Signals of a 2 TeV $W'$ boson and a heavier $Z'$ boson

We construct an $SU(2)_L\times SU(2)_R\times U(1)_{B-L}$ model with a Higgs sector that consists of a bidoublet and a doublet, and with a right-handed neutrino sector that includes one Dirac fermion and one Majorana fermion. This model explains the Run 1 CMS and ATLAS excess events in the $e^+e^-jj$, $jj$, $Wh^0$ and $WZ$ channels in terms of a $W'$ boson of mass near 1.9 TeV and of coupling $g_R$ in the 0.4--0.5 range, with the lower half preferred by limits on $t \bar b$ resonances and Run 2 results. The production cross section of this $W'$ boson at the 13 TeV LHC is in the 700--900 fb range, allowing sensitivity in more than 17 final states. We determine that the $Z'$ boson has a mass in the 3.4--4.5 TeV range and several decay channels that can be probed in Run 2 of the LHC, including cascade decays via heavy Higgs bosons.

of this model, using Monte-Carlo simulations, and extract the region of parameter space consistent with the observed deviations from the SM. We find that simulations of different W decay channels are required for this extraction due to contamination among signals.
In Section 2 we describe the model, we extract the value of the W coupling consistent with the CMS dijet excess [2], and we compute the W width and production cross section.
In Section 3 we discuss the right-handed neutrino sector, and we show that the CMS e + e − jj excess is accommodated for a range of right-handed neutrino masses. W decays into pairs of bosons are analyzed in Section 4. The properties of the Z boson are studied in Section 5. Our conclusions are summarized in Section 6.

W width and production cross section
We consider an SU (3) c × SU (2) L × SU (2) R × U (1) B−L gauge theory with the field content shown in Table 1. The right-handed neutrinos N i R (i labels the three generations) acquire masses at the TeV scale through the mechanism of Ref. [11], also discussed in section 3. The Higgs sector includes an SU (2) R doublet H R whose VEV, of several TeV, breaks SU (2) R × U (1) B−L down to the SM hypercharge group U (1) Y , and a bidoublet Σ whose VEV breaks SU (2) L × U (1) Y at the weak scale.
The only gauge fields beyond the SM are a W boson and a Z boson, which acquire masses primarily due to the H R VEV. For M W ≈ 1.9 TeV, as indicated by the 8 TeV LHC data, the Z boson has a mass of a few TeV (discussed in Section 5). The VEV of the  with the W L − W R mixing angle θ + given by [8] The parameters introduced here are as follows: g R is the SU (2) R gauge coupling, g ≈ 0.63 is the SM weak coupling at 2 TeV, and the angle β arises from the usual tan β ratio of VEVs in the Two-Higgs doublet model, which is the manifestation of the bidoublet scalar Σ below the SU (2) R breaking scale.
The couplings of the W boson to pairs of SM fermions, neglecting the W L − W R mixing, are given by 3) The quark fields here are in the mass eigenstate basis. Flavor-dependent perturbations to the above interactions are allowed by the SU (2) R gauge symmetry, but are constrained by measurements of flavor processes such as K −K meson mixing, and we assume here that they are negligible.
The couplings of the W boson to pairs of SM bosons are fixed by gauge invariance and take the form [8]: where c W ≡ cos θ W ≈ 0.87 (θ W is the weak mixing angle at the M W scale), and [µ, ν] represents the commutation of Lorentz indices. The W Z and W h signals (see Section 4) indicate 0.36 tan β 2.8. The agreement between the SM predictions and the measured properties of h 0 requires the mixing angle between the neutral CP-even Higgs bosons, α, to be near the alignment limit. The amount by which the mixing deviates from the alignment limit is δ = β − α − π/2 1.
The W partial widths into SM particles induced by the couplings shown in Eqs. (2.3) and (2.4) are given by [8] The phase-space suppression factors (ignored here) give corrections of order TeV. The next-to-leading order (NLO) QCD corrections (included here) are of order 3%, with α s ≈ 0.1 being the QCD coupling constant at the M W scale.
Besides the branching fractions into SM particles, the W boson can decay into a right-handed neutrino and an electron or τ , and also into two heavy Higgs bosons or one heavy Higgs boson and one SM boson. The absence of µµjj signals in Run 1 of the LHC [1,13] implies that the second-generation right-handed neutrino is heavier than (or nearly degenerate to) the W .
