Chiral Enhancement in the MSSM – An Overview

# Chiral Enhancement in the MSSM -- An Overview

## Abstract

In this article I review the origin and the effects of chirally enhanced loop-corrections in the MSSM based on Refs. [1, 2, 3]. Chiral enhancement is related to fermion-Higgs couplings (or self-energies when the Higgs field is replaced by its vev). I describe the resummation of these chirally-enhanced corrections to all orders in perturbation theory and the calculation of the effective fermion-Higgs and gaugino(higgsino)-fermion vertices. As an application a model with radiative flavor-violation is discussed which can solve the SUSY-CP and the SUSY-flavor problem while it is still capable of explaining the observed deviation from the SM in the mixing phase.

\instlist

Albert Einstein Center for Fundamental Physics, Institute for Theoretical Physics,
University of Bern, CH-3012 Bern, Switzerland. \PACSes14.65.Fy,14.80.Da,14.80.Ly

## 1 Introduction

In this article I summarize recent progress in the field of chirally enhanced self-energies in the MSSM done in collaboration with Jennifer Girrbach, Lars Hofer, Ulrich Nierste, Janusz Rosiek and Dominik Scherer. The discussion will skip the technical aspects and subtleties and instead focus on the essential features. The interested reader is referred to Refs. [1, 2, 3] for a detailed discussion.

In the standard model chirality violation is suppressed by small Yukawa couplings (except for the top quark). However, the MSSM does not necessarily possess the same suppression effects since the bottom Yukawa coupling can be big at large of and also the trilinear -terms do not necessarily respect the hierarchy of the Yukawa couplings. Thus, chirality-flipping self-energies can be enhanced either by a factor of [4] or by a ratio . This enhancement can compensate for the loop suppression leading to corrections which are of the same order as the corresponding physical quantities, i.e. of order one. These large corrections must be taken into account to all orders in perturbation theory (Sec. 3) leading to effective fermion-gaugino and fermion-Higgs couplings (see Sec. 4).

It is even possible that light-fermion masses and the CKM elements are entirely due to radiative corrections involving the trilinear -terms [5]. Such a model of radiative flavor-violation can solve the SUSY-CP [6] and the SUSY-flavor problem while still leading to interesting effects in flavor-observables (see Sec. 5).

## 2 Self-energies

One can decompose any fermion self-energy into chirality-flipping and chirality-conserving parts in the following way:

 Missing dimension or its units for \hskip (1)

Here and are flavor indices running from to . Since the SUSY particles are known to be much heavier than the SM fermions it is possible to expand in the external momentum. For our purpose it is even sufficient to work in the limit in which only the chirality-flipping parts remain. It is well known that in the MSSM these self-energies can be enhanced either by a factor [4] or by a factor [2] which compensates for the loop-suppression and leads to order one corrections. The chirality-changing part of the fermion self-energy (at , involving sfermions and gauginos(higgsions)) can be written as

 Σf~λLRji=−116π26∑s=1N∑I=1m~λIΓ~λIL⋆fj~fsΓ~λIRfi~fsB0(m2~λI,m2~fs). (2)

Here stands for the SUSY fermions () and denotes their corresponding number (2 for charginos, 4 for neutralinos and 8 for gluinos). The coupling coefficients and the loop functions are defined in the appendix of Ref. [1].

The couplings in Eq. (2) involve the corresponding sfermion mixing matrices which diagonalize the sfermion mass matrices: . In the case of neutralino-quark-squark and chargino-quark-squark vertices they also depend on Yukawa couplings and CKM elements.

An interesting feature of the self-energies in Eq. (2) is that they are finite and that they do not vanish in the limit of infinitely heavy SUSY masses. We refer to this approximation in which only such non-decoupling terms for the self-energies are kept as ”the decoupling limit”. Note, however, that we do not integrate out the SUSY particles but rather keep them as dynamical degrees of freedom.

