KCL-PH-TH/2015-56, LCTS/2015-46, CERN-PH-TH/2015-303

MCTP-15-33, CAVENDISH-HEP-15-14, DAMTP-2015-90

On the Interpretation of a

Possible GeV Particle Decaying into

John Ellis, Sebastian A. R. Ellis, Jérémie Quevillon,

Verónica Sanz and Tevong You

Theoretical Particle Physics and Cosmology Group, Physics Department,

King’s College London, London WC2R 2LS, UK

TH Division, Physics Department, CERN, CH-1211 Geneva 23, Switzerland

Michigan Center for Theoretical Physics (MCTP), Department of Physics, University of Michigan, Ann Arbor, MI 48109, USA

Department of Physics and Astronomy, University of Sussex, Brighton BN1 9QH, UK

Cavendish Laboratory, University of Cambridge, J.J. Thomson Avenue,

Cambridge, CB3 0HE, UK;

DAMTP, University of Cambridge, Wilberforce Road, Cambridge, CB3 0WA, UK

Abstract

We consider interpretations of the recent reports by the CMS and ATLAS collaborations of a possible state decaying into final states. We focus on the possibilities that this is a scalar or pseudoscalar electroweak isoscalar state produced by gluon-gluon fusion mediated by loops of heavy fermions. We consider several models for these fermions, including a single vector-like charge T quark, a doublet of vector-like quarks , and a vector-like generation of quarks, with or without leptons that also contribute to the decay amplitude. We also consider the possibility that is a dark matter mediator, with a neutral vector-like dark matter particle. These scenarios are compatible with the present and prospective direct limits on vector-like fermions from LHC Runs 1 and 2, as well as indirect constraints from electroweak precision measurements, and we show that the required Yukawa-like couplings between the particle and the heavy vector-like fermions are small enough to be perturbative so long as the particle has dominant decay modes into and . The decays and are interesting prospective signatures that may help distinguish between different vector-like fermion scenarios.

December 2015

## 1 Introduction

The CMS and ATLAS Collaborations have recently announced preliminary results
from the first /fb of data from Run 2 of the LHC at 13 TeV, and both have
reported enhancements in the inclusive spectrum at GeV
that could be interpreted as decays of a possible massive particle [1, 2].
In the words of Laplace, “Plus un fait est extraordinaire, plus il a besoin d’être appuyé de fortes preuves” ^{1}^{1}1“The more extraordinary a claim, the stronger the proof required to support it.”,
so this evidence would need to be strengthened greatly before the existence of a new state could
be regarded as established. Moreover, there are issues concerning the CMS and
ATLAS signals, e.g., the angular distributions of the final states and the energy
dependence of the reported signal. Nevertheless, while maintaining our proper scepticism, we think it
worthwhile to explore possible interpretations of this possible new particle, and how they could be
probed experimentally, in the hope of either corroborating and elucidating the signal or else
despatching it.

As in the case of the Higgs boson discovered in 2012 [3], one may first ask what the spin of the particle could be. As in that case, the leading hypothesis would be spin zero, though one should also consider spin two. The spin-two hypothesis would yield a angular distribution peaked in the beam directions [4]. There there is no significant evidence for this at the present time, but we consider the spin-two hypothesis more exotic. Therefore, we focus on spin-zero scenarios in the bulk of this paper, and on the corollary question whether the could be scalar or pseudoscalar.

In either case the decay mode reported would presumably arise from loop diagrams with circulating fermions or bosons [5]. Even if the had couplings to the quark or , the form factors for their loops would be suppressed at large invariant masses and the dominant decays of the would be to or . Hence the observation of the decay mode is prima facie indirect evidence for additional, heavier fermions and/or bosons whose masses are GeV. Having masses much greater than the electroweak symmetry-breaking scale, any such fermions would presumably be vector-like, and much of this paper explores scenarios with massive vector-like quarks and/or leptons. Alternatively, the decay could be induced (partially) by loops of massive bosons, and we discuss the possibility that these could correspond to the signal for a diboson resonance reported previously by ATLAS and CMS.

