Search for light sterile neutrinos from W^{\pm} decays at the LHC

Search for light sterile neutrinos from decays at the LHC

Claudio O. Dib claudio.dib@usm.cl Department of Physics and CCTVal, Universidad Técnica Federico Santa María, Valparaíso 2340000, Chile    C.S. Kim cskim@yonsei.ac.kr Department of Physics and IPAP, Yonsei University, Seoul 120-749, Korea Institute of High Energy Physics, Dongshin University, Naju 58245, Korea    Sebastian Tapia Araya s.tapia@cern.ch Department of Physics, University of Illinois at Urbana-Champaign, Urbana, IL 61801, USA
August 20, 2019
August 20, 2019
Abstract

We study the feasibility to observe sterile neutrinos at the LHC, with masses in the range 5 GeV  GeV, using exclusive semileptonic modes involving pions and . We thus cover a mass window for sterile neutrinos which is between what can be studied in meson factories and high energy colliders. We run simulations to study these exclusive events where pions should be distinguished from the background provided the neutrino decay exhibits a vertex displacement from its production point. In a previous work we have estimated the theoretical rates and here we analyze the observability of the processes at the LHC, given the fact that exclusive hadronic states may be difficult to identify. If a sample of bosons is available the end of the LHC Run 2, a sterile neutrino in the above mass range could be discovered, or at least the current bounds on the heavy-to-light lepton mixings could be improved by an order of magnitude, . Studying in addition equal sign and opposite sign dileptons, the Majorana or Dirac character of the sterile neutrino could be revealed.

preprint: NCTS-PH/1801

I Introduction

The discovery of neutrino oscillations  Fukuda et al. (1998); Ahmad et al. (2002); Eguchi et al. (2003) implies that at least two of the three neutrinos that participate in the weak interactions must be massive. Since neutrinos are massless in the Standard Model, these particles have become an important portal to physics beyond the Standard Model Gonzalez-Garcia and Maltoni (2008); Mohapatra and Smirnov (2006); Barger et al. (2003); Strumia and Vissani (2006). Now, the smallness of the observed neutrino masses is usually explained by introducing right-handed neutrinos, which must be sterile under electroweak interactions, inducing scenarios with a seesaw mechanism Minkowski (1977); Yanagida (1979); Ramond (1979); Gell-Mann et al. (1979); Glashow (1980); Mohapatra and Senjanovic (1980); Schechter and Valle (1982). While originally the seesaw mechanism resorted to the presence of very heavy extra neutrinos, there are also models where the extra fields are not so heavy, leaving the open possibility that the extra sterile neutrinos could have masses in the broad range from eV to TeV Deppisch et al. (2015), and so experimental searches must also cover all those possibilities. Indeed there are plenty of scenarios in the literature to explain the light neutrino masses. These masses can be generated at tree level or as loop contributions, and they almost invariably require the inclusion of extra fields. The so called type I, II and III include fermion singlets, scalar triplets and fermion triplets, respectively. Loop generated masses also include extra fields, typically scalars and/or fermions. Some of the scenarios may contain candidates for Dark Matter. In summary, in order to discriminate from the different scenarios that extend the Standard Model it will be important to know at least whether there exist extra neutral fermions, and in the affirmative case, to know their masses and whether they are Majorana or Dirac particles.

LHC searches for sterile neutrinos with mass above  Chatrchyan et al. (2012); Aad et al. (2015) are based on the inclusive processes ,  Keung and Senjanovic (1983); del Aguila et al. (2007); Atre et al. (2009); Das et al. (2018). For below , the jets are not energetic enough to pass the background reduction cuts, so purely leptonic modes could be preferred Cvetic et al. (2012); Dib and Kim (2015); Izaguirre and Shuve (2015); Dib et al. (2016, 2017a, 2017b); Dube et al. (2017), even though they have the problem of missing energy and flavor number due to the undetectable final neutrino. However, as one goes to lower searches, again low leptons plus missing neutrinos affect the observability of these leptonic decays. Now, for neutrino masses below GeV, there is an advantage: the neutrino may live long enough to leave an observable displacement from its production to its decay point, a feature that helps drastically reduce the backgrounds Helo et al. (2014); Dib and Kim (2014); Cottin et al. (2018). We then proposed to go back to using semileptonic modes for the searches in this mass range, but now with exclusive channels instead of jets Dib et al. (2018). Again, for below 5 GeV, factories may be more appropriate to search for the sterile neutrino than high energy hadron colliders, due to the cleaner environment and the production of in or lighter meson decays Cvetic et al. (2010); Aaij et al. (2012); Cvetic and Kim (2017); Dib et al. (2000); Kim et al. (2017).