Let us take a closer look at the quark self-energy with squarks and gluinos as virtual particles1. To leading order in , the self-energy is proportional to one chirality flipping element of the squark mass matrix:

 Σq~gLRfi = 2αs3πm~g3∑j,k,j′,f′=16∑s,t=1ΛqLLsfjΔqLRjkΛqRRtkiC0(m2~g,m2~qLm,m2~qRn). (3)

Here the off-diagonal elements of the sfermion mass matrices are given by

and the matrices take into account the flavor changes due to bilinear terms. Note that in the decoupling limit depends only on the bilinear terms.

For equal SUSY masses we can give a simple approximate formula for the self-energy in Eq. (3):

 Σd~gLRfi = −1100vd(Adfi/MSUSY+Yditanβδfi) (5) Σu~gLRfi = −1100vu(Aufi/MSUSY+Yuicotβδfi) (6)

Thus, generic -terms which are of the order lead to self-energies which are approximatly . The part of Eq. (6) containing is of the order of 2 GeV for . In the case of up-quarks, only the part of the self-energy proportional to can be important: it is of the order of 1.5 GeV for .

According to Eq. (4) and Eq. (6) the quark self-energy with a gluino as virtual particle can be divided into a part linear in a Yukawa coupling and a part linear in an -term. Such a decomposition is possible for all self-energies (in the decoupling limit) because either a Yukawa coupling or a trilinear -term is needed in order flip the chirality. Thus, we can also decompose the chargino self-energies (we do not consider the neutralino self-energy here, because it is usually subleading) in an analogous way. In the flavor changing case we also have to distinguish whether the flavor-change is due to a CKM element or not which is important when we consider later the CKM renormalization. Thus we decompose the down-quark self-energy as follows:

 ΣdLRii=ΣdLRiiYdi+vuYdiϵdiΣdLRfi=ΣdLRfiCKM+md3V(0)⋆3fϵFCδi3forf≠i (7)

Here is the part of the flavor-conserving down-quark self-energy proportional to divided by , is the sum of all self-energies where the flavor-change is not due to CKM elements and arises from the part of the chargino self-energy where the flavor change comes from a CKM element:

 ϵdFC=−116π2μYd3md33∑m,n=1Yu3⋆ΛqLLm33ΔuLR⋆33ΛuRRn33C0(|μ|2,m2~qLm,m2~uRn). (8)

For the discussion of the effective Higgs vertices we also need a decomposition of into its holomorphic and non-holomorphic parts. Here non-holomorphic means that the loop-induced coupling is to the other Higgs doublet than the on involved in the Yukawa-term of the superpotential, i.e. for down-quarks the self-energy involves and for up-quarks the self-energy contains . In the decoupling limit all enhanced holomorphic self-energies are proportional to -terms and we denote the the sum as , while the non-holomorphic part is denoted as :

 ΣfLRji=ΣfLRjiA+Σ′fLRji. (9)

## 3 Renormalization

Chirally-enhanced self-energies modify the relation between the bare Yukawa couplings and the corresponding physical fermion masses . For quarks we have the relation:

 mqi=vqYqi+ΣqLRii,(q=u,d). (10)

Eq. (10) implicitly determines the bare Yukawa couplings for a given set of SUSY parameters. In the up-quark sector the enhanced terms in the self-energy are independent of . Therefore Eq. (10) is easily solved for and one finds

 Yui=(mui−ΣuLRii)/vu. (11)

In the down-quark sector we have terms proportional to one power of at most (in the decoupling limit) and by solving Eq. (10) we recover the well-known resummation formula [7] with an extra correction due to the -terms [8]2:

 Ydi=mdi−ΣdLRiiYivd(1+tanβϵdi) (12)

The flavor-changing self-energies induce wave-function rotations in flavor-space which have to be applied to all external fermion fields. At the two-loop level is given by

 UqL=⎛⎜ ⎜ ⎜ ⎜ ⎜⎝1−12∣∣σq12∣∣2σq12+mq1mq2σq⋆21σq13+mq1mq3σq⋆31−σq⋆12−mq1mf2σq211−12∣∣σq12∣∣2σq23+mf2mq3σq⋆32−σq⋆13−mq1mq3σq31+σq⋆12σq⋆23−σq⋆23−mq2mq3σq321⎞⎟ ⎟ ⎟ ⎟ ⎟⎠, (13)

where we have neglected terms which are quadratic or of higher order in small quark mass ratios and we have defined the abbreviation . The corresponding expressions for is obtained from the one for by replacing . The rotations in Eq. (13) also renormalize the CKM matrix. The bare CKM matrix , which arises because of the misalignment between the bare Yukawa couplings, is now determined through the physical one by

