Lepton Flavour Violation in charged leptons within SUSY-seesaw

# Lepton Flavour Violation in charged leptons within SUSY-seesaw

## Abstract

In this paper we review our main results for Lepton Flavour Violating (LFV) semileptonic tau decays and muon-electron conversion in nuclei within the context of two Constrained SUSY-Seesaw Models, the CMSSM and the NUHM. The relevant spectrum is that of the Minimal Supersymmetric Standard Model extended by three right handed neutrinos, and their corresponding SUSY partners, , (). We use the seesaw mechanism for neutrino mass generation and choose a parameterisation of this mechanism that allows us to incorporate the neutrino data in our analysis of LFV processes. In addition to the full one-loop results for the rates of these processes, we will also review the set of simple formulas, valid at large , which are very useful to compare with present experimental bounds. The sensitivity to SUSY and Higgs sectors in these processes will also be discussed. This is a very short summary of the works in Refs. [1] and [2] to which we refer the reader for more details.

\psfragtanb \psfragtan b \psfraglog(mN) \psfragBR(tau -¿ 3mu)BR \psfragBR(tau -¿ 3e)BR \psfragBR(mu -¿ 3e)BR \psfragBR(mu -¿3e)BR \psfragBR(tau -¿ mu + gamma)BR \psfragBR(tau -¿ e + gamma)BR \psfragBR(mu -¿ e + gamma)BR \psfragmod(theta2) \psfragmod(theta1) \runtitle \runauthorE. Arganda, M. Herrero, J. Portoles, A. Rodriguez-Sanchez and A.M. Teixeira

## 1 Framework for LFV in charged leptons

From the present neutrino data on neutrino oscillations, we know that Lepton Flavour Violation (LFV) occurs in the neutral lepton sector. However, we do not know yet if this LFV occurs in the charged lepton as well. Even if it occurs, we do not know either if these two violations are related or not. Within the Standard Model with mass less neutrinos there is not LFV. Futhermore, it is extremely suppressed even with massive neutrinos. In contrast, in supersymmetric (SUSY) models with Majorana neutrinos LFV can be sizeable. In particular, we consider here the spectrum of the Minimal Supersymmetric Standard Model (MSSM) extended with three rigth handed neutrinos, , and their SUSY partners, (), and with the seesaw mechanism implemented to generate the neutrino masses, where it is known that large LFV rates occur. These are induced by the soft SUSY breaking slepton masses and are transmitted to the lepton sector by means of the Yukawa neutrino couplings, which can be large if the neutrinos are of Majorana type, and via loops of SUSY particles. Therefore, in the context we work within of SUSY-seesaw models the LFV in both the neutral and the charged lepton are closely related.

Regarding the seesaw mechanism we use the parameterisation proposed in  [3], which is very useful to implement the neutrino data into our analysis of LFV. With this parameterisation, the Yukawa coupling and Dirac mass matrices are set by , with the orthogonal matrix defined by three complex angles () which represent the additional mixing introduced by the right handed neutrinos. The other quantities in this formula are , GeV; denotes the three light neutrino masses, and the three heavy ones. is given by the three (light) neutrino mixing angles and , and three phases, and . With this parameterisation it is easy to accommodate the neutrino data, while leaving room for extra neutrino mixings (from the right handed sector). It further allows for large Yukawa couplings by choosing large entries in and/or .

Here we focus in the particular LFV proccesses: 1) semileptonic (), (), () decays and 2) conversion in heavy nuclei. The predictions in the following are for two different constrained MSSM-seesaw scenarios, with universal and non-universal Higgs soft masses. The respective parameters (in addition to the previous neutrino sector parameters) are: 1) CMSSM-seesaw: , , , and sign(), and 2) NUHM-seesaw: , , , sign(), and .

