# Searching for the Minimal Seesaw Models at the LHC and Beyond

Authors: Arindam Das
Journal: Advances in High Energy Physics
 (2018)

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## Abstract

The existence of the tiny neutrino mass and the flavor mixing can be naturally explained by type I Seesaw model which is probably the simplest extension of the Standard Model (SM) using Majorana type SM gauge singlet heavy Right Handed Neutrinos (RHNs). If the RHNs are around the Electroweak- (EW-) scale having sizable mixings with the SM light neutrinos, they can be produced at the high energy colliders such as Large Hadron Collider (LHC) and future 100 TeV proton-proton (pp) collider through the characteristic signatures with the same-sign dilepton introducing lepton number violations (LNV). On the other hand Seesaw models, namely, inverse Seesaw, with small LNV parameter can accommodate EW-scale pseudo-Dirac neutrinos with sizable mixings with SM light neutrinos while satisfying the neutrino oscillation data. Due to the smallness of the LNV parameter of such models, the “smoking-gun” signature of same-sign dilepton is suppressed where the RHNs in the model will be manifested at the LHC and future 100 TeV pp collider dominantly through the Lepton number conserving (LNC) trilepton final state with Missing Transverse Energy (MET). Studying various production channels of such RHNs, we give an updated upper bound on the mixing parameters of the light-heavy neutrinos at the 13 TeV LHC and future 100 TeV pp collider.


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## Body

## 1. Introduction

The experimental evidence of the neutrino oscillation and flavor mixings from neutrino oscillation experiments [1–6] indicates that the SM is not enough to explain the existence of the tiny neutrino mass and flavor mixing. After the pioneering discovery of the d=5 operator [7] within the SM using the SM leptons, SM Higgs doublets, and ΔL=2(L=Leptonnumber) unit of LNV, it turned out that the Seesaw mechanism [8–14] could be the simplest idea to explain the small neutrino mass and flavor mixing where the SM can be extended by the SM-gauge singlet Majorana type RHNs. After the Electroweak (EW) symmetry breaking, the light Majorana neutrino masses are generated after the so-called type I Seesaw mechanism.In type I Seesaw, we introduce SM gauge-singlet Majorana RHNsNRβ where β is the flavor index. NRβ couples with the SM lepton doublets lLα and the SM Higgs doublet H. The relevant part of the Lagrangian is(1)L⊃-YDαβlLα¯HNRβ-12mNαβNRαC¯NRβ+H.c.,where YDαβ is the Yukawa coupling, lLα is the SM SU2L lepton doublet, and mN is the Majorana mass term. After the spontaneous EW symmetry breaking by the vacuum expectation value (VEV), H=v/20, we obtain the Dirac mass matrix as MD=YDv/2 suppressing the indices. Using the Dirac and Majorana mass matrices we can write the neutrino mass matrix as (2)Mν=0MDMDTmN,where MD is the Dirac mass matrix and mN is the Majorana mass term. Diagonalizing Mν we obtain the Seesaw formula for the light Majorana neutrinos as (3)mν≃-MDmN-1MDT.For mN~100 GeV, we may find YD~10-6 with mν~0.1 eV. However, in the general parameterization for the Seesaw formula [15], YD can be large and sizable (O(1)), and this is the case we consider in this paper.The searches of the Majorana RHNs can be performed by the “smoking-gun” of the same-sign dilepton plus di-jet signal which is suppressed by the square of the light-heavy neutrino mixing parameterVlN2≃mDmN-12. A comprehensive general study on the parameters of VlN2 has been given in [16] using the data from the neutrino oscillation experiments [1–6], bounds from the Lepton Flavor Violation (LFV) experiments [17–19], Large Electron-Positron (LEP), and Electroweak Precision test [20–27] experiments using the nonunitarity effects [28, 29] applying the Casas-Ibarra conjecture [15, 30–33]. At this point we mention that [16] has a good agreement with a previous analysis [34] on the sterile neutrinos. The bounds in [16] have been compared with the existing results in [23, 26, 27, 35–37] considering the degenerate Majorana RHNs. In case of Seesaw mechanism the Dirac Yukawa matrix (YD) can carry the flavors where the RHN mass matrix is considered to be diagonal. This case is favored by the neutrino oscillation data as studied in [16, 30, 38–42]. Such a scenario for the Seesaw scenario is called the Flavor Nondiagonal (FND). The other possibility of considering both of the diagonal YD and mN is not supported by the neutrino oscillation data.Since any number of singlets can be added in a gauge theory without contributing to anomalies, one can utilize such freedom to find a natural alternative of the low-scale realization of the Seesaw mechanism. Simplest among such scenarios is commonly known as the inverse Seesaw mechanism [43, 44] where a small Majorana neutrino mass originates from tiny LNV parameters rather than being suppressed by the RHN mass as done in the case of conventional Seesaw mechanism. In the inverse Seesaw model two sets of SM-singlet RHNs are introduced which are pseudo-Dirac by nature and their Dirac Yukawa couplings can be even order one, while reproducing the neutrino oscillation data. Therefore, at the high energy colliders such pseudo-Dirac neutrinos can be produced through a sizable mixing with the SM light neutrinos [45–52].In the inverse Seesaw mechanism the relevant part of the Lagrangian is given by(4)L⊃-YDαβlLα¯HNRβ-mNαβSLα¯NRβ-12μαβSLα¯SLβC+H.c.,where NRα and SLβ are two SM-singlet heavy neutrinos with the same lepton numbers, mN is the Dirac mass matrix, and μ is a small Majorana mass matrix violating the lepton numbers. After the EW symmetry breaking we obtain the neutrino mass matrix as (5)Mν=0MD0MDT0mNT0mNμ.Diagonalizing this mass matrix we obtain the light neutrino mass matrix (6)Mν≃MDmN-1μmN-1TMDT.Note that the smallness of the light neutrino mass originates from the small LNV term μ. The smallness of μ allows the mDmN-1 parameter to be on the order one even for an EW scale RHNs. In the inverse Seesaw case we can consider YD as nondiagonal when μ and mN are diagonal which is called the Flavor Nondiagonal (FND) case. On the other hand we can also consider the diagonal YD, mN when μ will be nondiagonal. This situation is called the Flavor Democratic scenario. For the inverse Seesaw both of the FND and FD cases are supported by the neutrino oscillation data. In this article we will consider the FND case from the Seesaw and the FD case from the inverse Seesaw mechanisms.Through the Seesaw mechanism, a flavor eigenstate (ν) of the SM neutrino is expressed in terms of the mass eigenstates of the light (νm) and heavy (Nm) Majorana neutrinos such as (7)ν≃νm+VlNNm.Using the mass eigenstates, the charged current (CC) interaction for the heavy neutrino is given by(8)LCC⊃-g2Wμe¯γμPLVlNNm+H.c.,where e denotes the three generations of the charged leptons in the vector form, and PL=1/2(1-γ5) is the projection operator. Similarly, the neutral current (NC) interaction is given by (9)LNC⊃-g2cwZμNm¯γμPLVlN2Nm+νm¯γμPLVlNNm+H.c.,where cw=cos⁡θw with θw being the weak mixing angle and Wμ, Zμ are the SM gauge bosons.The main decay modes of the heavy neutrino areN→lW,νlZ,νlh. The corresponding partial decay widths [47] are, respectively, given by (10)ΓN⟶lW=g2VlN264πmN2-mW22mN2+2mW2mN3mW2,ΓN⟶νlZ=g2VlN2128πcw2mN2-mZ22mN2+2mZ2mN3mZ2,ΓN⟶νlh=VlN2mN2-mh2232πmN1v2.The decay width of heavy neutrino into charged gauge bosons is twice as large as neutral one owing to the two degrees of freedom (W±). We plot the branching ratios BRi=Γi/Γtotal of the respective decay modes Γi with respect to the total decay width Γtotal of the heavy neutrino into W, Z and Higgs bosons in Figure 1 as a function of the heavy neutrino mass mN. Note that for larger values of mN such as mN≥1500 GeV, the branching ratios can be obtained as (11)BRN⟶lW:BRN⟶νZ:BRN⟶νh≃2:1:1.Figure 1
Heavy neutrino branching ratios(BRi) for different decay modes are shown with respect to its mass mN [51].In this paper we study the RHN production from various initial states such as the quark-quark(qq), quark-gluon (qg), and gluon-gluon (gg) at the 13 TeV LHC and future 100 TeV pp collider. We consider the photon mediated processes as well as the gluon-gluon fusion (ggF), photon-proton interactions, and Vector Boson Fusion (VBF) processes to produce the RHNs. For different RHN masses (mN); we calculate the cross section of each of the processes normalized by the square of the light-heavy neutrino mixing angles.This paper is organized as follows. In Section2 we calculate the production cross sections at the 13 TeV LHC and future 100 TeV pp collider [53] with a variety of initial states. In Section 3 we study the multilepton decay modes of the RHNs at the 13 TeV LHC and future 100 TeV pp collider. For both of the cases we take the luminosity as 3000 fb−1. In Section 4 we put the bounds on the mixing angle as function of the RHN mass. Section 5 is dedicated for conclusions.