Turning to possible production mechanisms for the , we recall that, although each of CMS and ATLAS observe a signal with /fb at 13 TeV, neither reported a signal with /fb at 8 TeV [6, 7], although there is a small enhancement in the CMS data at GeV. The data at different energies would be accommodated more easily if the were produced via a mechanism with a steeper energy dependence. From this point of view, and assuming that the is not produced in association with any other particle, gluon-gluon fusion would be a more promising mechanism than annihilation (though the energy-dependence does not favour greatly this mechanism, and heavy annihilation would be preferred). Moreover, gluon-gluon fusion is favoured by historical precedent (the Higgs boson) and by Occam’s razor, since loops of heavy fermions could provide this production mechanism as well as the decay mode. Accordingly, in later sections of this paper we concentrate on the possibility that gluon-gluon fusion is the dominant production mechanism for the .

What fermions might generate the signal? The chirality of the Standard Model (SM) under the electroweak SU(2)U(1) gauge symmetries requires a Higgs boson to generate masses for elementary fermions, and electroweak precision tests exclude a fourth chiral generation of SM fermions at 7 [8]. Moreover, current bounds on the masses of new quarks from direct searches would require Yukawa couplings that is and hence unpalatably large. On the other hand, vector-like fermions could have gauge-invariant bilinear mass terms, , that are not tethered to the electroweak scale. However, by the same token, such a bilinear mass term poses an additional hierarchy problem. Explaining how and why vector-like fermions masses could be near the electroweak scale is a rich topic of research which we will not go into here, though we cannot resist remarking that their lightness may provide further motivation for supersymmetry (SUSY) or compositeness.

Setting aside this hierarchy problem, there is no known reason why vector-like fermions should not exist at or below the TeV scale. Indeed,
they appear in many theories of beyond the Standard Model (BSM) physics, and are sometimes even necessary. For example, even the
minimal supersymmetric extension of the SM (the MSSM) contains vector-like fermions in the form of the Higgsinos,
which are effectively a pair of vector-like lepton SU(2) doublets ^{2}^{2}2However, loops of
MSSM sparticles could not explain the signal..
In many string theories, such as D-brane theories [9]
or heterotic string compactifications [10], vector-like fermions occur quite frequently, often in complete vector-like families
with SM-like charges. From a bottom-up perspective, vector-like families are often found in composite Higgs
models [11, 12, 13, 14, 15, 16],
little Higgs models [17, 18, 19, 20], scenarios with warped extra
dimensions [21] and SUSY models beyond the
MSSM [22, 23, 24, 25, 26, 27, 28, 29, 30]. Recently, vector-like fermions have been considered in the context of the decay of a CP-odd scalar to vector bosons [31].

In this paper we take an agnostic attitude towards the possible origin and nature of vector-like fermions, and consider the following representative scenarios, always assuming that the is an SU(2) singlet: (i) is coupled to an SU(2)-singlet vector-like top partner, (ii) is coupled to an SU(2)-doublet vector-like quark partner, (iii) is coupled to a vector-like copy of a generation of SM quarks, i.e., one SU(2) doublet and two singlets, all with SM-like charge and hypercharge assignments, (iv) is coupled to a complete vector-like generation of SM-like quarks and leptons. We estimate the required coupling as a function of the masses of the vector-like fermions in these models, and we consider in each case their possible signatures, including indirect constraints from precision electroweak data, flavour physics and dark matter relic density as well as direct LHC searches for the decays of heavy particles.

The outline of this paper is as follows. In Section 2 we present a general analysis of the production of a scalar or a pseudoscalar with a mass GeV via gluon fusion through loops of massive vector-like quarks, and its subsequent decay via analogous loops, including also the possibility of massive vector bosons. If a single vector-like quark were to contribute, we find that it would require quite a large coupling. However, this requirement would be relaxed if there were more vector-like quarks, or if heavy bosons also contributed to the coupling. In Section 3 we introduce the four vector-like fermion models we consider. Section 4 we present some of the diboson decay signatures of these models, confronting them with the corresponding experimental sensitivities, and Section 5 summarizes our conclusions. Finally, in an Appendix we give details of the models in two-component notation for the vector-like fermions.

