tth 0 / bth + and/or (3.7a) G + → π 3b → tbB / tbh 0 / bbh + and/or (3.7c) Note thatG 0 resembles a Dirac gluino in extended SUSY models [62], while the charge one gluoniG + is a novel state from composite models without a SUSY analog. For completeness, we note that for a fixed mass the QCD production cross sections fulfill the relation In addition, there are subdominant EW production cross sections for the SU(2) L doublet such as In Section IV we will focus on the final states discussed above, and present numerical studies of the bounds coming from current LHC searches. For simplicity, we will focus on the case y R y L , so that onlyB appears in the π 3 decays.

B. Scenarios without a DM candidate
If π 3 is lighter thanB, lepton or baryon number violating interactions need to be included in order to avoid a stable π 3 . As we have seen in the previous section, these interactions are not allowed by the symmetries of the low energy Lagrangian (including the top partial compositeness couplings), hence they must be generated by new couplings in the UV completion.
The corresponding operators can then be added to the low energy effective Lagrangian via appropriate spurions. Also,B will be allowed to decay via the inverse process in Eq. (3.4).
The simplest possibilities are The former violates baryon number whereas the latter violates lepton number. This implies that only one of the two interaction types can be present as otherwise there would be the danger of proton decays at a rate incompatible with experiment. This scenario corresponds to typical R-parity violating SUSY models for the stop decays, although the origin of the couplings is very different from the SUSY case and no R-parity analog exists in the composite model.
The QCD-singlet top partnersh 0 ,h + andB can decay according tõ Furthermore, there could be mixing ofh 0 andh − with the left-handed leptons, extending the spirit of partial compositeness to the leptonic sector. In such a case one can well imagine thatB plays the role of a heavy right-handed neutrinos. Additional decay channels into EW gauge bosons and pNGBs would be present, such as to name a few. Note that this possibility is only compatible with the π 3 decay in Eq. (3.11), as it involves lepton number violation, and it also holds if π 3 is heavier than these states.
The final states from the decays of the color-octet baryon will contain additional jets and leptons from the new decays of π 3 and the singlet baryons, and reduced missing transverse momentum. We leave a detailed study of these signatures to future investigations.

C. Phenomenology of other composite states
The model contains other composite states, whose phenomenology does not depend on the cases A and B, and we summarize them here.
Firstly, the EW coset SU(5)/SO (5) [49]. The EW pNGBs can be produced in Drell-Yann, pair produced via their EW gauge interactions, or appear in the final states of the decays of top partners, as we will discuss below.
The decays and the resulting LHC phenomenology of the octet pNGB π 8 are also independent on the spectrum, as listed in Eq. (3.5). Their phenomenology has been widely studied, both in the case of composite models [37,38,40] and in effective and supersymmetric set-ups (sgluons) [65][66][67][68][69][70][71][72]. In the following we will assume that π 8 can either decay into tt and/or g g. 3 Current bounds on the π 8 mass from LHC searches for pair production with dominant decays into tt and gg lie at ∼ 1.05 TeV and ∼ 0.85 TeV, respectively, while bounds from single production are strongly model dependent [40].
In this model under consideration, the usual color triplet top partners, B, T i and X 5/3 , have additional exotic decay modes [25] beside the ones used by the ATLAS and CMS for the searches. In absence of the exotic decays, top partner pair production searches ATLAS and CMS established bounds on the top partner mass of the order of 1.3 -1.6 TeV (depending on the top partner branching ratios) [73][74][75][76][77][78][79][80][81][82][83][84][85][86][87][88][89][90][91], but the presence of exotic decay modes can alter these mass bounds. We list the possible decays for the color triplet top partners below, starting from the usually considered decays into third generation quarks and EW bosons, followed by the exotic decays with other EW and QCD-colored pNGBs: The spectrum in Fig. 3 also allows decays into the color octetsg,G 0 orG + plus a colored pNGB, however due to the large mass of π 3 and π 8 we assume here that they are kinematically forbidden. The signatures from top partner pair production will consist of at least two jets (stemming either directly from a b and/or from a b resulting from a t decay) in combination with jets and leptons stemming from the decays of the electroweak bosons. Moreover, there will be substantial missing transverse momentum in final states with decays intoB andh.