## 2. Production Cross Sections

The RHNs can be produced at the 13 TeV LHC and future 100 TeV pp collider from various initial states. We consider the combined production of the heavy neutrinos from various initial states including quark-(anti)quark(qq′¯), quark-gluon (qg), and gluon-gluon (gg) interactions. We also study contributions coming from the gluon-gluon fusion (ggF), photon-proton interactions, and Vector Boson Fusion (VBF) processes to produce the RHNs at the LHC and beyond. In this section we consider the RHN productions in association with SM leptons and jets. To obtain the cross sections and generate the events we implement our model in MadGraph [54] bundled with PYTHIA [55] and DELPHES [56]. The production modes of the heavy neutrinos in association with leptons and jets are proportional to the square of the mixing angle, VlN2. In this section we use VlN2=10-4 to estimate the cross sections. (The EWPD bounds VlN2 have been discussed in [20, 26, 27]. The universal bound has been considered to be 9×10-4 which rules out the possibility of the mixing angles above this value. Therefore, we used a value of VlN2<9×10-4 to calculate the cross sections.)(1)
Charged current interaction is mediated byW:
(i)
generate  pp→Nl(ii)
add process  pp→Nlj(iii)
add process  pp→Nljjalong with the charge conjugates wherej stands for the jets.In this process the thes-channel quark-antiquark pair of different flavors (qq′¯) will interact through the W exchange and finally follow (8) to produce the RHN (N) in association with a lepton (l). The corresponding Feynman diagram for qq′¯→Nl is given in Figure 2.The contributions from the quark-quark interaction(qq′¯) to one-jet (Nlj) are given in Figure 3 for the t-channel process and additional contributions to the one-jet process from the quark-gluon (qg) interaction as shown in Figure 4 form the s,t-channel processes. In both of the cases W is radiated from the quarks/antiquarks and hence follows the CC to produce N in association with l.Two-jet contributions(Nljj) coming from the qq′¯ process are shown in Figure 5. In this case, the s, t channel contributions between the quarks are involved to produce N with l in association with two jets following the CC interactions at the N production vertex. The quark-gluon (qg) processes contributing in the two-jet case are shown in Figure 6 where the s, t channel contributions between the quarks and gluons are involved to produce N with l in association with two jets following the CC interactions at the N production vertex. In addition to that gluon-gluon (gg) processes contributing in Nljj are shown in Figure 7 in the s, t-channel followed by the N production from the CC interactions with l in association with two jets.We combine all these processes to compute the production cross section of the RHNs through the charged current interaction forNlX final state where X stands for n-jet and n=0,1,2,3. To produce such processes we use the following trigger cuts:
(a)
transverse momentum of the jets,pTj>30 GeV(b)
transverse momentum of the leptons,pTl>10 GeV(c)
pseudo-rapidity of the jets,ηj<2.5(d)
pseudo-rapidity of the leptons,ηl<2.5,with the Multi-Leg Matching (MLM) scheme. In the MLM matching scheme one can obtainn-parton events by MadEvent generator under the kT clustering algorithm. After the reweight, each final state parton can find the node where it was generated. This n-parton shower can be generated (μg2) in the directions of the primary partons so that the initial condition for each parton shower is kept at μg2. Hence running the kT clustering algorithm one can find all the jets at the resolution scale (τr). If all the jets match with the primary partons then the event is accepted; otherwise it is rejected. To elaborate discussions on this mechanism for the event generators, see [57–69]. In MadGraph the switch ickkw=1 stands for the MLM scheme in MadGraph [54] using
(i)
ickkw=1(ii)
xqcut=pTj(iii)
QCUT = Maxxqcut+5 GeV, 1.2∗xqcutusingMSTP(81) = 21. The MSTP switches modify the generation procedure. In this case it switches off or on the Initial State Radiation (ISR), Final State Radiation (FSR), and Multiple Interactions (MI) among the beam jets and fragmentation. It is also used to give the “parton skeleton” of the hard process. MSTP(81) = 21 is the master switch in PYTHIA 6.4 which switches on the Multi-Interactions (MI) for the new model at the time of showering and hadronization. The MSTP= 21 is used for the pT ordered shower switching on SHOWER-KT [70–73] in PYTHIA [55]. The trigger cuts are used on the basis of the anomalous multilepton searches done by the CMS [74, 75]. The use of cone jets or kT jets is decided by whether the parameter xqcut (specifying the minimum kT jet measure between jets, i.e., gluons or quarks (except top quarks) which are connected in Feynman diagrams) in the MadGraph is set to be 0 or not. If xqcut  =  0, cone jets are used, while if xqcut  >  0, kT jet matching is assumed. In this case, transverse momentum of jet (pTj) and separation between the jets (ΔRjj) should be set to zero. For most processes, the generation speed can be improved by setting pTj = xqcut which is done automatically if the switch auto − ptj − mjj is set to “T” at the time of event generation using MadGraph to control the transverse momentum of the jets (pTj) and the invariant mass of the jets (mjj). If some jets should not be restricted this way (as in single top or Vector Boson Fusion (VBF) production, where some jets are not radiated from QCD) in that case the switch auto − pTj − mjj should be set to “F” in the MagGraph at the time of event generation. QCUT is used for the matching with the kT scheme; in this case the jet measure cutoff is used by Pythia. If the value is not given, it will be set to max(xqcut + 5, xqcut  ∗  1.2), where xqcut is taken from the MadGraph [58, 59]. We use such cuts to keep the analysis collinear safe. The production cross sections are shown in Figures 11 and 12, respectively, as a function of mN.Figure 2
q q ′ ¯ ( q q ¯ ) process to produce Nl(Nν) from the CC(NC) interaction.Figure 3
1-jet process to produceN with l(ν) in association with a jet from the CC(NC) interaction from qq′¯(qq¯) initial state.Figure 4
1-jet process to produceN with l(ν) in association with a jet from the CC(NC) interaction from qg initial state.Figure 5