## 2 General Aspects of the Signal

The best-fit cross-section for the signal at 13 TeV can be estimated by reconstructing the likelihood, assumed here to be essentially Gaussian, from the 95% CL expected and observed limits as was done for the Higgs boson in [32]. We assume a resonance mass of 750 GeV and use the 95% CL ranges from ATLAS and CMS at 13 TeV [1, 2] and CMS at 8 TeV [7] (the ATLAS 8 TeV exclusions do not extend up to 750 GeV [6]). These are reported for narrow widths, which do not vary much at 750 GeV for widths below 10 GeV, as shown in Fig. 9 of [7]. The excess remains significant at both narrow and wide widths, with a slight preference from ATLAS for the latter but, given the limited information publicly available, here we combine the best fits for the reported narrow width exclusions as an indicative cross-section range.

Fig. 1 displays the resulting global function for the fit for the 750 GeV resonance production
cross-section times branching ratio at 13 TeV. The individual CMS (ATLAS) Run 2 results
are shown as blue (red) dashed lines
while the CMS Run 1 result is shown as a green dotted line, where we have rescaled from 8 TeV to 13 TeV as described in
detail below. The combination is displayed as a solid black line, with the best-fit cross-section value and 68% C.L.
range found using the method of [32] to be fb ^{3}^{3}3The method
of [32] assumes a Gaussian approximation to reconstruct the likelihood which, as they note,
becomes accurate only when the number of events . With the current limited data this estimate
deviates from an estimate based on Poisson statistics, but we use this method to give a rough indication of the signal cross-section
region of interest should the signal grow with more statistics, recognising that the formal error it yields is probably an
underestimate..

The particle could be produced by a or a intial state but, as already mentioned, we assume here the gluon-initiated production mechanism, which is better able to accommodate the increase of the signal significance from LHC Run 1 at 8 TeV to LHC Run 2 at 13 TeV.

It is important to take into account the increase in the background as well as the energy dependence of the signal in estimating the relation between the observations at Run 2 and the exclusion limits by Run 1 searches. We can quantify the increase in the signal significance via the double ratio

(2.1) |

where , , and are the cross sections of signal () and background (). If one rescales (2.1) with the appropriate integrated luminosities (/fb for Run 1 and /fb for Run 2) this ratio corresponds to the expected statistical increase in the number of standard deviations from the 8-TeV run to the 13-TeV run. We find that the increases for the two production mechanisms are

(2.2) |

These double ratios are largely insensitive to the mass of the resonance in a range of GeV, and to the spin and CP properties of the resonance, e.g. , and . The spin of the resonance alters the kinematics, though, leading to a different distribution in the rapidity bins.

We evaluated the background events by simulating the main irreducible background () using Madgraph [33] at LO and performed a cut , as well as . In principle, there are additional reducible backgrounds from + jet and dijet events, but Fig. 2 of [7] indicates that these are small compared with the irreducible background for invariant masses GeV. We estimated the NLO K-factor for a -initiated resonance by computing a heavy Higgs K-factor with MCFM [34]. This K-factor is , although its dependence roughly cancels out in the double ratio.

The cross-section excluded at the 95% CL by the absence of a signal in the CMS Run 1 data [7] is approximately 0.5-2 fb for a spin-zero resonance with mass in the range of 700-800 GeV. This Run 1 limit can be translated into a 95% CL upper limit on the allowed cross-section at 13 TeV using the value of :

(2.3) |

where we have used and . The excluded cross-section from CMS Run 1 depends on the assumed total decay width, with typically stronger limits for narrower widths, but the uncertainty in the signal-to-background ratio does not allow a more meaningful extrapolation from 8 to 13 TeV of the limits, other than the broad range of 2-8 fb that we calculated here, which seems completely compatible with the strengths of the signals reported by CMS and ATLAS. The 2 (8) fb exclusions by CMS Run 1 are shaded in light (dark) blue in Fig. 1, and we see that the combined best-fit cross-section is within sigma of the weakest exclusion. More data will be needed to answer whether there is a statistically significant incompatibility between the 8 and 13 TeV data that requires further explanation.