If decays into the strongly interacting pNGBs dominate one gets signatures alike those of color octet baryons discussed above. In case of single production of the color triplet top partners one has on the one hand the commonly considered signatures arising from the decay into a third generation quark and a SM boson. On the other hand, one has also final states consisting of a top quark and two vector bosons or a single top quark plus missing transverse momentum. Several, but by far not all of the exotic decay channels have been discussed in the literature [25][26][27][28][29][30][31][32][33][34][35][36].

IV. LHC BOUNDS ON FERMIONIC COLOR OCTETS
In this section, we provide a first phenomenological study of the fermionic color octets.
In the model M5, they are part of the same Sp(6) multiplet as the color triplet top partners, and -as discussed in Sec. III A -they are expected to have masses comparable to the usual top partners. Due to their QCD representation, the production cross section for the octet top partners will be significantly larger than the one for the usual top partners, as is shown in Fig. 2. Henceforth, the octet top partner signatures might be the first sign of the model, if realized in nature. We focus on the scenario with DM candidate described in Sec. III A.
Based on the discussion in Sec. III A, we make a number of simplifying assumptions for our phenomenological study. We assume all the octet top partners Q 8 = (g,G +,0 ) to be mass degenerate. The boniB is assumed to be the lightest hyper-baryon which is taken to be (at least collider scale) stable. Furthermore, we assume the higgsonish +,0 to be nearly mass degenerate with the boni and that they promptly decay to the boni plus soft leptons. Therefore all (color) singlet top partners Q 1 = (B,h +,0 ) have a common mass scale.
Moreover, we assume that π 3 decays dominantly into tB for simplicity.
We study three scenarios which cover the different possible octet top partner decay channels based on the spectra and interactions discussed in Sec. III A: • Scenario 1: Octet top partners decay dominantly to π 3 and 3rd generation quarks.
• Scenario 3: Octet top partners decay through both the above channels (with comparable branching ratios).
For each scenario, we determine bounds from current LHC searches for gluino pair produc- We do not attempt any combination. As could be expected, we find that the most sensitive available searches for the final states under consideration are ATLAS and CMS searches for stops and gluinos [59,108,109]. In Appendix D, we provide more details on the exclusion power of various existing searches in a few sample scenarios.   For lightB, the bound on mG+ extends to 2.4 TeV. This bound is higher than forg pair production which is owed to the fact that theG + G − production cross section is twice as large. In Fig. 5 (b) for nearly degenerate mass spectrum, the bound on mG+ appears less reduced than for mg. The reason for this apparent difference is that for Fig. 5   Ref. [38] as where κ g = 2d χ and d χ = dim(χ) = 2N c = 4 is the dimension of the χ representation. 5 The ratio of π 8 decays into tt and g g is given by The value of C t,8 depends on the details of the mixing of the top partners with the top, see Ref. [40] for a discussion. Therefore we consider three cases: (i) exclusive decay π 8 → g g, (ii) decay π 8 → g g, tt with equal branching ratio, and (iii) exclusive decay π 8 → tt. In each case, we fix m π 8 = 1.1 TeV which is at the level of current experimental constraints on m π 8 [40]. Depending on the mass splitting, higgsoni decays could yield displaced vertices, but the LHC searches which we use to determine bounds, here, are not sensitive to the displacement, and the higgsoni effectively yields p miss T like the boni. 6 Thus the effective final states are 4j +p miss T 5 We neglect π 8 decays into g γ and g Z (see [40]) as well as into a pair of light quarks here as they do not dominate in M5. 6 On a technical level, for our event simulation, the higgsonis are chosen 5 GeV heavier than the boni and to decay promptly into boni and 1st generation leptons.  with subsequent decay to a singlet fermion Q 1 and a π 8 . The octet pNGB mass is fixed to m π 8 = 1.1 TeV. In the first row only the gluoni is considered, which decays to a π 8 and a boni. In the second row the complete multiplets are taken into account, Q 8 = (G + ,G 0 ,g) and Q 1 = (h + ,h 0 ,B). The multiplets are assumed to be almost mass degenerate. The boni is stable, for the π 8 we consider the decays to gg (left column), to tt (right column) or to either with equal branching ratio of 50% (middle column).