 V(0)=UuLVUdL†. (14)

This equation can be solved analytically by exploiting the CKM hierarchy. First one calculates the effects of which lead to an additive change in the CKM elements. Then the self-energies containing CKM elements lead to a scaling of new CKM elements elements by a factor (similar to Eq. (12)).

## 4 Effective Vertices

### 4.1 Higgs Vertices

The effective Higgs vertices are most easily obtained in an effective field theory approach [9] which is an excellent approximation to the full theory. In addition to the flavor-diagonal holomorphic couplings of quarks to the Higgs fields flavor-changing couplings to both Higgs doublets are induced via loops. The resulting effective Yukawa-Lagrangian is that of a general 2HDM of type III and is given (in the super-CKM basis) by:

 LeffY=¯QafL[(Ydiδfi+Edfi)ϵabHbd−E′dfiHa⋆u]diR−¯QafL[(Yuiδfi+Eufi)ϵabHbu+E′ufiHa⋆d]diR. (15)

Here and denote  - indices and is the two-dimensional antisymmetric tensor with . The loop-induced couplings are given by

 Edij=ΣdLRijAvd,E′dij=Σ′dLRijvu,Euij=ΣuLRijAvu,E′uij=Σ′uLRijvd. (16)

Diagonalizing the effective quark mass matrices (after electroweak symmetry breaking) and decomposing the Higgs fields into their physical components leads to the following effective neutral Higgs couplings:

 ΓH0kLReffufui=xku(muivuδfi−˜E′uficotβ)+xk⋆d˜E′ufi,ΓH0kLReffdfdi=xkd(mdivdδfi−˜E′dfitanβ)+xk⋆u˜E′dfi, (17)

with

 ˜E′qfi=UqL∗jfE′qjkUqRki≈E′qfi−ΔE′qfi, (18) Missing or unrecognized delimiter for \right

The new term is especially interesting: it contains a non-holomorphic flavor-conserving part which multiplies a flavor-changing holomorphic term. In this way the holomorphic -terms can lead to flavor-changing neutral Higgs couplings. The origin of this term can be understood in the following way: Even though the couplings are holomorphic, they lead to an additional rotation (if is flavor non-diagonal) which is needed to diagonalize the effective quark mass matrix. These rotations then lead to off-diagonal neutral Higgs couplings even if is flavor conserving. This effect will allow us to explain the mixing in our model with radiative flavor-violation.

### 4.2 Gaugino(Higgsino)-Fermion-Vertices

Effective gaugino(higgsino)-fermion-vertices which include the chirally-enhanced corrections are obtained by inserting the bare values for the Yukawa couplings and the CKM elements into the corresponding Feynman-rules and applying the wave-function rotations in Eq. (13) to all external fermion fields. Since the genuine vertex corrections are not enhanced, these vertices then include all chirally enhanced effects.

The smallness of the off-diagonal CKM elements and the Yukawa couplings of the first two generations suggests the idea that these quantities might be due to radiative corrections, i.e. they are zero at tree-level. Indeed, as we have see previously, the self-energies involving the trilinear -terms lead to order one effects in the renormalization of the CKM elements and the light fermion masses and it is possible that they are generated by the self-energy radiative corrections [5]. From Eq. (6) we see that this is the case if the -terms are of the same order as the other SUSY parameters.

However, the third generation fermion masses are too heavy to be loop generated (without unnaturally large values for the -terms which would violate vacuum stability[10]) and the successful bottom – tau (top – bottom) Yukawa coupling unification in SU(5) (SO(10)) GUTs suggests to keep the third generation fermion masses. Thus we assume the following structure for the Yukawa couplings of the MSSM superpotential:

 Yfij=Yf3δi3δj3,V(0)ij=δij. (19)

This means that (in the language of [11]) the global flavor symmetry of the gauge sector is broken down to by the Yukawa couplings of the third generation. Here the five factors correspond to rotations of the left-handed doublets and the right-handed singlets of the first two generation fermions in flavor space, respectively.