For the sterile neutrino mass range of 5 GeV 20 GeV, in a previous work Dib et al. (2018) we proposed to use neither nor trilepton events, but the exclusive semileptonic processes , followed by , and , which are modes with no missing energy. The decay channels in the secondary process were not considered in order to avoid misidentification of electrons and pions. We concluded that the most promising modes should be followed by a displaced decay either , or for a Majorana sterile neutrino, or followed by , or for a Dirac neutrino. We studied those rates, including the comparison of different models for the pion form factors.

Now in this article we want to complement the previous work by studying the observability of these processes at the LHC. In general, the observability of these modes is not a trivial matter, since pions with relatively low need to be selected from backgrounds; neutral pions, which decay almost instantly into , are also difficult to identify; pions and electrons should be clearly distinguished in order to avoid fake signals. On the other hand, the vertex separation due to the sizable lifetime of the sterile neutrino with mass below 20 GeV Helo et al. (2014); Dib and Kim (2014); Cottin et al. (2018); Nemev?ek et al. (2018); Cottin (2018) can help to reject considerably all backgrounds.

In Section II we review the processes in question in very brief form, as more details can be found in the previous work Dib et al. (2018). In Section III we present our current analysis and simulations, where we study the detectability of the processes at the LHC. In Section IV we state our conclusions.

Ii Theoretical summary of the processes

Here we give a short summary on our previous work on the decay and decays with . Detailed formulae with full theoretical discussions are shown in Ref. Dib et al. (2018).

ii.1 The decay :

The leptonic sector in a generic SM extension includes one or more extra neutral lepton singlets, , in addition to the three generations of left-handed SM lepton doublets. The neutral lepton singlets are known as sterile neutrinos, because they do not directly interact with other SM particles in the absence of any mixing with the active neutrino sector.

At the LHC, sterile neutrinos with masses around will be mainly produced from the decay of on-shell bosons. The decay rate can be easily calculated, neglecting the lepton mass, the branching ratio is:

(1)

where GeV is the total decay width of the boson Patrignani et al. (2016). From here, the heavy neutrino can decay in several modes, depending on its mass. Here we are interested in the decays into pions, namely , and . Both charged modes will occur for a Majorana , while for a Dirac only the decays into a negative charged lepton will be produced.

ii.2 The decay :

The mode is a charged current process:

(2)

where and denote the mass of the charged pion and sterile neutrino, respectively; is the CKM matrix and is the pion decay constant; the function is defined as . The formation of a single pion in the final state is relatively suppressed with respect to multi pion modes, because it requires the two produced quarks to remain close together. Indeed, the suppression relative to the open quark production is about , which is for GeV Dib et al. (2018).

ii.3 The decay :

The decay into two pions, , is similar to the lepton decay in terms of their interaction lagrangian and Feynman diagram, except for the lepton flavor and charge. However, one must be aware that the kinematic range for the form factor in the decays is extended to higher , so an extrapolation of the form factor will be required. Considering the above, the differential decay rate for can be written as

(3)

where , , , , , and is the hadronic form factor of the charged current, defined by

(4)

The decay rate is then obtained after integrating over , within the limits and . This expression is analogous to Cirigliano et al. (2001, 2002). The form factor in the time-like region, i.e. , is experimentally known from  Fujikawa et al. (2008) in the limited range . The extrapolation to larger values of is done in our previous work Dib et al. (2018), based on two alternatives: a vector dominance model Lees et al. (2012) and on light front holographic QCD Brodsky et al. (2015). They both give very similar results Dib et al. (2018).

ii.4 The decay :

In much the same way as in the two-pion mode, the differential decay rate of the general hadronic decay can be written in terms of form factors with an expression identical to that of the tau decay Gómez Dumm et al. (2010), again provided that the form factors are extrapolated to larger values of . Denoting the momentum and mass of the hadron () by and respectively, and defining the momentum of the hadronic part by , the differential decay rate can be expressed as:

(5)

In this expression, the functions and are given in Ref Dib et al. (2018).

The decay rate is obtained after integration over within the limits and .

ii.5 Theoretical results

With the expressions described above we were able to estimate the exclusive semileptonic decay rates of into , and , for a neutrino with mass in the range 5 to 20 GeV, produced at the LHC in the process .

Figure 1: “Canonical” decay rates for , , and the inclusive mode (left) and “canonical” branching ratios for the full processes (right) as a function of the neutrino mass , with all mixing factors removed. To obtain the actual values, the “canonical” values must be multiplied by the factor (left), or (right).