## 3 The Couplings to Vector Bosons

In the following we focus on a spin-zero particle, considering two options for the CP properties, namely a scalar and a pseudoscalar state. Possible UV origins of the scalar resonance are a dilaton [35] from the breaking of conformal invariance, or equivalently a radion [36] from an extra dimension. A pseudoscalar particle could also have several origins, e.g., an axion-like particle from the breaking of a Peccei-Quinn symmetry [37], or a pseudo-Goldstone boson from symmetry breaking in a composite Higgs model [38]. One could also contemplate the possibility that the resonance at 750 GeV is part of an extended Higgs sector, such as a 2-Higgs-doublet model (2HDM) that might originate from supersymmetry. Alas, in a 2HDM the coupling to fermions and gauge bosons is constrained, leading to a branching ratio to photons two orders of magnitude below what would be required to explain the signal. In this paper we consider a different approach, with new heavy fermions inducing the coupling of the resonance to gauge bosons.

Irrespective of the specific origin of the resonance, the couplings of a generic scalar and pseudoscalar to pairs of photons and gluons are described via dimension-five operators in an effective field theory (EFT):

(3.1) | |||||

Within the EFT, one can compute the partial widths of the to gluons and photons as

(3.2) |

where or . The total decay width is very small if we assume domination by these decays into gluons and photons. For example, in Fig. 2 we display contours of widths including only decays into gluons and photons for a typical model with a heavy vector-like quark of charge responsible for the loop-induced coupling, as a function of the mass of the quark and its coupling to the scalar. Although ATLAS reports that its significance is largest for a width of 6% of [2], the excess remains almost as significant for narrow widths. In the following we treat the decay width as a free parameter and plot the parameter space for both a narrow width as above and a wide width of 45 GeV.

The partonic production cross section has the standard leading-order expression

(3.3) |

and this gluon-fusion production cross-section can be rescaled to the proton-proton production cross-section by numerical factors determined by the gluon-gluon luminosity functions at the different energies. We find that at LHC13

(3.4) | |||||

where we have assumed that the branching ratio
, as the ratio among the couplings tends to be hierarchical:
.
We plot in Fig. 3 contours of the production cross-section times branching ratio in units of femtobarns,
as functions of the inverses of the effective couplings in units of TeV, for the two different decay width hypotheses.
The solid black line denotes our best-fit cross-section of 6.2 fb, which is very compatible with the observed excess,
while the light green (yellow) shaded region indicates 1 (2) sigma cross-sections ranging from 4.2 (5.2) to 7.2 (8.2) fb.
The fb bounds from Run 1 correspond to the light blue and dark blue shaded regions, and we see that the
potential signal in Run 2 requires a cross-section that lies within this uncertainty. Given the limited statistics,
the Run 1 and Run 2 data are quite compatible. We also show shaded in red the excluded region from dijet searches for decays into gluons [39], which only places weak limits on TeV ^{4}^{4}4The dijet limit is
obtained from the octet scalar limit in [39] rescaled to 13 TeV with an acceptance of %..

In the following Section we consider various models with loops of vector-like fermions to generate the EFT coefficients and , which we parametrize as a sum over vector-like fermions with mass and charge :

(3.5) |

where 0 for coloured (un-coloured) fermions. The contributions to the couplings of , to gluons can be computed by evaluating a simple fermion loop. The resulting coupling is proportional to the trace and axial anomaly for [5, 40, 36] and [41], respectively. In the next Section we present a set of models involving vector-like fermions and evaluate their effect on the diphoton signal as well as decays into other vector states, , and , using their matching to the EFT.

For example, in the scalar case, the contribution of a single heavy coloured fermion with charge to the EFT coefficient is as follows:

(3.6) |

By inspecting the expression above and the total cross section at LHC13 in Eq.(3.4), one can see that in order to get a cross section in the region of few fb with such a single coloured fermion one would require

(3.7) |

which indicates that this minimal scenario would require large couplings and/or a sub-TeV vector-like fermion. In more realistic vector-like fermion models, such as those described in the next Section, we expect more fermionic degrees of freedom to contribute to the production, which would then scale as

(3.8) |

where is the number of coloured fermions in the model. Moreover, the branching ratio to diphotons could be affected by the presence of new bosonic degrees of freedom. For example, one could think of incorporating the reported excess in massive dibosons at 2 TeV invariant mass [42] within this framework. This or any other massive would contribute to the decay of , but not to the coupling.