The increase of the total width due to decays involving right-handed neutrinos (see Section 3) is between 4% and 12% (depending on the masses of right-handed neutrinos); an additional increase of up to 6% is due to decays involving heavy Higgs scalars (discussed in Section 4). Including these contributions, and taking the range for tan β into account, the total W width is The W coupling g R can be determined from the cross section required to produce the dijet resonance near M W . The CMS dijet excess [3] at a mass in the 1.8-1.9 TeV range indicates that the W production cross section times the dijet branching fraction is in the 100-200 fb range (this is consistent with the ATLAS dijet result [14], which shows a smaller excess at 1.9 TeV) 1 . This was assumed in Refs. [6,17] to be the range for where j is a hadronic jet associated with quarks or antiquarks other than the top. We point out here that the large W mass implies that the CMS dijet search is also sensitive to merged jets arising from the decays of boosted top quarks and boosted W , Z or h 0 bosons produced in W decays. 1 The CMS [15] dijet search with 2.4 fb −1 of Run 2 data has a small excess (less than 2 σ) in the 1.7-1.8 TeV range that may be consistent with the Run 1 excess. The ATLAS [16] result with 3.6 fb −1 of Run 2 data has no excess in the 1.8-2 TeV range, and sets a 95% CL upper limit on the dijet production cross section of around 300 fb at M W = 1.9 TeV. Reinterpreting this limit in our model we find g R 0. 44. To see that, note that the CMS search [3] identifies a narrow jet of cone ∆R ≤ 0.5, and then includes all hadronic activity in a wider cone of ∆R ≤ 1.1. This procedure is designed to collect all the radiation associated with the jet so that the invariant mass distribution is properly calibrated. An additional consequence of this procedure is that it cannot separate W decays into two light jets from those into heavy SM particles that decay hadronically.
Consider first the W → tb channel. The case where the top quark decays hadronically implies that there is a narrow b jet back-to-back to a merged jet formed of three jets. As the CMS search is not using b-tagging, and the merged jet is typically much narrower than ∆R = 1.1, this topology will contribute to the dijet peak near M W .
The case of semileptonic top decays is more complicated. The lepton is almost collinear with the jet arising from the top decay so that it usually does not pass the isolation requirement. The missing transverse energy carried by the neutrino is typically large enough to move the invariant mass of the system formed by theb jet and the lepton-plusb jet to values significantly lower than M W . Thus, the fraction of W → tb decays that contribute to the dijet peak near M W is expected to be roughly given by B(W → jj) ≈ 67.4%. This would imply that combining the W → tb and W → jj processes increases the number of dijet events by ∼ 34% compared to the W → jj process.
To improve this estimate, we have implemented the interactions (2.3) and (2.4) in FeynRules [18], which automatically generated the MadGraph [19] model files available at [20]. Using the Delphes [21] detector simulation and the NN23LO1 parton distributions [22], we find that W → tb increases the number of dijet events that pass the selection cuts and have an invariant mass above 1.7 TeV by 37% compared to W → jj by itself.
A similar discussion applies to W → W Z or W h 0 . Events in which both the W and Z decay hadronically contribute to the dijet peak. These represent B(W → jj)B(Z → jj) ≈ 47.1% of all W → W Z events. In the case of W → W h 0 , the purely hadronic decays lead to a W merged jet back-to-back to a Higgs merged jet. The fraction of W → W h 0 events that contribute to the dijet peak near M W is expected to be B(W → jj)B(h 0 → jj, 4j) ≈ 54.1%, where B(h 0 → jj, 4j) ≈ 80.2% is the total hadronic branching fraction of the SM Higgs boson for M h = 125 GeV [23]. Note that decays involving taus include missing energy so that their contribution to the dijet peak near M W is suppressed.
Our simulations show that the contributions from W → W Z and W h 0 to the dijet peak are larger than the above estimates. However, given the small branching fractions of these modes, the increase in the number of dijet events that pass the selection cuts and have an invariant mass above 1.7 TeV is only 4%.
Finally, the W decays to heavy Higgs bosons (if kinematically open) also contribute to the dijet signal. The main channels, W → H ± A 0 and H ± H 0 , followed by H + → tb and A 0 /H 0 → tt give two merged jets: one containing W bb and the other one containing W + W − bb. When these three W bosons decay hadronically (a 31% combined branching fraction), the reconstructed mass of the two merged jets is again near M W .