Let us first consider the quark sector. Here we demand that the light quark masses and the off-diagonal CKM elements are generated by gluino self-energies. Regarding only the first two generations, no direction in flavor space is singled out by the Yukawa term in the superpotential and the Cabbibo angle is generated by a misalignment between and 3. Regarding the third generation, the situation is different because their non-zero Yukawa couplings fix the quark-field rotations involving the third generation. Thus are generated by a misalignment between the , and the third generation Yukawa couplings. We will consider the two limiting cases in which the CKM elements arise only from a mismatch between () and () which we call CKM generation in the down (up) sector for obvious reasons. This means we require

 ΣdLR23=mbVcb≈−mbV∗ts,ΣdLR13=mbVub, (20) orΣuLR23=−mtVcb≈mtV∗ts,ΣuLR13=mtV⋆td. (21)

If the CKM matrix is generated in the down-sector the most stringent constraint stems from an enhancement of due to the off-diagonal element in the squark mass matrix. The resulting bounds on the squark and gluino mass are shown in the left plot of Fig. 1. In addition flavor-changing neutral Higgs coupling are induced according to Eq. (17) which gives an additional contribution to . Also mixing can be affected but because it is protected by a Peccei-Quinn symmetry a double Higgs penguins contributes only if also is non-zero (see right plot in Fig. 3).

In the case of CKM matrix generation in the up-sector, the most stringent constraints stem from (see right plot of Fig. 1) which receives additional contributions via a chargino box diagram involving the double mass insertion . At the same time the rare Kaon decays and receive sizable corrections (see Fig. 2) which is very interesting for NA62.

Radiative mass generation is also possible in the lepton sector. Here the anomalous magnetic moment of the muon probes the soft muon Yukawa coupling because it gets an additive contribution which depends only on the SUSY scale. If one demands that SM contribution plus the supersymmetric one is within the 2 region of the experimental measurement the smuon mass must lie between and for if its Yukawa coupling is loop-generated (see left plot of Fig. 3). If a smuon is found to be lighter, the observed muon mass cannot entirely stem from the soft SUSY-breaking sector and consequently the muon must have a nonzero Yukawa coupling in the superpotential.

## 6 Conclusions

In the MSSM self-energies can be chirally enhanced by a factor or by a factor which can compensate for the loop-suppression. This leads to order one corrections which must be taken into account to all orders in perturbation theory. This goal can be achieved by using effective vertices which include these corrections. The trilinear -terms can even entirely generate the light fermion masses and the off-diagonal CKM elements via radiative corrections. Such a model of radiative flavor violation can both solve the SUSY CP problem and is consistent with FCNC constraints for SUSY masses of the order of 1 TeV. In addition in the case of CKM generation in the down-sector and mixing receive additional contributions via Higgs penguins which and can even generate a sizable phase in mixing. In the case of CKM generation in the up sector the branching ratio of the rare Kaon decays and can be enhanced compared to the SM prediction.

###### Acknowledgements.
I thank the organizers, especially Gino Isidori, for the invitation to the ”La Thuille conference”. This work is supported by the Swiss National Foundation. I am grateful to Lars Hofer and Lorenzo Mercolli for proofreading the manuscript. The Albert Einstein Center for Fundamental Physics is supported by the “Innovations- und Kooperationsprojekt C-13 of the Schweizerische Universitätskonferenz SUK/CRUS”.

### Footnotes

1. The gluino contribution is the dominant one in the flavor-conserving case. In the presence of non-minimal sources of flavor-violation it is also usually the dominant one.
2. This equation can be directly transferred to the lepton sector by replacing fermion index for , except for the vev.
3. This also implies that the quark-squark gluino vertex is flavor-diagonal for transitions between the first two generations in the super-CKM basis.

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