## 4 Models with Massive Vector-Like Fermions

### 4.1 Specifications of the Models

Having established the general viability of models in which loops of vector-like fermions generate production and its decay into , we now present four specific models, with the aim of studying their specific features, constraints and signatures that could serve to distinguish them. As already mentioned, in all these models we assume that the particle is an isosinglet.

Model 1:

In Model 1, we couple the to an SU(2)-singlet vector-like top-like quark. We define this top-like quark in two-component notation as

(4.1) |

which is to be compared with the in the SM:

(4.2) |

The charge and representation assignments in this model are shown in Table 1.

U(1) | SU(2) | SU(3) | |
---|---|---|---|

0 | 1 | 1 | |

1 | |||

1 | 3 |

Because of this choice of charges and representations, the SU(2)-singlet top-like quark can also couple via the SM Higgs field to all the left-handed SM charge 2/3 quarks, and via bilinear mass terms to all the right-handed SM charge 2/3 quarks, since no symmetry forbids these couplings. Assuming mixing to only the third generation of SM quarks, the Lagrangian is then

(4.3) | ||||

where .

The mass matrix for mixing between the vector-like states and the SM states can be written down in four-component notation as

(4.4) |

where we have defined with the appropriate Yukawa couplings in each case. We have used the fact that the mass term can be rotated away by choosing a field basis with an appropriate combination of and , and redefining the Yukawa couplings. This mass matrix is diagonalised by

(4.5) |

where

(4.6) |

For simplicity, we consider here the limit of small mixing.

Model 2:

In Model 2, we couple the to an SU(2)-doublet vector-like quark partner, defined in two-component notation as

(4.7) |

which may be be compared to a typical left-handed SM quark doublet:

(4.8) |

The charge and representation assignments in this model are shown in Table 2.

U(1) | SU(2) | SU(3) | |
---|---|---|---|

0 | 1 | 1 | |

2 | 3 | ||

2 | 3 |

Because of this choice of charges, the SU(2)-doublet vector-like quark can also couple via the SM Higgs field to the right-handed SM quarks, and via a bilinear mass term to the left-handed SM quarks, since no symmetry forbids these couplings. The Lagrangian is then

(4.9) | ||||

As in the singlet vector-like quark case, the bilinear mass term can be rotated away by choosing a basis with an appropriate combination of the quark fields and redefinitions of Yukawa couplings.

The mass matrix can then be written as

(4.10) |

The mass matrices can be diagonalised in the following way:

(4.11) |

and similarly for the down-type quarks:

(4.12) |

where

(4.13) |

As before, for simplicity, we consider here the limit of small mixing.

Model 3:

In Model 3 we take a vector-like copy of one generation of SM quarks, i.e., one SU(2) doublet and two singlets, with SM-like charge assignments. We then have a combination of the singlet vector-like top quark defined in Section 4.1, the doublet defined in Section 4.1, and a down-type singlet vector-like bottom quark, which can be written in two-component notation as:

(4.14) |

to be compared with the right-handed SM bottom quark

(4.15) |

The charge and representation assignments in this model are shown in Table 3.

U(1) | SU(2) | SU(3) | |
---|---|---|---|

0 | 1 | 1 | |

2 | 3 | ||

2 | 3 | ||

1 | |||

1 | 3 | ||

1 | |||

1 | 3 |

Although there is no symmetry forbidding bilinear mass terms coupling the vector-like SU(2) doublet to the SM doublet, and likewise coupling the vector-like SU(2) singlet to the SM singlet, these mass terms can be rotated away as we saw in the previous models. Therefore for notational ease, we drop those terms in the Lagrangian for Model 3. We do, however, now have couplings that mix the vector-like doublet with the vector-like singlet via the SM Higgs boson. The Lagrangian for this model is then:

(4.16) | ||||

The mass matrix can then be written as

(4.17) |

which can be diagonalised to find the mass eigenstates. In the limit where , the vector-like quarks can still decay into the SM quarks, and precision constraints are no longer relevant. Since we require only that the couplings be large enough for the decay to occur promptly, we assume that our model lives in this regime. Then we are most interested in the mass eigenstates of the vector-like quarks themselves, taking into account the couplings . The mass matrices can then be written as