Summing over all these modes, we find that the total branching fraction of decays contributing to the dijet peak near M W is B(W → dijet) ≈ 81 − 89%, with the uncertainty arising mainly due to the right-handed neutrino masses. The total production cross section at √ s = 8 TeV required to explain the dijet peak is This observed range needs to be compared with the predicted cross section. For M W = 1.9 TeV, the leading-order W production cross section at √ s = 8 TeV, computed with MadGraph, is 155 fb (g R /0.5) 2 . Next-to-leading order QCD effects can be taken into account by multyplying the leading-order cross section by K 8 (W ) ≈ 1.15 [24] (this is consistent with the result of an MCFM [25] computation, but somewhat smaller than the K-factor computed in [26]). Thus, the predicted cross section is Combining this with Eq. (2.6) implies a total width Γ W = 20-48 GeV. Note that combining Run 1 and Run 2 dijet results reduces the required production cross section, but there is a theoretical lower bound g R > g Y ≈ 0.363 (see section 5).
Searches for tb resonances using LHC Run 1 data impose a stronger upper limit on g R . The semileptonic top decay is used by CMS [27] to set a cross section limit σ(pp → W → tb) < 100 fb at the 95% CL. The hadronic top decay leads to a stronger CMS limit [28]: σ(pp → W → tb) < 60 fb at the 95% CL. The combination [28] of these two tb final states gives σ(pp → W → tb) 40 fb for M W = 1.9 TeV. This implies g R 0.45.
The ATLAS searches using semileptonic [29] and hadronic [30] top decays impose weaker upper limits on σ(pp → W → tb), of 120 fb and 210 fb, respectively. The discrepancy between the CMS and ATLAS tb sensitivities in the case of hadronic top decays is due in part to the b tagging efficiencies, which are not well understood in the case of the large jet p T associated with a resonance near 2 TeV.
The W production at the 13 TeV LHC is 6.3 times larger than in Run 1, taking into account a K-factor of K 13 (W ) ≈ 1.2 [31]. For 0.4 < g R < 0.44 the Run 2 production cross section lies between 720 and 875 fb. Consequently, the existence of the W can be tested in the W → jj and W → tb channels with O(10) fb in Run 2.

W → eN D and N D decay widths
responsible for the right-handed neutrino masses. In this Section we analyze a mechanism that allows the three right-handed neutrinos to acquire masses consistent with the CMS e + e − jj excess [1] and the lack of a signal in related LHC searches (especially in the samesign eejj final state [32]). This mechanism does not require any field of mass below the Table 1. This relies, though, on higher-dimensional operators whose origin requires additional fields (discussed at the end of this Section) that have masses below ∼ 20 TeV.
Let us consider the following lepton-number-violating dimension-5 operators: The flavor structure of these operators is a consequence of the flavor symmetry introduced in [11]: a global U (1) symmetry with L e R , L µ R , L τ R carrying charge −1, 0, +1, respectively. All other fields shown in Table 1 have global U (1) charge 0. Replacing the SU (2) R doublet H R by its VEV in Eq. (3.1) leads to the following mass matrix for right-handed neutrinos: Although these are Majorana masses, the N e R and N τ R fields form a Dirac fermion [11], labelled here N D . This has a mass m N D = C eτ u 2 H /m eτ ψ , and its left-and right-handed components are given by N D L ≡ (N τ R ) c and N D R ≡ N e R , respectively. The muon righthanded neutrino N µ R remains a Majorana fermion of mass m N µ = C µµ u 2 H /m µµ ψ . The couplings of the W boson to the Dirac fermion N D , or the muon right-handed neutrino N µ R , and the SM charged leptons in the mass eigenstate basis follow from the SU (2) R gauge symmetry: where the W coupling g R is the same as in Eq. (2.3).
As no µµjj signal has been observed yet, we will assume the following mass hierarchy: As a result, the W → µ N µ decay is kinematically closed or strongly phase-space suppressed, and we will ignore the presence of N µ R in what follows. The W partial widths into a SM lepton and an N D Dirac fermion follow from Eq. (3.3): The W couplings shown in Eq.