2-jet process to produceN with l(ν) in association with a jet from the CC(NC) interaction from qq′¯(qq¯) initial state.Figure 6
2-jet process to produceN with l(ν) in association with a jet from the CC(NC) interaction from qg initial state.Figure 7
2-jet process to produceN with l(ν) in association with a jet from the CC(NC) interaction from gg initial state.( 2 )
Neutral current interaction is mediated byZ:
(i)
generate p p → N ν (ii)
add process p p → N ν j (iii)
add process p p → N ν j j followed by the same production procedure as we discussed in(1). Using quark-antiquark pair of same flavor (qq¯) at the s-channel by (9) N can be produced in association with a light neutrino (ν) as shown in Figure 2. The Nνj (in Figures 3 and 4) and Nνjj (in Figures 5, 6, and 7) processes are the same as those which have been discussed in (1). The only difference is the production vertex of Nν coming from the NC from (9). Combining these final states we can denote NνX where X stands for n-jet with n=0,1,2,3. In this case we use the following trigger cuts:
(a)
transverse momentum of the jets,pTj>30 GeV (b)
pseudo-rapidity of the jets,ηj<2.5 and the same matching scheme used in(1). Such pTj cuts will keep the analysis collinear safe specially in (1) and (2) to calculate the cross sections using MLM matching [57–61, 66–69] schemes. The production cross sections at the 13 TeV LHC and future 100 TeV pp collider are shown in Figures 11 and 12, respectively, as a function of mN. ( 3 )
Gluon-fusion channel (ggF): In the ggF top loop produces the SM Higgs and Higgs can decay intoN in association with ν [45, 46, 76]. The corresponding Feynman diagram is given in Figure 8(a). There is another complementary production channel of N in association with ν which comes from Z [45, 77]. The corresponding Feynman diagram is given in Figure 8(b). The production process depends on mN; one can produce them promptly from the Higgs decay when mN<mh, where mh is the Higgs mass and also from the off-shell Z(Z∗). When mN<mh, Higgs can decay into RHNs and the partial decay width can be written as (12)Γhnew=YD2mH8π1-mN2mh22. This has additive contribution to the total decay width of the SM Higgs boson keepingYD as a free parameter. Constraints on YD and VlN2 have recently been studied in [35, 45, 46]. The cross section goes down at the 13 TeV LHC for mh<mN due to the off-shell decay. However, at the future 100 TeV pp collider the cross section again rises around mN=250 GeV due to large contributions coming from the gluon PDFs. In this channel we are testing mN=100 GeV–1 TeV. The production cross sections are shown in Figures 11 and 12, respectively, with respect to mN. At the future 100 TeV, the large gluon PDF starts contributing to the RHN production resulting in a rise in the ggF curve compared to the 13 TeV result. ( 4 )
Photon initiated processes: The photon (denoted bya in MadGraph) initiated processes also have important contributions in the RHNs production which have been studied in [49, 78–83]. In case of the the photon initiated process, the photon can be radiated from the proton and also from a parton. Those production channels will give additive contributions at the colliders once the RHNs decay into multilepton modes. The corresponding Feynman diagrams for these processes are given in Figure 9. The Nlj production process is possible as γ→WW vertex is present which will make the production cross section for Nlj higher in comparison to that of Nνj where γ→ZZ vertex is not present under the SM gauge group. Nνj will be produced from the Z→Nν vertex under the NC interaction according to (9). For the photon initiated production processes we use
(i)
generate p a → N l j  QED= 3 QCD= 0 (QED (Quantum Electrodynamic) processes switches the QED interactions with photon, W and Z bosons, QED = 3 means the order of the interaction whereas QCD stands for the Quantum Chromodynamic processes with QCD =0 being the order of the interaction.) withpTj>30 GeV, pTl>10 GeV, ηl,j<2.5. To generate the Nνj final state with photon initiated process we use (ii)
generate p a → N ν j  QED= 3 QCD= 0 withpTj>30 GeV, ηj<2.5. ( 5 )
Vector Boson Fusion (VBF) channels: The VBF processes are shown in Figure10 where the Nl and Nν are produced with two widely separated jets and the corresponding final states will be Nljj(Nνjj) depending on the CC (NC) vertex. In the VBF case the γWW and ZWW vertices will come into effect to produce the N in association with l(ν) depending on the CC (NC) of N-W(N-Z). To generate the Nljj(Nνj) final state from the VBF channels we use
(i)
generate p p → N l j j  QED= 4 QCD = 0 withpTj>30 GeV, pTl>10 GeV, ηl<2.5, ηj1-ηj2>4.2, pTj1,leading=pTj2,trailing>50 GeV, mjjmin=250 GeV. (ii)
generate p p → N ν j j  QED = 4 QCD= 0 withpTj>30 GeV, pTl>10 GeV, ηl<2.5, ηj1-ηj2>4.2, pTj1,leading=pTj2,trailing>50 GeV, mjjmin=250 GeV. The corresponding production cross sections for the 13 TeV LHC and future 100 TeV pp collider are shown in Figures 11 and 12, respectively, with respect to mN.Figure 8
ggF production of the heavy neutrinos from Higgs(h) and Z bosons. h→Nν can be prompt when mh>mN giving an enhancement to the Nν production from the ggF channel. For mh<mN, off-shell Higgs (h∗) produces Nν final state. Similarly off-shell Z(Z∗) can also produce Nν final state when mN>mZ. For the Higgs mediated case, top quark loop will contribute dominantly whereas for the Z∗ case all contributions coming from the quarks will be counted according to its coupling with the quarks.
(a) (b)Figure 9
The photon initiatedNlj final state. The Nνj final state can also be obtained; however, the contribution will be low as γ→ZZ vertex is absent due to the gauge invariance.Figure 10
VBF production of theNljj final state from the W→Nl vertex. The Nνjj finals state can also be obtained using the Z→Nν vertex. The two jets can be obtained at the forward-backward regions.Figure 11
Production cross sections of the RHNs in association with leptons from different modes at the 13 TeV LHC withVlN2=10-4. “a” stands for photon (γ) as it is defined by MadGraph.Figure 12
Production cross sections of the RHNs in association with leptons from different modes at the future100 TeV pp collider with VlN2=10-4. “a” stands for photon (γ) as it is defined by MadGraph.