(4.18) |

and the mass eigenstates are then found by rotating

(4.19) |

and analogously for the down-type quarks, with angle . The solutions for the angles are

(4.20) |

and the mass eigenvalues are given by

(4.21) | ||||

(4.22) |

Model 4:

In this model we consider adding vector-like copies of a full generation of SM fermions. The particle content is therefore the same as in
Model 3, with the addition of a doublet of vector-like leptons and a singlet vector-like electron partner. This model can be thought of as
adding vector-like pairs of and in the language of SU(5) grand unification. An extension,
which we will also consider below, is to add a neutral vector-like partner, which is a pair of singlets under SU(5). This can be thought of as adding a
in the language of SO(10). One motivation for adding the neutral vector-like state is that it could provide a natural dark matter (DM) candidate if it is stable. We note that renormalization effects would typically give positive corrections to the masses of
the and states in these multiplets ^{5}^{5}5On the other
hand, in a SUSY version of this scenario, the lightest supersymmetric particle would also be a natural dark matter candidate.. Since the neutral singlet plays no role in the production of or its decay, the model is recovered by setting the couplings and mass to zero. In this case the neutral component of the doublet, could provide a DM candidate if it is stable.

Rather than reproduce the Lagrangian from Model 3, we write here only the terms for the lepton content of Model 4. We define the vector-like doublet as

(4.23) |

and the vector-like singlets as

(4.24) |

The charge and representation assignments in this model are shown in Table 4, where is the third-generation charged SM lepton.

U(1) | SU(2) | SU(3) | |
---|---|---|---|

0 | 1 | 1 | |

2 | 3 | ||

2 | 1 | ||

1 | |||

1 | 1 | ||

1 | |||

1 | 1 |

We mirror our approach for the quarks by only including couplings to the third generation. We may then write down the most general Lagrangian, again taking advantage of the fact that we can rotate away the vector-like-SM mixing mass bilinear by an appropriate redefinition of fields and Yukawa couplings:

(4.25) | ||||

We note that, by including the neutral vector-like singlet, one could introduce an explicit Yukawa coupling to give mass to the SM left-handed neutrino. There are very stringent bounds on this Yukawa coupling, forcing it to be [8], so in our analysis we assume it to vanish, and we may then write the mass matrix as

(4.26) |

As for the quark sector in Model 3, we can consider the limit without compromising the ability of the vector-like partners to decay promptly. In this limit, the mass matrices reduce to mixing only among vector-like partners:

(4.27) |

The mass eigenstates are then found by rotating

(4.28) |

and analogously for the neutral leptons, with angle . The solutions for the angles are

(4.29) |

and the mass eigenvalues are given by

(4.30) | ||||

(4.31) |

The lighter of the two neutral leptons could be a dark matter candidate if it is stable. It is precisely this observation which leads us to have written down the couplings between the neutral vector-like lepton and the hypothetical or fields, because while they do not contribute to the production or decay of /, they would be important for the calculation of the relic density. Models involving a radion, like our particle, and axion, i.e., , have been studied elsewhere, see, e.g., Refs [43, 44, 45, 46], and in this case the main annihilation would be to gluons:

(4.32) |

This annihilation is p-wave suppressed for the case of the scalar and s-wave for the pseudoscalar candidate. The annihilation cross section for the pseudo-scalar is given by

(4.33) |

We note that a large cross section for annihilation into gluons could in principle be probed in direct detection experiments, although the limits degrade steeply with the dark matter particle mass, and above 300 GeV it is out of reach of the XENON1T that is now starting [47] .

### 4.2 Summary of Vector-Like Models

For the reader’s convenience, we present here a short summary of each model we consider. We list in Table 5 the new field contents of the various models, now in four-component notation.