The predictions presented here include a full one-loop computation of the SUSY diagrams contributing to these LFV processes and do not use the Leading Logarithmic (LLog) nor the mass insertion approximations. In the case of semileptonic tau decays we have not included the boxes which are clearly subdominant, but we have included correspondingly: the , Z and Higgs bosons, and , mediated diagrams in , and the Z boson and Higgs boson mediated diagrams in . The hadronisation of quark bilinears in all these semileptonic channels is performed within the chiral framework, using Chiral Perturbation Theory [4] to order and Resonance Chiral Theory  [5] whenever the resonances like the , etc., play a relevant role. The predictions for the conversion rates include the full set of SUSY one-loop contributing diagrams, mediated by , Z and Higgs bosons, as well as boxes. In this case we have followed very closely the general parameterisation and approximations of ref. [6].

## 2 Results and discussion

Here we present the predictions for BR() (), BR() (), BR() () and CR(, Nuclei) within the previously described framework and compare them with the following experimental bounds: BR, BR, BR, BR, BR, BR, BR, CR and CR.

As a general result in LFV processes that can be mediated by Higgs bosons we have found that the and contributions are relevant at large if the Higgs masses are light enough. It is in this aspect where the main difference between the two considered scenarios lies. Within the CMSSM, light Higgs and bosons are only possible for low (here we take to reduce the number of input parameters). In contrast, within the NUHM, light Higgs bosons can be obtained even at large . In Fig. 1 it is shown that some specific choices of and lead to values of and as low as 110-120 GeV, even for heavy values above 600 GeV. Therefore, the sensitivity to the Higgs sector is higher in the NUHM.

We start by presenting

the results for the semileptonic tau decays. The mentioned sensitivity to the Higgs sector within the NUHM scenario can be seen in Fig. 2. Concretely, the BRs of the channels , , , , and present a growing behaviour with , in the large region, due to the contribution of light Higgs bosons, which is non-decoupling. The decays involving Kaons and mesons are particularly sensitive to the Higgs contributions because of their strange quark content, which has a stronger coupling to the Higgs bosons. On the other hand, the largest predicted rates are for and , dominated by the photon contribution, which are indeed at the present experimental reach in the low region.

The comparison between the various contributions to the semileptonic LFV tau decays in the NUHM scenario for BR() and BR() can be seen in Fig. 3. It is clear from this figure, that is dominated by the photon contribution, except in the large region , say GeV, and large region, say , where the Higgs boson contribution plays an important role. Similar results are found for . In contrast, in , the photon contribution dominantes largely the rates in all the studied region of the parameter space and therefor it is not sensitive at all to the Higgs sector. In the channel, only the Higgs boson contributes, but the rates are extremely small. They are indeed much smaller that decays into kaons due to the fact that the Higgs couplings to the pions are proportional to whereas the the Higgs couplings to the pions are proportional to . On the other hand, the channel is dominated by the Higgs boson contribution for all values, and for moderate and large , say . Notice that for smaller values of it is, however, dominated by the Z boson contribution.

A set of useful formulae for all these channels, within the mass insertion approximation which are valid at large , have also being derived by us in [1]. We include the most relevant of these aproximate formulas here, for completeness. The approximate results for the -mediated contributions and the -mediated contributions are shown separately for comparison,

 BR(τ→μη)Happrox= 1.2×10−7|δ32|2(100mA0(GeV))4(tanβ60)6 BR(τ→μη′)Happrox= 1.5×10−7|δ32|2(100mA0(GeV))4(tanβ60)6 BR(τ→μπ)Happrox= 3.6×10−10|δ32|2(100mA0(GeV))4(tanβ60)6 BR(τ→μπ0π0)Happrox= 1.3×10−10|δ32|2(100mH0(GeV))4(tanβ60)6 BR(τ→μπ+π−)Happrox= 2.6×10−10|δ32|2(100mH0(GeV))4(tanβ60)6 BR(τ→μK+K−)Happrox= 2.8×10−8|δ32|2(100mH0(GeV))4(tanβ60)6 BR(τ→μK0¯K0)Happrox= 3.0×10−8|δ32|2(100mH0(GeV))4(tanβ60)6 BR(τ→μπ+π−)γapprox= 3.7×10−5|δ32|2(100MSUSY(GeV))4(tanβ60)2 BR(τ→μK+K−)γapprox= 3.0×10−6|δ32|2(100MSUSY(GeV))4(tanβ60)2 BR(τ→μK0¯K0)γapprox= 1.8×10−6|δ32|2(100MSUSY(GeV))4(tanβ60)2

We have shown that the predictions with these formulae agree with the full results within a factor of about 2. In the case of this comparison is shown in Figs. 3 and  4. It is also clear, from Fig. 3 that the approximation works much better in the large region, where the boson dominates. Similar conclusions are found for . The next relevant channel in sensitivity to the Higgs sector is , but it is still below the present experimental bound. To our knowledge, there are not experimental bounds yet available for and .