## 3. Decay of the RHNs at the LHC

Implementing our model in the event generatorMadGraph, we produce the RHNs and allow it to decay in various multilepton modes. We use kinematic cuts in this adopting from the CMS analysis in [74, 75]. According to our choice we consider two models such as type I Seesaw and Inverse Seesaw. In type I Seesaw the RHN is Majorana type and in inverse Seesaw the RHN is pseudo-Dirac type. From the Majorana RHN we get LNV same-sign dilepton plus di-jet signal, whereas from the pseudo-Dirac type RHNs we get LNC trilepton plus MET (ETmiss/ɆT) final state. Considering the leading decay mode of the RHNs (N→Wl) and depending on the choice of the final states, W will decay either leptonically or hadronically. We consider the 13 TeV LHC to study such processes. We consider mN=100 GeV in this section for different production processes. We use the data files after the hadronization using PYTHIA [55] and detector simulation using DELPHES [56] bundled with MadGrpah [54] and use the MLM matched results as prescribed in the previous section. In this analysis the leading particle is the particle having longest transverse momentum (pT) distribution whereas the trailing particle is that which has shorter transverse momentum (pT) distribution. We have plotted the transverse momentum distributions of the leptons (pTl) in Figure 13 and the Missing Transverse Energy (MET/ETmiss/ɆT) distribution in the Figure 14 from the trilepton plus MET (3l+MET+X) signal. We notice that the leading lepton transverse momentum, pTl, for l1 peaks around 40 GeV whereas the trailing leptons mostly stay between 10 GeV and 40 GeV. Looking at the distribution of the leading lepton and the peak of the distribution we suggest that the leading lepton is coming from the leptonic decay of W. The MET distribution peaks around 40 GeV which also backs the ides of having the leading lepton of W. Therefore, for the trilepton analysis at mN=100 GeV using ETmiss<50 GeV will be reasonable choice.Figure 13
Transverse momenta distributions for the three leptons from the3l + MET final state from pp→NlX, N→lW, W→lν at the 13 TeV LHC.Figure 14
MET distribution from the3l + MET final state from pp→NlX, N→lW, W→lν at the 13 TeV LHC.We study the same-sign dilepton plus di-jet(l±l±jj+X) where X stands for the radiated jets. This signal is an important signature to test the Majorana nature of the RHNs produced from type I Seesaw model. The transverse momentum of the leptons (pTl) and the jets (pTj) are plotted in Figures 15 and 16, respectively. The invariant mass distribution of the two jets is plotted in Figure 17. The distribution shows a peak around mW. The invariant mass distribution of the lepton plus two-jet system has been shown in Figure 18. The figure shows the distributions including ml1jj and ml2jj. Among them ml1jj shows a peak around the assumed mN value around 100 GeV.Figure 15
Transverse momentum distributions of leptons(pTl) from the same-sign dilepton plus di-jet final state events.Figure 16
Transverse momentum distributions of the jets(pTj) from the same-sign dilepton plus di-jet final state.Figure 17
The invariant mass distributions of two-jet system(mjj) from the same-sign dilepton plus di-jet final state showing a peak around the W mass (mW).Figure 18
The invariant mass distributions of one lepton plus two-jet system(mljj) showing a peak around mN~100 GeV (blue) from the same-sign dilepton plus di-jet signal.We study the VBF processes to produce the heavy neutrinos and hence study the trilepton plus MET final state. We have used the VBF prescriptions written in the previous section where the jetsj1 and j2 are widely separated. The other two jets are initial state radiations (ISR) which also are not populating the central region. The rapidity distributions of the jets are shown in Figure 19. This is a striking feature of the VBF process. The leading lepton coming out of the W decay after the W boson is produced from the N→Wl decay. The leading leptons are also slightly away from the central region. We use a lepton pseudo-rapidity cut, ηl<2.5. The rapidity distributions of the leptons are shown in Figure 20.Figure 19
Rapidity distributions of the associated jets in the trilepton mode from VBF process.Figure 20
Rapidity distributions of the the leptons in the trilepton mode from VBF process.Another important contribution is coming from theNνjj+X process from the NC interaction between the RHNs and Z bosons. Here X are the radiated jets. The final state consists of a single lepton, two jets, and MET. The produced jets can be used to reconstruct the W boson. The distribution shows a peak around the W mass. Similarly from the RHN decay we get N→ljj and the invariant mass distribution of the ljj system can show a peak around the RHN mass (mN). The invariant mass distribution of mjj is shown in Figure 21 and that of mljj is shown in Figure 22.Figure 21
Invariant mass distribution of the two-jet system(mjj) from the l+MET+2j+X final state from the pp→NνX process. The two-jet system shows a peak around the W mass (mW).Figure 22
Invariant mass distribution of the lepton plus two-jet systems(mljj) from the l+MET+2j+X final state from the pp→NνX process. The lepton plus two-jet system shows a peak around mN~100 GeV.We produced the RHNs from the ggF process where the top loop becomes dominant to produce the Higgs which can promptly decay into the RHN whenmN<mH. In our case we consider the mN=100 GeV and the Higgs will decay promptly into Nν and the RHN will decay into W followed by its hadronic decay. The invariant mass distribution of the two-jet system (mjj) is shown in Figure 23 whereas that of the lepton and two-jet system are shown in Figure 24. The mjj distribution peaks around the W mass whereas the mljj distribution peaks around the RHN mass. Detailed results regarding the Higgs decaying into RHNs can be found in [35, 45, 46] with pervious and updated limits.Figure 23
Invariant mass distribution of the two-jet system(mjj) from the l+MET+2j final state coming from ggF process. The two-jet system shows a peak around the W mass (mW).Figure 24
Invariant mass distribution of the lepton plus two-jet systems(mljj) from the l+MET+2j final state coming from ggF process. The lepton plus two-jet system shows a peak around the RHN mass (mN) at the 13 TeV LHC.