Model | Field content | U(1) | SU(2) | SU(3) |

All models | X | 0 | 1 | 1 |

1, 3 & 4 | +2/3 | 1 | 3 | |

-2/3 | 1 | |||

2, 3 & 4 | +2/3 | 2 | 3 | |

-2/3 | ||||

2, 3 & 4 | -1/3 | 2 | 3 | |

+1/3 | ||||

3 & 4 | -1/3 | 1 | 3 | |

+1/3 | 1 | |||

4 | 0 | 2 | 1 | |

0 | ||||

4 | -1 | 2 | 1 | |

+1 | ||||

4 | -1 | 1 | 1 | |

+1 | 1 | |||

4 | 0 | 1 | 1 | |

0 | 1 |

If we assume, for simplicity, a degenerate spectrum for each model, and universal couplings, we can easily quantify the predicted branching ratios for each decay mode of the particle as a function of the number of fermions and their charges under . The couplings are as follows

(4.34) |

where , , with the weak mixing angle, and . The coefficients are given by

(4.35) |

where is a triangle loop function, and and are the hypercharge and Dynkin index of the representation of the fermion , respectively. The triangle loop function is defined as

(4.36) |

where . In the limit we consider where , . The contribution to the gluon coupling can be obtained in a similar way as the other couplings. We use these expressions to obtain the ratios of partial widths to vector bosons in the various models listed in Table 6.

Model | ||||||
---|---|---|---|---|---|---|

1 | 0 | 180 | 1.2 | 0.090 | 0 | |

2 | 3 | 460 | 10 | 9.1 | 61 | |

3 | 3 | 460 | 1.1 | 2.8 | 15 | |

4 | 4 | 180 | 0.46 | 2.1 | 11 | |

Current limit | 7 | 13 | 30 |

In Fig. 4 and Fig. 5 we display the contours of production cross-section times branching ratio, with the 1- and 2-sigma bands in light green and yellow denoting the favoured region by a global fit to the ATLAS and CMS data and the dark (light) blue regions the weakest (strongest) exclusions at 95% CL by Run 1 of CMS. Fig. 4 assumes a photon and gluon dominated branching ratio with a narrow width, and we see that models 1 and 2 must be in a strongly-coupled and/or relatively low mass regime to obtain a large enough signal cross-section. This is alleviated somewhat in model 3 with the larger number of fermion contributions, and model 4 is a fully perturbative weakly-coupled model.

We note, in particular, that Model 4 contains a dark matter candidate, and we show the relic density constraint [49] by a red dashed line in the lower right panel of Fig. 4. For a large range of dark matter particle masses, this contour lies within the bands favoured at the 1- and 2- level.

On the other hand, Fig. 5 assumes a large width corresponding to 6% of the 750 GeV resonance mass ^{6}^{6}6We do not address the model-dependent issue what additional modes might dominate decays in this case.
These might be induced by small couplings to some Standard Model particles such as , which would be allowed by experimental constraints as discussed in [48], or there might be
invisible decays., which excludes all of model 1 and 2 for and practically all of Model 3. Only model 4 survives in a corner of the parameter space with strong coupling. There is therefore a tension between increasing the decay width and perturbativity for the models we consider here. Moreover, the relic density constraint [49] indicated by the red dashed line does not traverse the 1- and 2- bands.

### 4.3 Present and Future Constraints on Vector-Like Partners

The charged vector-like fermions are not stable, and decay via small Yukawa couplings to the Standard Model fermions via the SM Higgs boson. As such, a vector-like partner can have either a prompt or a displaced decay. If the decay is to be prompt, which we define as m, then we can place a limit on GeV [50]. If we assume couplings only to the third generation of SM fermions, then there are no applicable constraints due to induced tree-level FCNC decays such as or . The constraints in the case of mixing with the third generation arise from the oblique parameters and (), the coupling and the modification of . In the limit where mixing with the SM is small, however, these constraints no longer apply[51, 52]. Since our models do not need large couplings to the SM, but just require that the decay occurs, the constraints on mixing with the SM particles are not strong in our models.

In Models 3 and 4 however, there are relevant constraints from the electroweak oblique parameters and (), due to mixing between the vector-like states themselves via the SM Higgs, which we calculate using the results of [50]. We show in Figs. 7 and 7 our results for Model 4. (The results for Model 3 are quite similar.) It is important to note that the central values from the GFitter collaboration for and (after fixing ) exclude the SM at more than the 68 % C.L. [53]. Therefore, even in the large-mass decoupling limit for the vector-like states, the contours of regions allowed by and never drop below the 68 % C.L. contour for either model.