for case (i), 4t + p miss T for case (iii) and both of these plus 2t + 2j + p miss T for case (ii). Note that the 4t + p miss T final state resembles theg pair production final state considered in the last subsection, but it has completely different kinematics, as here, the two tt pairs form the π 8 resonances. Efficiencies and bounds are thus expected to be altered as compared to the bounds presented in the last subsection. Figure 7 shows the obtained bounds for various cases. Again, we find the implemented search [59] to dominate the bound over most of the parameter space and refer to Appendix D for more information on bounds from other searches. Finally, we consider a scenario in which color octet top partner decays to both pNGB triplets and octets are present. To study this case in more detail, we performed a scan in which we set the couplings of the color octet top partners to π 3 and π 8 to a fixed ratio of  Br(Q 8 → π 8 Q 1 ) = 0. In case of π 8 we take Br(π 8 → gg) = Br(π 8 → tt) = 50%.
octet and singlet fermion masses, keeping m π 8 = 1.1 TeV, m π 3 = 1.4 TeV and the couplings fixed. Due to the decay phase space factors, the Q 8 branching ratios vary depending on the Q 8 and Q 1 masses, as is shown in Fig. 8. For the π 8 decay, we assume a branching ratio of 50% into tt and gg. We display the resulting bounds on the color octet top partner masses in Fig. 9 assumingg pair production only (left),G +G− production only (middle), and pair production of all color octet top partner states (right). As expected, the bounds are comparable to the cases of Br(Q 8 →qπ 3 ) = 1 and Br(Q 8 → π 8 Q 1 ) = 1.

V. CONCLUSIONS AND OUTLOOK
This is the first of a series of papers where we explore the collider phenomenology of composite Higgs models with a concrete UV completion. Here we have focused on the so- We briefly summarize here for completeness some main results of [49] for the electroweak (EW) Goldstone boson sector. It can be parameterized by a scalar field Σ ψ in the symmetric 2-tensor representation 15 of SU(5), transforming like gΣ ψ g T where g ∈ SU(5).
The EW preserving vacuum which respects the SO(5) subgroup of SU(5) reads It has a slightly unusual form but this form helps to uniquely identify the SO(4) part which at the level of the Lie algebras is isomorphic to SU(2) L × SU(2) R . This facilitates also the identification of the quantum numbers of the hyper-baryons. The (unbroken) generators of SU(2) L,R of the EW preserving vacuum are: The Goldstone-boson matrix reads with where η is an electroweak singlet, H is the Higgs doublet,H = iσ 2 H * , and π 0 = 1 √ 2 π i 0 σ i , π − = π i 0 σ i = (π + ) † form a SU(2) L ×SU(2) R bi-triplet. Replacing as usual linear combinations of the real fields by complex fields, one gets more explicitly Moreover, we parameterize H as With respect to the vacuum Σ 0,ψ , Σ ψ is given by However, the Higgs vacuum expectation value (vev) v breaks the electroweak symmetry, and we expand around the true (misaligned) vev. The misaligned vacuum is given by where s θ = sin(θ) = v/f ψ and is the misalignment of the vacuum along the Higgs direction due to the non-zero Higgs vev.

Appendix B: Alternative hyper-baryon embedding
In the main text, we presented in detail the case where the top partial compositeness involves operators transforming as the (5,15) of the global symmetry SU(5) × SU (6). Here we recap the other two cases, corresponding to (5,15) and (5,35).
For the former, (5,15), the embedding is very similar, and one has This implies a simple change in sign of the colored pNGB couplings in Eqs. (2.18) and (2.20).
Hence, the phenomenology of this case will be the same as that described in the main text.
For the latter, (5,35), one main difference is the presence of the 21 of Sp(6) hyper-baryon: To write couplings to the top, stemming from the four-fermion interactions, analog to The embeddings of the hyper-baryons in the adjoint of SU(6) and anti-fundamental of SU (5) read where the singlet Q 1 does not appear as is does not enter in the four-fermion operators that couple to the top quark fields. Instead, the elementary top fields are embedded in the SU (6) adjoint as where the embedding in the fundamental of SU(5) reads: The main difference with the previous cases is that couplings of a single colored pNGB with two top partners or one top partner and one top field are absent. The lowest order couplings contain two colored pNGB, hence the phenomenology of this case differs enormously from the other cases. We leave this case for further exploration.  [31][32][33]36]. For this work, we extended the implementation by colornon-triplet fermions as well as BSM-BSM-SM interactions required for our simulations. The following modules are implemented (and available upon request): • A neutral color singlet scalar S 0 1 .