In Fig. 1 (left) we reproduce what we called the “canonical” decay rates for the modes and the inclusive estimate given by as a function of the neutrino mass (“canonical” here means that all lepton mixing elements are factorized out of the expressions). In Fig. 1 (right) we show the “canonical” branching ratios for the full processes and . The actual rates (left) and branching ratios (right) can be obtained by multiplying these canonical values by (left) and (right), respectively. From these figures we were able to estimate the expected number of events at the LHC, or equivalently the minimal value of the lepton mixing element that would generate 5 events or more, for a benchmark value of  GeV. At this mass, the figure gives a canonical branching ratio

(6)

According to Ref. Aad et al. (2016), at the end of the LHC Run II one may expect a sample of decays. Therefore, in order to obtain more than 5 events, we must have:

which implies , provided other mixing elements are smaller. If instead all mixing elements are comparable, then this lower bound increases by a factor 3, i.e. . These results are in ideal conditions, with no cuts or backgrounds. These bounds can be made about one order of magnitude stronger if one adds both charges and all lepton flavors , i.e. .

One last important point in the observability of these processes is the long lifetime of , which would cause an observable displacement in the detector between the production and decay vertices of . This displacement will drastically help reduce the possible backgrounds. For a sterile neutrino with mass in the range 5 GeV to 20 GeV, the total width can be estimated as Dib and Kim (2015):

(7)

The lighter is, the longer it will live, for a given mixing . Using the current upper bound , we find that vertex displacements should be in the range to 20 (for 20 GeV and 5 GeV respectively). The relativistic factor will increase the displacement and a smaller mixing as well.

Iii Detector simulations and Discussion

Now we run simulations in order to study the observability of these modes at the LHC. In principle they could be observed provided the pions can be identified and the background can be reduced using the spatial displacement between the production and decay vertices of the heavy neutrino . This vertex displacement should be observable for below 20 GeV Helo et al. (2014); Dib and Kim (2014).

We use MadGraph5_aMC@NLO Alwall et al. (2014) to generate heavy neutrinos via the charge current Drell-Yan process shown in Fig. 2. Then, decay and hadronization processes are done with Pythia 8.1 Sjostrand et al. (2008, 2006). A fast detector simulation is performed by Delphes 3 de Favereau et al. (2014); we use the card ATLAS.tcl included in the package. The UFO Degrande et al. (2012) files were implemented with Wolfram Mathematica Inc. using the FeynRules libraries Alloul et al. (2014). In our simulations we consider a sample of 15 thousand events.

Figure 2: Heavy-neutrino produced via charged current Drell-Yann process: . The second muon as corresponds to a Majorana ; for it corresponds to either a Dirac or Majorana .

Concerning the and reconstruction, the events are selected based on the ATLAS/CMS Aad et al. (2008); Chatrchyan et al. (2008) standard requirements: muon GeV, , and tracks MeV and . As the heavy-neutrino mass is considered to be smaller than 20 [GeV], the quarks produced in the neutrino decay are likely to hadronize in the specific pion states described above. We also require events with at least two muons where one of them must show a transverse momentum significantly larger than the other.

The two muons plus the pions coming from the decay should reconstruct the mass. In addition, the less energetic muon plus the pions should reconstruct the mass. However, we must take into account that the neutral pions in the processes will not be detected: they decay immediately into two rather collinear photons which will not have enough energy to be distinguished from noise in the EM calorimeter, in the cases of interest GeV. Therefore, we can have only two types of events: () the muons and one charged pion and () the muons and three charged pions. The latter corresponds clearly to , but the former will be the sum of the three decay modes, namely , and .

Figure 3: Simulation of a heavy-neutrino reconstructed in hypothetically isolated processes (left) and (right) where the cannot be detected. In both cases the invariant mass is of the pair muon-charged pion. Red: idealized case where all particles including neutral pions are detected. Blue: simulation where neutral pions are not detected. Green: same as Blue but smeared by detector resolution (Delphes). A sample of 15 k events was used, with a benchmark GeV.

In Fig. 3 (left) we show the simulation of the hypothetical case in which the decay into a single pion, , could be separated from the decays (this separation is not realistic because neutral pions are not detected). The peak at is clear. In Fig. 3 (right), we simulate the decay into two pions, where one of the pions has to be neutral due to charge conservation: . Now, since the is not observed, the distribution shows that effect as an extended continuum into lower invariant masses, with an upper cutoff at .

Figure 4: Simulation of a heavy-neutrino reconstructed in hypothetically isolated process (left) and in the three-charged pion mode . Red: idealized case where all particles including neutral pions are detected. Blue: simulation where neutral pions are not detected. Green: same as Red but smeared by detector resolution. A sample of 15 k events was used, with a benchmark GeV.

In Fig. 4 we show the simulations for the decay into three pions. Now there are two modes: (left) and (right). In Fig. 4 (left) one can see again a continuous distribution due to the missing , which is even more pronounced to low invariant masses of the charged pair, compared to the single missing of Fig. 3 (left). In contrast, the three-charged pion mode shows in Fig. 4 (right) shows a clear reconstruction of the peak at .