Another constraint that should be taken into account is the effect of adding vector-like fermions that mix with the SM Higgs on the Higgs couplings themselves. This has been studied in various guises (see for example [57, 58, 59, 50, 60]), finding that even for relatively large mixing between the vector-like fermions, it is possible that the Higgs couplings are not shifted dramatically, so they can be compatible with experimental bounds.

Searches for coloured vector-like quarks have been performed at Run 1 by ATLAS [55]
and CMS [56] (vector-like tops only) reaching about 800 GeV.
The increase of production from 8 TeV to 13 TeV is for the region of 900 to 1200 GeV,
but the backgrounds grow at a similar rate. Nevertheless, boosted techniques and more efficient
multivariate discrimination techniques may lead to a Run 2 sensitivity to vector-like quarks around 2 TeV
for models with coloured particles, see e.g., Ref. [61] for a recent study.
However, the current LHC limits on vector-like quarks are already sufficient to push the fermionic form factor
(4.36) close to its asymptotic value ^{7}^{7}7The same would be true for any massive that
might contribute to the vertex. We note that, unlike the case of the Higgs boson where
the relative signs of fermion and boson loops are opposite, the same is not necessarily the case for
their contributions to the vertex, where they may interfere constructively..
The same is not necessarily the case for any vector-like leptons, but we
assume it here, for simplicity.

## 5 Other Searches for at LHC Run 2

We now recast the constraints that have been established by the ATLAS and CMS Collaborations
on diboson final states in the context of heavy SM Higgs boson searches.
We concentrate on the experimental analyses that provide the most constraining results for a state of mass GeV.
Since we are assuming the the couplings of the X resonance to the SM fermions are small,
we focus on possible X decays to SM gauge bosons, or to the Higgs boson, or to both of them.
With regard to the exploitation of the experimental analyses of a heavy Higgs
boson , , we note that the vertex for an electroweak singlet decaying into a pair of gauge bosons
given in (3.1) is different from that of a Standard Model-like Higgs boson.
In the case studied here of a CP-conserving spin-0 field, , decaying into a pair of on-shell
spin-1 particles with masses much smaller than via an or
vertex,
there is only one possible helicity amplitude ^{8}^{8}8Processes involving at least one off-shell boson, such
as the production of the boson in association with a gauge boson, would provide good opportunities
to distinguish between Lorentz structures [62]., yielding final states split equally
between helicity states.
Consequently, the kinematics of such an electroweak singlet decaying to pairs of gauge bosons
should be different from the case of a heavy Higgs boson, where also zero-helicity states may be produced.
However, we have checked that the differences in acceptance are at the 10 to 15% level for both the and
final states, and are not important for our purposes.

Limits can be borrowed from searches for a heavy SM Higgs boson in its decays to massive gauge bosons . The search for , and channels, have been performed in the framework of the SM with the full event sample recorded at the LHC run 1, namely 5.1 fb at TeV and 19.7 fb at TeV for CMS [63] and 20.3 fb at TeV for ATLAS [64]. The mass range analyzed extended to TeV. One should note that in a dedicated X search, this channel will lead to more effective constraints as heavy SM Higgs particles have total decay widths that are completely different, a priori. Whereas the SM state would have been a very wide resonance (for a mass GeV the total decay width is GeV), the boson might be a relatively narrow resonance as discussed previously, allowing one to select smaller bins for the invariant masses that lead to a more effective suppression of the backgrounds. CMS expressed their result in term of a ratio between the number of observed events relative to the SM expectation. Translated into cross-sections, the observed CL limit for a GeV SM-like resonance reads: . This experimental limit gives then a upper value on the production cross section of the particle decaying to bosons during LHC Run 1 that is

which can be re-written in the form fb. We have seen previously that LHC Run 1 put a upper limit of order 1 fb for the production cross section times its branching ratio to photons. Therefore, we end up with a first crude estimate that . ATLAS results give the CL upper limit