Finally, the maximum sensitivity to the Higgs sector is found for and channels, largely dominated by the boson exchange. Fig. 4 shows that BR() reaches the experimental bound for large heaviest neutrino mass, large , large angles and low . For the choice of input parameters in this figure, it occurs at GeV, , and GeV.

Next we comment on the results for conversion in nuclei. Fig. 5 shows our predictions of the conversion rates for Titanium as a function of in both CMSSM and NUHM scenarios. As in the case of semileptonic tau decays, the sensitivity to the Higgs contribution is only manifest in the NUHM scenario. The predictions for CR(, Ti) within the CMSSM scenario are largely dominated by the photon contribution and present a decoupling behaviour at large . In this case the present experimental bound is only reached at low . The perspectives for the future are much more promising. If the announced sensitivity by PRISM/PRIME of is finally attained, the full studied range of will be covered.

Fig. 5 also illustrates that within the NUHM scenario the Higgs contribution dominates at large for light Higgs bosons. The predicted rates are close to the present experimental bound not only in the low region but also for heavy SUSY spectra. As in the previous semileptonic tau decays, we have also found a simple formula for the conversion rates, within the mass insertion approximation, which is valid at large  [2] and can be used for further analysis. This is dominated by the Higgs contribution and is given by,

 CR(μ−e,Nucleus)|Happrox≃ m5μG2Fα3Z4effF2p8π2Z(Z+N)2∣∣g(0)LS∣∣21Γcapt, g(0)LS=g248π2G(s,p)Smμmsm2H0δ21(tanβ)3

It shows clearly the relevant features: the enhacement of the rates, the Higgs mass dependence, , and the strange quark mass dependence, .

The predictions of the conversion rates for several nuclei are collected in Fig. 6. We can see again the growing behaviour with in the large region due to the non-decoupling of the Higgs contributions. At present, the most competitive nucleus for LFV searches is Au where, for the choice of input parameters in this figure, all the predicted rates are above the experimental bound. We have also shown in [2] that conversion in nuclei is extremely sensitive to , similarly to and and, therefore, a future measurement of this mixing angle can help in the searches of LFV in the sector.

In conclusion, we have shown that semileptonic tau decays nicely complement the searches for LFV in the sector, in addition to . The future prospects for conversion in Ti are the most promising for LFV searches. Both processes, semileptonic tau decays and conversion in nuclei are indeed more sensitive to the Higgs sector than .

## Acknowledgements

M.J. Herrero would like to thank the organizers of this tau-08 conference for the invitation to participate in this interesting and fruitful event. She also acknowledges project FPA2006-05423 of Spanish MEC for finantial support.

### References

1. E. Arganda, M. J. Herrero and J. Portoles, JHEP0806 (2008) 079 [arXiv:0803.2039 [hep-ph]].
2. E. Arganda, M. J. Herrero and A. M. Teixeira, JHEP 0710 (2007) 104 [arXiv:0707.2955 [hep-ph]].
3. J. A. Casas and A. Ibarra, Nucl. Phys. B 618 (2001) 171 [arXiv:hep-ph/0103065].
4. S. Weinberg, PhysicaA 96 (1979) 327; J. Gasser and H. Leutwyler, Annals Phys. 158 (1984) 142.
5. G. Ecker, J. Gasser, A. Pich and E. de Rafael, Nucl. Phys. B 321 (1989) 311;
6. Y. Kuno and Y. Okada, Rev. Mod. Phys. 73 (2001) 151 [arXiv:hep-ph/9909265].
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