• A neutral color octet scalar S 0 8 .
• Color octet fermions with charges Q = 1 (Q 1 8 ), Q = 0 (Q 0 8 ) and a Majorana (Q 0 8,M ). An overview of the notation for the fields is given in Tab. III, where we also indicate the corresponding fields in M5. For modules that correspond to multiple fields, e.g. S10, we add copies of the corresponding files with the replacements S10 → S102,S103 etc.
In the following we present the Lagrangians for the new fields, excluding lepton and baryon number violating terms. The Lagrangians are given in the mass eigenbasis, so the fields are eigenstates of SU(3) c × U(1) em .
General Lagrangian for S 0 1 ∈ 1 0 : General Lagrangian for S 1 1 ∈ 1 1 : General Lagrangian for S 2 1 ∈ 1 2 : General Lagrangian for S 2/3 3 ∈ 3 2/3 : General Lagrangian for S 0 8 = S 0,a 8 T a ∈ 8 0 : General Lagrangian for Dirac fermion Q 1 1 ∈ 1 1 : General Lagrangian for Dirac fermion Q 0 1 ∈ 1 0 : General Lagrangian for Dirac fermion Q 1 8 ∈ 8 1 : We have also implemented selected vertices that mix different modules:  In this appendix, we highlight the recasted searches that are most sensitive to the decays of the octet top partners. To this end, we show the mass bounds for the scenarios 1 and 2 separately for each search in Fig. 10. Here, the gray dots are the simulated points, for which we generated 10000 events each. The coarse structures in the contour lines are due to the limited resolution of the grid and could be improved if a more precise knowledge of the bounds is required. Fig. 10 shows that the bounds are dominated by only a few searches.
• CMS-SUS-19-006 [59]: This is a search for gluino and squark pair production with multiple jets and large MET in the final state using 137 fb −1 of data. The results are interpreted within multiple simplified models, including the 4t + p miss T , 4b + p miss T , 4q + p miss T and 4q + 2V + p miss T final states from gluinos, where q = u, d, s, c are light quarks and V = W, Z. The signal candidates are divided into 174 orthogonal SRs, and covariance and correlation matrices for the SRs are provided. These are used by the recast implemented in MA [110] to perform a statistical combination of the SRs. This explains why this search gives the strongest bound for most scenarios. The optimization for both 4t and 4j final states makes the recast competitive both for π 8 → tt and π 8 → gg.
• ATLAS-CONF-2019-040 [108]: This search looks for gluinos and squarks in final states containing jets and MET but no charged leptons. It uses the full Run 2 dataset of 139 fb −1 . The simplified model for the gluinos assumesg → qqχ 0 1 org → q qWχ 0 1 , where q ( ) are light quarks. We therefore expect the recast to be very sensitive to final states with multiple light jets, such as those from π 8 → gg. This is confirmed by comparing Figs. 10c-e. For the final states dominated with top quarks, however, this search is subdominant. Note that it is implemented in both MA and CM. Figure 10 shows the mass bounds from several other searches, which however are less sensitive to our signatures. We briefly summarize those: ATLAS-CONF-2018-041 [109] presents a search for gluino pair production with decays to third generation quarks and neutralinos using 79.8 fb −1 of data. ATLAS-1908-03122 [117] searches for bottom-squark production with Higgs bosons in the final state. ATLAS-SUSY-2016-07 [114] is a search for gluinos and squarks in final states with light quarks and no leptons. It is implemented in both MA and CM. CMS-SUS-16-033 [115] searches for pair production of gluinos and stops decaying to light or third-generation quarks, similarly to CMS-SUS-19-006 but using only 35.9 fb −1 . Finally, ATLAS-2101-01629 [116] searches for pair production and chain decays of gluinosg → qq χ ± 1 and squarksq → q χ ± 1 withχ ± 1 → W ±χ0 1 .