For m N D close to M W one has to use the exact formula for this width given in the Appendix. The width for N D → e − tb is smaller: where the phase-space suppression is included in There is also a 2-body decay on N D , proceeding through the small W L − W R mixing: (3.8) 600 800 1000 1200 1400 1600 1800 0 The W couplings shown in Eq. (3.3) imply that the decays of N D involving τ 's have opposite charges compared to the decays involving electrons [11]. The N D → τ + W * → τ +ū d or τ +c s widths are equal to that given in Eq. The branching fraction of the N D 3-body decay into ejj is where we ignored terms of order M 4 W /m 4 N D . Multiplying this branching fraction by B(W → eN D ) we obtain the total branching fraction shown in Figure 1.
Let us compare the CMS e + e − jj signal [1] with the predicted rate for pp → W → eN D → e + e − jj. The acceptance-times-efficiency of the CMS event selection, estimated through our simulation, for events with eejj mass above 1.8 TeV arising from the 3-body decay N D → ejj decreases from 32% to 26% when m N D grows from 0.5 TeV to 1.6 TeV. The analogous acceptance-times-efficiency ranges for N D → etb and N D → e − W + are 28%-21% and 8.4%-7.2%, respectively. Given that there are 10 excess events, and the luminosity is 19.7 fb −1 , we obtain a central value for the signal cross section of 0.84 Integrating out the ψ L fermions gives the operators (3.1), with coefficients C eτ = y eψ y τ ψ and C µµ = y 2 µψ .

Bosonic W decays
In addition to the couplings to SM particles (see Section 2) and to right-handed neutrinos (see Section 3), the W also has couplings to the heavy Higgs bosons present in the Σ bidoublet (H ± , H 0 , A 0 , as in Two-Higgs-doublet models) and in the H R doublet (a single neutral scalar, h 0 R ). These couplings are due to the kinetic terms of the scalar fields and are determined by gauge invariance. For simplicity we assume that the Σ VEV is CP invariant, and that h 0 R scalar is heavier than the W boson. The W coupling to the W and a heavy neutral Higgs boson arises (up to negligible corrections of order M 2 W /M 2 W ) from the kinetic term of Σ: By contrast, the kinetic terms of Σ and H R have comparable contributions to the W coupling to the Z and the heavy charged Higgs boson, with the sum given by The W couplings involving two charged Higgs bosons are, again, almost entirely due to the Σ kinetic term: The W partial widths induced by the above couplings are corrections to each of these are given in [8]. As expected, the partial widths to modes related by Goldstone equivalence are equal, up to kinematic factors that have been ignored here. The W branching fractions are displayed as a function of tan β in Figure 3. (J is a merged jet arising from a boosted W or Z) corresponds to 13 observed events of invariant mass 1.85 TeV ≤ m JJ ≤ 2.05 TeV, with an expected background of 5 events.
In a related CMS analysis [34], which does not attempt to distinguish between W and Z merged jets, there is a smaller 1.3σ excess. If the ATLAS diboson excess is due to a W decaying into W Z followed by hadronic decays of W and Z, then excess events should eventually also appear in other W Z decay channels at the same mass.
The branching fraction for W → W Z → ν is too small to be useful in Run 1 (we expect less than 1 event to be observed in 20 fb −1 of 8 TeV data). The semileptonic channels, W Z → νJ and W Z → J + − , however, are as sensitive to a W as the W → W Z → JJ channel. The CMS search in the W Z → J + − channel has indeed yielded a 2σ excess at a mass in the 1.8-1.9 TeV range, while the CMS search in the W Z → νJ channel, which is slightly more sensitive, has only a 1σ excess in that mass range. The ATLAS searches in the semileptonic channels, however, are in good agreement with the background estimate. Given that the sensitivity in all these channels is comparable, the ATLAS W Z → JJ result is in conflict at more than 2σ with the ATLAS combination of W Z semileptonic and leptonic channels [35]. This discrepancy may be due to a statistical fluctuation. We point out, however, that the resolution of this issue may be more convoluted. It may not be possible to analyze the W Z channels separately from other W decay modes.
Consider first the W → jj channel. The hadronic jets produced by a light quark have invariant masses that may be much larger than mass of the initial quark. Some of these jets may resemble a boosted W or Z decaying hadronically. Through simulation, we estimate that approximately 1% of the jj events give two jets with jet masses close to the W or Z mass. Even if ∼ 40% of these jets fail jet grooming requirements [5], the branching fraction for W → jj is ∼ 30 larger than for W → W Z and so this mode contributes a significant number of events to the JJ signal. A precise simulation of the event selection and detector effects in this channel is beyond the scope this work, but can be performed by the ATLAS and CMS collaborations.