## 4. Bounds on the Mixing Angle

FormN<MZ, the RHN can be produced from the on-shell Z-decay through the NC interaction in association with missing energy; however, if mN>MZ off-shell production will take place with the same final state. The heavy neutrino can decay according to the CC and NC interactions. Different production processes, different decay modes of the heavy neutrinos, and various phenomenologies have been discussed in [51, 52, 82, 84–94]. RHN production from various initial states and scale dependent production cross sections at the Leading Order (LO) and Next-to-Leading-Order QCD (NLO QCD) of Nν have been studied at the 14 TeV LHC and future 100 TeV pp collider [51, 52]. The L3 collaboration [21] has performed a search on such heavy neutrinos directly from the LEP data and found a limit on B(Z→νN)<3×10-5 at the 95% CL for the mass range up to 93 GeV. The exclusion limits from L3 are given in Figure 25 where the red solid line stands for the limits obtained from electron (L3-e) and the red dashed line stands for the exclusion limits coming from μ (L3-μ). The corresponding exclusion limits on Vl=eN at the 95% CL [22, 23] have been drawn from the LEP2 data which have been denoted by the dark magenta line. In this analysis they searched for 80GeV≤MN≤205GeV with a center of mass energy between 130 GeV and 208 GeV [23].Figure 25
Bounds on the square of the mixing angle from the same-sign dilepton plus di-jet final state as a function of the heavy neutrino mass(mN). The shaded region is ruled out by DELPHI, EWPD, and Higgs data. Prospective bounds from the Higgs data had been calculated in [45] for the LHC at the high luminosity (3000 fb−1) and future 100 TeV pp collider.The DELPHI collaboration [24] had also performed the same search from the LEP-I data which set an upper limit for the branching ratio B(Z→Nν) about 1.3×10-6 at 95% CL for 3.5 GeV ≤mN≤50 GeV. Outside this range the limit starts to become weak with the increase in mN. Here it has been considered that N→Wl and N→Zν decay after the production of the heavy neutrino was produced. The exclusion limits for l=e,μ,τ are depicted by the blue solid, dashed, and dotted lines in Figure 25.The search of the sterile neutrinos can be made at high energy lepton colliders with a very high luminosity such as Future Circular Collider (FCC) for the Seesaw model. A design of such collider has been launched recently where nearly 100 km tunnel will be used to study high luminositye+e- collision (FCC-ee) with a center-of-mass energy around 90 GeV to 350 GeV [25]. According to this report, a sensitivity down to |VlN|2~10-11 could be achieved from a range of the heavy neutrino mass, 10 GeV ≤mN≤80 GeV. The darker cyan-solid line in Figure 25 shows the prospective search reaches by the FCC-ee. A sensitivity down to a mixing of VlN2~10-12 can be obtained in FCC-ee [25], covering a large phase space for mN from 10 GeV to 80 GeV.The heavy neutrinos can participate in many electroweak (EW) precision tests due to the active-sterile couplings. For comparison, we also show the95% CL indirect upper limit on the mixing angle, VlN<0.030,0.041 and 0.065 for l=μ,e,τ respectively, derived from a global fit to the electroweak precision data (EWPD), which is independent of mN for mN>MZ, as shown by the horizontal pink dash, solid, and dolled lines, respectively, in Figure 25. The bounds from the EWPD have been studied in [20, 26, 27]. For the mass range, mN<MZ, it is shown in [83] that the exclusion limit on the mixing angle remains almost unaltered; however, it varies drastically at the vicinity of mN=1GeV. For the flavor universal case the bound on the mixing angle is given as VlN2=0.025 from [20] which has been depicted in Figure 25 with a pink dot-dashed line.The CMS limits from the8 TeV LHC are represented by the Plink lines. The dashed Pink line represents μ and solid pink line represents e. For both of the flavors CMS has tested the mass range, 40 GeV ≤mN≤200 GeV. For electron it has probed down to 10-4 and for muon it has probed down to 10-5 for VeN2 and VμN2, respectively. The ATLAS bounds from the 8 TeV LHC are weaker than the CMS bounds. The ATLAS [36] bounds are represented by the brown dashed lines for μ(VμN2) and brown dotted line represents the bounds from e(VeN2) in Figure 25.The relevant existing upper limits at the95% CL are also shown to compare with the experimental bounds using the LHC Higgs boson data in [35, 48] using [95–99]. The darker green dot-dashed line named Higgs boson shows the relevant bounds on the mixing angle. In this analysis we will compare our results taking this line as one of the references. We have noticed that VlN2 can be as low as 4.86×10-4 while mN=60 GeV and the bound becomes stronger at mN=100 GeV as 3.73×10-4. When mN>100 GeV, the bounds on VlN2 become weaker.