In a realistic case, therefore, the search for a mode with a single charged pion will be the sum of the three pionic final states, , and , as we show in the simulations of Fig. 5 (there are modes with even more pions, but those are suppressed with respect to the three cases considered here). Fig. 5 (left) shows the result from Pythia and Fig. 5 (right) the smeared distribution due to detector resolution given by Delphes. The latter is a more spread distribution, but qualitatively they are similar in the sense that the dominant feature is a continuous distribution with an upper endpoint at the mass. The single pion decay channel with no neutral pions, namely , which is the only mode with a clear peak, is suppressed compared to the other two channels and its peaked feature is lost in the distribution. This feature contrasts with the events with 3 charged pions, shown in Fig. 4 (right), where the peak is still clear. In a real search there should be a continuous part due to the 4-pion mode, but it is subdominant.

Besides the reconstruction of the , one should verify the reconstruction of the from the full event, which essentially adds the prompt muon to the decay of . Given that we are considering GeV, i.e. considerably lighter than , the prompt muon should be more energetic that the one coming for the decay and, due to the relatively long lifetime of an with such masses, the decay vertex of should be displaced with respect to the prompt muon. Figs. 6 show the distributions for the reconstruction in the respective modes for the decays described above, namely with a single charged pion (Fig. 6 left) and in the mode with three charged pions (Fig. 6 right).

Figure 5: Simulation of a heavy neutrino reconstructed in events with a muon and a single charged pion. The events combine the decays into , and where the neutral pions are missing. A sample of 15 k events was used, with a benchmark GeV.
Figure 6: Simulation of the boson decaying into followed by the decay, reconstructed in events with two muons and a single charged pion (left), and three charged pions (right). A sample of 15 k events was used, with a benchmark GeV.

Considering backgrounds, in order to eliminate them we can request:

1) Minimal amount of missing : with this cut we remove all events that have SM neutrinos, such as or production.

2) Displaced vertex, associated with the muon with lower . Since GeV, the prompt muon, which is associated with the production, is more energetic that the second muon, which comes from the decay. Moreover, since is long-living for GeV, the second muon should come from a displaced secondary vertex. This cut should remove almost all remaining backgrounds with the exception of heavy-flavors, e.g -hadrons, that typically decay into one displaced muon plus tracks. We can remove the heavy-flavor background by requiring isolation in the prompt muon in addition to requirement that the invariant mass of the two muons plus the tracks should be close to the W mass.

Iv Conclusions

In this work we have studied the observability at the LHC of the exclusive process , which is appropriate to discover a sterile neutrino with mass in the range 5 GeV GeV. This is an intermediate region where neither rare meson decays (, , etc.) nor modes at the LHC are sensitive to the presence of such neutrinos. The modes we use are exclusive semileptonic, containing pions in their hadronic component. Because of the pions in the final state, the reconstruction of the events at a hadron collider is not a trivial matter. However, one particular feature of this process that helps reducing drastically all backgrounds is the fact that a sterile neutrino with mass below 20 GeV should have a lifetime long enough to travel an observable distance in the detector before it decays. Indeed, given the current upper bounds on the sterile neutrino mixing with the muon flavor , a vertex displacement above 20 would occur for GeV, and longer than 20 for GeV.

Naively, the most favorable mode should have a single charged pion in the final state, namely . However this mode is suppressed compared to the two-pion and three-pion modes. Moreover, since neutral pions would go undetected at the LHC, the single charged pion events will contain the modes and as well. We have simulated the events that contain one prompt muon, followed by a displaced muon and charged pion (the second muon should also have less than the prompt muon). The invariant mass of the displaced charged particles will show a continuous distribution with an upper endpoint at the mass, and the invariant mass of all three charged particles will show a continuous distribution with an endpoint at .

Accordingly, the cleanest mode is the one with three charged pions in the final state: . Modes with more pions are suppressed compared to this one, so we have neglected their effect in the invariant mass distributions (one would expect only a small continuous tail to lower invariant masses, due to the modes with additional neutral pions that go undetected). In this mode, the invariant mass of the secondary muon and the charged pions will show a peak at and the invariant mass that includes the prompt muon will show a peak at .

These exclusive semileptonic processes, including the feature of vertex displacement, are therefore observable at the LHC, provided is within the range indicated and the mixing is within a few orders of magnitude of the current bound. Complementary, if no signal is found, these searches will improve the current upper bounds on the mixing of sterile neutrinos with the muon flavor by at least one order of magnitude.

Acknowledgements

C.S.K. was supported in part by the National Research Foundation of Korea (NRF) grant funded by the Korean government (MSIP) (NRF-2018R1A4A1025334). S.T.A was supported by the National Science Fundation (NSF) grant 1812377. This work was supported by FONDECYT (Chile) grant 1170171 and and CONICYT (Chile) PIA/Basal FB0821.

References

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