Similarly, contributions to what appear to be W → W Z → JJ events may be due to other W signals, including It is tempting to speculate that the whole ATLAS diboson excess is due to these other signals, in which case there would be no lower limit on the W → W Z branching fraction (or equivalently on sin 2 2β). However, the CMS W Z → J + − excess seems to contradict this possibility. Furthermore, the CMS search [2] for a W h 0 resonance, with W → ν and h 0 → bb has a 2.2σ excess, corresponding to 3 events with W h 0 invariant mass between 1.8 TeV-1.9 TeV and 0.3 background events. In the alignment limit, the W Z and W h 0 branching fractions are equal, so these observations place a lower limit on sin 2 2β. The pp → W → W Z cross section that would account for the W Z → J + − and W h 0 → νbb events is roughly in the 5-10 fb range, assuming the selection acceptance-times-efficiency for W h 0 to be similar to that of W Z → JJ, 0.1 ≤ A × ≤ 0.2 [5]. This cross section indicates that these modes may have undergone a slight upward fluctuation and that sin 2β must be close to maximal. Assuming that the entire JJ excess does come from the W Z final state places a similar constraint, 0.5 tan β 2.0 for g R = 0.4, and 0.36 tan β 2.8 for g R = 0.5.
Recently, at Run 2 of the LHC, there have been searches for diboson final states.
CMS, using 2.6 fb −1 of data, have searched for a resonance in both the νqq and JJ final states [36], while ATLAS, using 3.2 fb −1 of data, have searched in the JJ final state [37]. Neither experiment has more than a 1σ excess in the region of M W ≈ 1.9 TeV. The CMS result places the strongest constraint: g R 0.46 at M W = 1.9 TeV. This bound is comparable to that coming from the Run 2 ATLAS dijet resonance search [16], which is sensitive to the W → jj channel. The W h resonance search at Run 2 [38] has a small (∼ 1.5σ) excess at M W = 1.9 TeV, consistent with the W h excess at the same mass in Run 1 [2].
Another interesting diboson channel is W → W Z followed by Z → νν and W → jj [39]. As the W and Z bosons are highly boosted, the first channel would appear as missing transverse energy (E T / ) and a merged jet (J) of mass near M W whose p T is back-to-back with the E T / . The invariant mass distribution of the J + E T / system ("merged mono-jet") has a plateau-like shape that extends between a few hundred GeV and M W . The monojet searches [40,41,42] have produced an excess of events that may have a shape of this type, but it is too early to draw a conclusion as to whether its origin is new physics. With an increase in data, this will be an interesting search channel both in merged mono-jet and using sub-structure techniques.
There are additional diboson channels that, with more accumulated luminosity, will provide nontrivial tests of the W properties. These involve some of the smaller W , Z, or h 0 branching fractions. Final states involving three or more leptons receive contributions from multiple topologies, each with different kinematics, e.g., W → W Z → ν and W → W h 0 → ν ν ν. Both W Z and W h 0 give contributions to final states with three taus.
Besides decays to SM bosons, W bosons can generically decay into the heavy scalars associated with the Higgs sector responsible for breaking the extended gauge symmetry [43]. In the model discussed here, the W decays into heavy Higgs bosons leads to toprich final states, e.g., W → H + A 0 → tbtt. As was pointed out in [8] these final states have the potential to explain the ATLAS same-sign leptons plus b-jets excess [9]. Due to differences in the structure of the right-handed neutrino sectors discussed here and in [8], the relative contributions from heavy Higgs and heavy neutrinos to the same-sign leptons plus b-jets final state is slightly altered.

Properties of the Z boson
In addition to the electrically-charged gauge bosons, W ± L and W ± R (whose linear combinations give the W and W bosons), the SU (2) L × SU (2) R × U (1) B−L gauge fields include three electrically-neutral bosons: W 3µ L , W 3µ R , A µ B−L . Two linear combinations of these acquire masses due to the scalar VEVs, and become the Z and Z bosons, while the third linear combination is the photon.