### 4.1. Same-Sign Dilepton Plus Di-Jet Signal

For simplicity we consider the case that only one generation of the heavy neutrino is light and accessible to the LHC which couples to only the second generation of the lepton flavor. To generate the events in theMadGraph we use the CTEQ6L1 PDF [100] with xqcut= pTj = 20 GeV and QCUT= 25 GeV. We calculate the cross sections for the combined processes NlX,N→ljj as functions of mN from various initial states as described in Figures 11 and 12. Comparing our generated events with the recent ATLAS results [36] at the 8 TeV LHC with the luminosity 20.3 fb−1, we obtain an upper limit on the mixing angles between the Majorana type heavy neutrino and the SM leptons as a function of mN. In the ATLAS analysis the upper bound of the production cross section (σATLAS/CMS) is obtained for the final state with the same-sign di-muon plus di-jet as a function of mN. For σATLAS results we use the cross sections given in [36] and for σCMS we use [101]. Implementing our model in MadGraph we generate the signal event and compare the experimental cross sections from ATLAS and CMS using (13)VμN2≲σATLAS/CMSpp→NlX,N→ljj+Allsamesigndileptonmodes.Our upper bounds for the13 TeV LHC with 3000 fb−1 luminosity on the mixing angles are shown in Figure 25 along with the exclusion limits obtained from the different experimental results shaded in gray as described in the previous subsection. We can see that a significant improvement on the bounds can be made adding the jets and various initial states as described in this paper. Applying the ATLAS bound at 8 TeV with 20.3 fb−1 luminosity [36], we put a prospective upper bound on the mixing angles at the 13 TeV LHC with 3000 fb−1 luminosity. Recently the CMS has performed the same-sign dilepton plus di-jet search [101]. Using this result and adopting the same procedure for the ATLAS result we calculate the upper bound on the mixing angles at the 13 TeV LHC with 3000 fb−1 luminosity using (13). The results are shown in Figure 25.A significant improvement for the upper bound on the mixing angle is obtained by combining all the processes with jets and various initial states as described in this paper. We can see that, at91.2 GeV ≤mN≤200 GeV, the bounds obtained using the ATLAS (ATLAS13-μ@3000fb-1) analysis is better than the recent exclusions limits shaded in gray. Using the 8 TeV CMS result [101] we obtain prospective bound at the 13 TeV LHC for the luminosity 3000 fb−1  (CMS13-μ@3000 fb−1) in Figure 25. The results are also shown in Figure 25. In this analysis we have only chosen the μ flavor. The purple lines represent the 13 TeV LHC and black lines represent the future 100 TeV pp collider. The corresponding improved bounds at the future 100 TeV pp collider with 3000 fb−1 luminosity are shown in Figure 25 with the black dashed and dot-dashed lines corresponding to the ATLAS and CMS data marked as (100 TeV-μ@3000 fb−1), respectively, in Figure 25. The prospective bounds calculated from (13) at the 13 TeV LHC are represented by the purple and those for the future 100 TeV are represented by black lines.We find that, at the HL-LHC, using the same-sign di-muon and di-jet final state LHC can probe the squared of the mixing angle down to1.95×10-5 for the μ flavor whereas the future 100 TeV pp collider can probe the square of the mixing angle down to 5.83×10-6 for the μ flavor.