The VEVs of the bidoublet Σ and of the SU (2) R doublet H R have the form where v H √ 2M W /g ≈ 174 GeV is the weak scale, and the SU where g L g is the SU (2) L gauge coupling, and g B−L is the U (1) B−L gauge coupling, which is related to the SM hypercharge gauge coupling (g Y ≈ 0.363 at 2 TeV) by The mass terms in Eq. (5.3) lead to a 3×3 mass matrix of rank 2, which is diagonalized by the following unitary transformation that relates the photon (A µ ) and the Z and Z bosons to the SU (2) L × SU (2) R × U (1) B−L gauge fields: where we kept only the leading order in M 2 W /M 2 Z for each element of the matrix. In analogy to the SM s W ≡ sin θ W , we defined s R ≡ sin θ R and c R ≡ cos θ R , with which implies a simple relation between θ R and g R : The mass of the Z boson is related to the W mass by As the ranges for M W and g R can be derived from the W signals, a range for M Z can be predicted. We will show, however, that a more stringent lower limit on M Z in this model is imposed by Z searches in Run 1 of the LHC.

Z branching fractions
The coupling of the Z boson to a chiral fermion ψ is determined by the fermion's hypercharge (Y , in the normalization where the hypercharge of weak singlets equals their electric charge) and SU (2) R charge (T 3 R ), and is given by As a result, the tree-level Z decay widths into lepton pairs are We assumed here that the Z → N µ RN µ R channel is kinematically closed. The Z decay widths into quark-antiquark pairs are the same for the three fermion generations (the m 2 t /M 2 Z corrections are negligible), and given by The Z also couples to pairs of gauge and Higgs bosons. The triple gauge boson couplings are fixed by gauge invariance, and the Z W W coupling is The decay width is If heavy enough, i.e. c R < 1/2, the Z can decay to a pair of W bosons, 14) The Z has couplings to the five Higgs bosons coming from the Σ bidoublet (h 0 , H 0 , A 0 , H ± ) as well as the single scalar (h 0 R ) left after the doublet H R VEV breaks SU (2) R × U (1) B−L to U (1) Y . We will assume that h 0 R is too heavy to be involved in Z decays. The relevant couplings controlling the decay of Z to final states involving two Higgs bosons If all the heavy Higgses are lighter than M Z /2 the decay widths that survive in the alignment limit are where we assumed as in Section 4 that M A 0 M H 0 M H + . The couplings of the Z to one Higgs boson and one gauge boson are 17) and the corresponding width is There are two further modes that are negligible in the alignment limit, The decays to H + W − , H + W − and W W are suppressed by M 2 Z /M 2 Z , and so are too small to be of interest at present. There are also 3-body decays that have small branching fractions and we ignore here. the M Z mass range can be ruled out. To derive the lower limit on M Z , we require less than three predicted Z → + − events in the dilepton searches performed by ATLAS [46] and CMS [47] taken together. The Z production cross section at the 8 TeV LHC, obtained by multiplying the MadGraph result with K(Z ) = 1.16 [46], decreases from 1.6 fb for M Z = 2.8 TeV to 1.1 fb for M Z = 2.9 TeV. The acceptance-times-efficiency in the dielectron (dimuon) channel is 65% (40%) at ATLAS [46] and 55% (80%) at CMS [47].  The Z production cross section at the 13 TeV LHC, computed at leading order with MadGraph and multiplied by K(Z ) = 1.16 is shown in Figure 5. A Z whose mass saturates the Run 1 bound has a production cross section of ∼ 19 fb at Run 2, which predicts approximately five dilepton Z events after 5 fb −1 . Although after 65 pb −1 CMS observed a dielectron event [48] with invariant mass of 2.9 TeV (the probablity for this event to be due to the SM background is ∼ 10 −3 ) the more recent Run 2 analyses of CMS [49] and ATLAS [50] have no deviation from the SM prediction. The ATLAS result, using 3.2 fb −1 , places a lower bound of 3.4 TeV on the Z mass, corresponding to g R = 0.44 and a total width of Γ Z ≈ 80 GeV.
The dominant branching fraction is Z → jj (see Figure 4). Furthermore, Higgs bosons lighter than ∼ 1 TeV and SM bosons or top quarks, produced in the decay of the Z , will be sufficiently boosted that their decay products will lie in a single jet. Thus, the effective dijet branching fraction for a 2.9 TeV Z , and g R = 0.48, increases from 62% to about 70%, with the remaining 30% due to 5% for each of e + e − , µ + µ − and τ + τ − , and a 14% invisible branching fraction; we have assumed that N D is heavier than M Z /2. Assuming the acceptance-times-efficiency for these high p T jets coming from Z decay is approximately 50% at both CMS and ATLAS we estimate that the signal in each experiment is ∼ 8 dijet events with invariant mass around 3 TeV in Run 1. This signal is too small compared to the QCD background [3,14].