### 4.2. Trilepton Signal

In this analysis we consider two cases. One is the Flavor Diagonal (FD) case, where we introduce three generations of the degenerate heavy neutrinos and each generation couples with the single, corresponding lepton flavor. The other one is the Single Flavor (SF) case where only one heavy neutrino is light and accessible to the LHC which couples to only the first or second generation of the lepton flavor using theCTEQ6L PDF [100]. In this analysis we consider NlX final state followed by N→llνl.We generate thecombined parton level events using MadGraph and then gradually hadronize and perform detector simulations with xqcut= pTj = 30 GeV and QCUT= 36 GeV for the hadronization. In our analysis we use the matched cross section after the detector level analysis. After the signal events are generated we adopt the following basic criteria, used in the CMS trilepton analysis [74, 75]:(i)
The transverse momentum of each lepton:pTl>10 GeV(ii)
The transverse momentum of at least one lepton:pTl,leading>20 GeV(iii)
The jet transverse momentum:pTj>30 GeV(iv)
The pseudo-rapidity of leptons:ηl<2.4 and of jets: ηj<2.5(v)
The lepton-lepton separation:ΔRll>0.1 and the lepton-jet separation: ΔRlj>0.3(vi)
The invariant mass of each OSSF (opposite-sign same flavor) lepton pair:ml+l-<75 GeV or >105 GeV to avoid the on-Z region which was excluded from the CMS search. Events with ml+l-<12 GeV are rejected to eliminate background from low-mass Drell-Yan processes and hadronic decays(vii)
The scalar sum of the jet transverse momenta:HT<200 GeV(viii)
The missing transverse energy:ɆT<50 GeVThe additional trilepton contributions come fromN→Zν,hν, followed by the Z, h decaying into a pair of OSSF leptons. However, the Z contribution is rejected after the implementation of the invariant mass cut for the OSSF leptons to suppress the SM background and the h contribution is suppressed due to very small Yukawa couplings of electrons and muons. Using different values of ɆT and HT, the CMS analysis provides different number of observed events and the corresponding SM background expectations. For our analysis the set of cuts listed above are the most efficient ones as implemented by the CMS analysis [74, 75]. To derive the limits on VlN2, we calculate the signal cross section normalized by the square of the mixing angle as a function of the heavy neutrino mass mN for both SF and FD cases, by imposing the CMS selection criteria listed above. The corresponding number of signal events passing all the cuts is then compared with the observed number of events at the 19.5 fb−1 luminosity [74, 75]. For the selection criteria listed above, the CMS experiment observed the following:(a)
510 events with the SM background expectation of560±87 events for ml+l-< 75 GeV which is called below the Z-pole(b)
178 events with the SM background expectation of200±35 events for ml+l-> 105 GeV which is called above the Z-poleIn case (a) we have an upper limit of 37 signal events, while case (b) leads to an upper limit of 13 signal events. Using the limits obtained in case (b), we can set an upper bound onVlN2 for a given value of mN. In this analysis we use above the Z-pole situation with 3000 fb−1 luminosity for the 13 TeV LHC and future 100 TeV pp collider. (Exactly the same procedure can be adopted for the situation with ml+l-<75 GeV.)The mixing-squared versusmN contours shown in Figure 26 are allowed by the EWPD within the range 91.2 GeV ≤mN≤163 GeV for the SF case at the 13 TeV LHC at 3000 fb−1 luminosity. At the same time we analyze the FD case through which one can probe the range of 91.2 GeV ≤mN≤195 GeV. The limits for the FD case are roughly twice stronger than the SF case. However, at the future 100 TeV pp collider with 3000 fb−1 luminosity the upper bounds on mN go up to 200 GeV and 275 GeV for the SF and FD cases, respectively, keeping lower mass bound at the 91.2 GeV. As the coupling between the Higgs and RHNs can not distinguish between the Majorana and pseudo-Dirac neutrinos, we use the same limits for both of cases. Similarly the EWPD can measure the deviation from the SM couplings so we can use the same bounds in both cases.Figure 26
Bounds on the square of the mixing angle from the trilepton plus MET final state as a function of the heavy neutrino mass(mN). The shaded region is ruled out by the EWPD and Higgs data. Prospective bounds from the Higgs data had been calculated in [45] for the LHC at the high luminosity (3000 fb−1) and future 100 TeV pp collider.


## 4.1. Same-Sign Dilepton Plus Di-Jet Signal

For simplicity we consider the case that only one generation of the heavy neutrino is light and accessible to the LHC which couples to only the second generation of the lepton flavor. To generate the events in theMadGraph we use the CTEQ6L1 PDF [100] with xqcut= pTj = 20 GeV and QCUT= 25 GeV. We calculate the cross sections for the combined processes NlX,N→ljj as functions of mN from various initial states as described in Figures 11 and 12. Comparing our generated events with the recent ATLAS results [36] at the 8 TeV LHC with the luminosity 20.3 fb−1, we obtain an upper limit on the mixing angles between the Majorana type heavy neutrino and the SM leptons as a function of mN. In the ATLAS analysis the upper bound of the production cross section (σATLAS/CMS) is obtained for the final state with the same-sign di-muon plus di-jet as a function of mN. For σATLAS results we use the cross sections given in [36] and for σCMS we use [101]. Implementing our model in MadGraph we generate the signal event and compare the experimental cross sections from ATLAS and CMS using (13)VμN2≲σATLAS/CMSpp→NlX,N→ljj+Allsamesigndileptonmodes.Our upper bounds for the13 TeV LHC with 3000 fb−1 luminosity on the mixing angles are shown in Figure 25 along with the exclusion limits obtained from the different experimental results shaded in gray as described in the previous subsection. We can see that a significant improvement on the bounds can be made adding the jets and various initial states as described in this paper. Applying the ATLAS bound at 8 TeV with 20.3 fb−1 luminosity [36], we put a prospective upper bound on the mixing angles at the 13 TeV LHC with 3000 fb−1 luminosity. Recently the CMS has performed the same-sign dilepton plus di-jet search [101]. Using this result and adopting the same procedure for the ATLAS result we calculate the upper bound on the mixing angles at the 13 TeV LHC with 3000 fb−1 luminosity using (13). The results are shown in Figure 25.A significant improvement for the upper bound on the mixing angle is obtained by combining all the processes with jets and various initial states as described in this paper. We can see that, at91.2 GeV ≤mN≤200 GeV, the bounds obtained using the ATLAS (ATLAS13-μ@3000fb-1) analysis is better than the recent exclusions limits shaded in gray. Using the 8 TeV CMS result [101] we obtain prospective bound at the 13 TeV LHC for the luminosity 3000 fb−1  (CMS13-μ@3000 fb−1) in Figure 25. The results are also shown in Figure 25. In this analysis we have only chosen the μ flavor. The purple lines represent the 13 TeV LHC and black lines represent the future 100 TeV pp collider. The corresponding improved bounds at the future 100 TeV pp collider with 3000 fb−1 luminosity are shown in Figure 25 with the black dashed and dot-dashed lines corresponding to the ATLAS and CMS data marked as (100 TeV-μ@3000 fb−1), respectively, in Figure 25. The prospective bounds calculated from (13) at the 13 TeV LHC are represented by the purple and those for the future 100 TeV are represented by black lines.We find that, at the HL-LHC, using the same-sign di-muon and di-jet final state LHC can probe the squared of the mixing angle down to1.95×10-5 for the μ flavor whereas the future 100 TeV pp collider can probe the square of the mixing angle down to 5.83×10-6 for the μ flavor.


## 4.2. Trilepton Signal

In this analysis we consider two cases. One is the Flavor Diagonal (FD) case, where we introduce three generations of the degenerate heavy neutrinos and each generation couples with the single, corresponding lepton flavor. The other one is the Single Flavor (SF) case where only one heavy neutrino is light and accessible to the LHC which couples to only the first or second generation of the lepton flavor using theCTEQ6L PDF [100]. In this analysis we consider NlX final state followed by N→llνl.We generate thecombined parton level events using MadGraph and then gradually hadronize and perform detector simulations with xqcut= pTj = 30 GeV and QCUT= 36 GeV for the hadronization. In our analysis we use the matched cross section after the detector level analysis. After the signal events are generated we adopt the following basic criteria, used in the CMS trilepton analysis [74, 75]:(i)
The transverse momentum of each lepton:pTl>10 GeV(ii)
The transverse momentum of at least one lepton:pTl,leading>20 GeV(iii)
The jet transverse momentum:pTj>30 GeV(iv)
The pseudo-rapidity of leptons:ηl<2.4 and of jets: ηj<2.5(v)
The lepton-lepton separation:ΔRll>0.1 and the lepton-jet separation: ΔRlj>0.3(vi)
The invariant mass of each OSSF (opposite-sign same flavor) lepton pair:ml+l-<75 GeV or >105 GeV to avoid the on-Z region which was excluded from the CMS search. Events with ml+l-<12 GeV are rejected to eliminate background from low-mass Drell-Yan processes and hadronic decays(vii)
The scalar sum of the jet transverse momenta:HT<200 GeV(viii)
The missing transverse energy:ɆT<50 GeVThe additional trilepton contributions come fromN→Zν,hν, followed by the Z, h decaying into a pair of OSSF leptons. However, the Z contribution is rejected after the implementation of the invariant mass cut for the OSSF leptons to suppress the SM background and the h contribution is suppressed due to very small Yukawa couplings of electrons and muons. Using different values of ɆT and HT, the CMS analysis provides different number of observed events and the corresponding SM background expectations. For our analysis the set of cuts listed above are the most efficient ones as implemented by the CMS analysis [74, 75]. To derive the limits on VlN2, we calculate the signal cross section normalized by the square of the mixing angle as a function of the heavy neutrino mass mN for both SF and FD cases, by imposing the CMS selection criteria listed above. The corresponding number of signal events passing all the cuts is then compared with the observed number of events at the 19.5 fb−1 luminosity [74, 75]. For the selection criteria listed above, the CMS experiment observed the following:(a)
510 events with the SM background expectation of560±87 events for ml+l-< 75 GeV which is called below the Z-pole(b)
178 events with the SM background expectation of200±35 events for ml+l-> 105 GeV which is called above the Z-poleIn case (a) we have an upper limit of 37 signal events, while case (b) leads to an upper limit of 13 signal events. Using the limits obtained in case (b), we can set an upper bound onVlN2 for a given value of mN. In this analysis we use above the Z-pole situation with 3000 fb−1 luminosity for the 13 TeV LHC and future 100 TeV pp collider. (Exactly the same procedure can be adopted for the situation with ml+l-<75 GeV.)The mixing-squared versusmN contours shown in Figure 26 are allowed by the EWPD within the range 91.2 GeV ≤mN≤163 GeV for the SF case at the 13 TeV LHC at 3000 fb−1 luminosity. At the same time we analyze the FD case through which one can probe the range of 91.2 GeV ≤mN≤195 GeV. The limits for the FD case are roughly twice stronger than the SF case. However, at the future 100 TeV pp collider with 3000 fb−1 luminosity the upper bounds on mN go up to 200 GeV and 275 GeV for the SF and FD cases, respectively, keeping lower mass bound at the 91.2 GeV. As the coupling between the Higgs and RHNs can not distinguish between the Majorana and pseudo-Dirac neutrinos, we use the same limits for both of cases. Similarly the EWPD can measure the deviation from the SM couplings so we can use the same bounds in both cases.Figure 26
Bounds on the square of the mixing angle from the trilepton plus MET final state as a function of the heavy neutrino mass(mN). The shaded region is ruled out by the EWPD and Higgs data. Prospective bounds from the Higgs data had been calculated in [45] for the LHC at the high luminosity (3000 fb−1) and future 100 TeV pp collider.


## 5. Conclusions

In this paper we have studied both type I and inverse Seesaw models where SM singlet RHNs are involved. The RHNs involved in type I Seesaw mechanism are Majorana type whereas those present in the inverse Seesaw model are pseudo-Dirac in nature. We have studied the production mechanisms of the RHNs from various initial states at the 13 TeV LHC and future100 TeV pp collider considering the square of the mixing angle as 10-4 when the RHNs are produced in association with charged lepton and neutral lepton along with the jets. It has been shown due to the prompt decay of Higgs boson (mN<mH) into the RHNs and SM light neutrino that the cross section dominates over all the remaining production modes. Such heavy neutrinos can dominantly decay into the lW mode at the colliders. Depending on the nature of the model we pick up two distinguishing signals from type I Seesaw and inverse Seesaw in the form of same-sign dilepton plus di-jet and trilepton plus MET, respectively.Using the recent searches by the CMS and ATLAS for type I Seesaw with same-sign di-muon and di-jet final state we put a prospective upper bound onVμN2 for the 13 TeV LHC and future 100 TeV pp collider at 3000 fb−1 luminosity. Applying the cuts used in the anomalous multi-lepton search done by the LHC, we can put upper bounds on the square of the mixing angle between the SM light and of the degenerate RHNs. We consider the SF and FD cases where the limits in FD case are twice stronger than the SF case.We have noticed that our currently given projected limits on the square of the mixing angles are better than those obtained from different experiments and even at the current stage of the LHC. We expect improvements in the status at the HL-LHC and future100 TeV pp collider when multilepton final states will be studied from the decays of the RHNs which will lead us to a more optimistic conclusion.



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*Source: 9785318-2018-04-19.xml*