After 30 fb −1 of Run 2 each experiment, assuming a similar acceptance and efficiency as in Run 1, should have ∼ 200 dijet events. The sizable QCD background makes this a challenging search channel, although it may be possible to use various signal features, including angular distributions, quark-versus-gluon discriminants, and substructure techniques (for the hadronic decays of boosted objects) to reduce the background.

Conclusions
The CMS and ATLAS Collaborations, analyzing LHC Run 1 data, have accumulated an intriguing set of excess events over disparate final states. These include excesses near 2 TeV in jj, W Z, W h and e + e − jj resonance searches [1]- [5], as well as an excess in the final state with same-sign leptons plus b jets [9]. We have shown that there is a common explanation for all these excess events in a model with SU (3) c × SU (2) L × SU (2) R × U (1) B−L gauge structure, a Higgs sector with only a bidoublet and an SU (2) R doublet, and a flavor symmetry that controls the masses of the right-handed neutrinos. We refer to this as the Reτ D model, to emphasize that there is a flavor symmetry acting on the e and τ right-handed neutrinos, and that the SU (2) R × U (1) B−L symmetry is broken by a Doublet.
Let us briefly mention some differences between this model and the "RDiT model" presented in [6,8] and the "Reτ T model" presented in [11]. Both RDiT and Reτ T use an SU (2) R Triplet to break the SU (2) R × U (1) B−L gauge symmetry. As a result, the relation between the W and Z masses shown in Eq. (5.8) for our Reτ D model is modified by a factor of √ 2, pushing the Z mass above 3.5 TeV. The RDiT model has Dirac masses for right-handed neutrinos, with the left-handed Dirac partners provided by vectorlike SU (2) R -doublet leptons. As a result, there is an additional parameter that controls the W coupling to an electron and a Dirac right-handed neutrino. By contrast, in the Reτ T model and our Reτ D model the e and τ right-handed neutrinos form a Dirac fermion (N D ), whose mass must be in the 1.4-1.6 TeV range (see Figure 2) to explain the CMS e + e − jj excess.
The excess events from Run 1, taken together, point towards a W of mass ∼ 1.9 TeV, which means that the decay products of the W are highly boosted. The jj excess is not only sensitive to W decays to light quarks but also to its decays to heavy SM particles, which subsequently decay hadronically. This raises the effective hadronic branching fraction from ∼ 60% to 80 − 90%. We take this effect into account and reanalyze the dijet excess and determine that the range necessary to explain the excess is 0.4 g R 0.59, corresponding to a W width of 20 − 48 GeV. We also point out that the lack of an excess in the CMS tb resonance search places a nontrivial constraint, g R 0.45, while the constraints from ATLAS are considerably weaker and allow the whole coupling range favored by the dijet excess.
An upper limit on g R is placed by dilepton resonance searches in Run 2: the M Z 3.4 TeV limit corresponds to g R 0.44 in this Reτ D model. A comparable limit on g R is set GeV [8].
Our MadGraph model files [20] include all the new particles discussed here: W , Z , N D , H + , H 0 , A 0 . These allow simulations of the many signals predicted in this model, and can be used by the experimental collaborations to disentangle the cross-contamination of new-physics channels (e.g., W → jj versus W → W Z → JJ, mentioned in Section 4).
There are many W decays that can be tested in Run 2. From Figure 3, it follows that there are at least 7 channels with branching fractions at percent level or above. The N D fermion produced in two of these channels has several decay modes: ejj, etb, eW (as well as others with small branching fractions, including eW h and eW Z) and the same with e replaced by τ . We thus obtain more than 17 final states (without even counting the various decay modes of the SM bosons) in which the LHC Run 2 will have sensitivity to the existence of the W boson.
The Z presents a separate set of opportunities. Taking into account the W mass and production cross section that fit the Run 1 dijet excess and the lower M Z limit set by Run 2, the Z mass is in the 3.4 − 4.5 TeV range. The Z branching fractions, shown in Figure 4, are large enough to allow sensitivity in 9 channels, with many additional ones (originating from N DND and W W ) opening up for large enough M Z .
Here m 12 and m 13 are the invariant masses of the tb and eb systems, respectively. After integrating over phase space we find the following width: In the limit m t → 0 this is equal to the width for N D → e − ud: