A low Fermi scale from a simple gaugino-scalar mass relation

In supersymmetric extensions of the Standard Model, the Fermi scale of electroweak symmetry breaking is determined by the pattern of supersymmetry breaking. We present an example, motivated by a higher-dimensional GUT model, where a particular mass relation between the gauginos, third-generation squarks and Higgs fields of the MSSM leads to a Fermi scale smaller than the soft mass scale. This is in agreement with the measured Higgs boson mass. The μ parameter is generated independently of supersymmetry breaking, however the μ problem becomes less acute due to the little hierarchy between the soft mass scale and the Fermi scale as we will argue. The resulting superparticle mass spectra depend on the localization of quark and lepton fields in higher dimensions. In one case, the squarks of the first two generations as well as the gauginos and higgsinos can be in the range of the LHC. Alternatively, only the higgsinos may be accessible at colliders. The lightest superparticle is the gravitino.


Introduction
The unification of gauge couplings and the prediction of viable dark matter candidates provides a strong theoretical motivation for supersymmetric extensions of the Standard Model with TeV superparticle masses [1][2][3]. So far searches for heavy superparticles at the Large Hadron Collider (LHC) have only led to lower bounds on scalar quark and gluino masses of about 1-2 TeV [4 -11]. On the other hand, the discovery of a 126 GeV Higgs boson [12][13][14] allows, without or with supersymmetry, for an extrapolation of the Standard Model up to the scale of grand unification.
The Higgs boson mass is consistent with the mass range predicted by the minimal supersymmetric standard model (MSSM). However, since the Higgs mass significantly exceeds its tree-level upper bound of 91 GeV, quantum corrections are large, which generically requires multi-TeV scalar masses. This raises the question why the Fermi scale, the expectation value of the Higgs field, H = ( √ 2G F ) −1/2 = 246 GeV, is much smaller than the scale of supersymmetry breaking, and the required fine-tuning of seemingly unrelated parameters is often considered as unnatural. Possible answers to this question invoke the anthropic principle and the string landscape, as in split supersymmetry [15,16], the focus point idea [17][18][19][20], or similar accidental cancellations between non-universal gaugino and scalar masses at the grand unification scale [21][22][23][24][25][26][27]. The naturalness problem might also be solved in a non-minimal extension of the MSSM with additional sub-TeV degrees of freedom (for instance, the NMSSM, reviewed in [28]), or through non-decoupling effects such as in [29]. 1 In this note we restrict ourselves to the MSSM, and attempt to answer a question which is intimately connected with the naturalness problem: is there a well motivated and simple set of boundary conditions for the GUT-scale soft terms which favours a 'little hierarchy' between the soft and the electroweak scale? And, what can we expect from this soft mass pattern for the upcoming second LHC run?
Our main findings can be summarized as follows. Since the µ parameter of the MSSM can be generated independently of supersymmetry breaking, it is technically natural to JHEP03(2014)075 choose it smaller than the typical soft SUSY breaking parameters, say, of the order of the electroweak scale. Usually, explaining why µ should be of the order of the soft masses is a well known challenge (the 'µ problem') in SUSY model building. Here, as we will argue, the µ problem becomes less severe once one accepts a little hierarchy. To obtain proper electroweak symmetry breaking at large tan β, the loop-corrected up-type Higgs soft mass needs to be of the same order as µ at the scale where the MSSM is matched to the Standard Model, requiring an accidental cancellation between the tree-level and radiative contributions to this parameter. We identify a simple soft mass pattern which suggests this cancellation, and which is motivated by a six-dimensional GUT model (although we expect that there are other models that can lead to the same pattern). Within this model, we obtain an estimate for the possible range of the gluino mass, which will be partly probed at LHC-14. Squarks and sleptons may also be within reach, and by construction there are higgsino-like charginos and neutralinos with electroweak-scale masses which can be discovered at a linear collider.
Note that we are not claiming to solve the fine-tuning problem: the fine-tuning in our model is as large as one would expect from a generic MSSM-type model without large contributions to the lightest Higgs mass from stop mixing, i.e. at the permille level. Our model predicts the relevant soft terms only up to factors of order one, and while the predicted pattern non-trivially allows for a little hierarchy, these unknown factors still need to be tuned in order to actually realize it. We anticipate that fully understanding the origin of the cancellations involved will require a better understanding of the complete UV theory.

Electroweak symmetry breaking with a little hierarchy
Matching the MSSM to the Standard Model. The scalar potential for the MSSM Higgs fields depends on the higgsino mass µ, which is a parameter of the superpotential, and the soft supersymmetry breaking parameters m 2 Hu , m 2 H d and Bµ, Our starting assumption is that the only scalar with an electroweak-scale mass is the lightest Higgs, while all others (in particular the remaining Higgs bosons) are much heavier. In this so-called decoupling limit the Higgs vacuum expectation value (vev) is approximately aligned with the lightest mass eigenstate. It is convenient to work with the fields H and H defined by 2 3) 2 In the usual notation for the tree-level mass eigenstates, would-be Goldstone bosons, and mixing angles (see e.g. [31]) this corresponds to

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such that the quadratic part of the potential is diagonal in the new fields: where Within the MSSM the measured mass of the lightest Higgs boson requires large radiative corrections from heavy stop squarks. Therefore we take the scale M S = (mt 1 mt 2 ) 1/2 to be much larger than the electroweak scale, of the order of several TeV. At the scale M S the MSSM is matched to the Standard Model with scalar potential where The Higgs mass parameter m 2 encodes the prediction for the electroweak scale, v 2 = −m 2 /λ, with λ being O(1).
Conditions for a little hierarchy. When keeping the electroweak scale fixed, the treelevel contribution to the lightest Higgs mass is maximized at large tan β (since in that limit | cos 2β| → 1 in eq. (2.8)), approaching its limit value of m Z = 91 GeV. The region of at least moderately large tan β 10 is therefore favoured by the large observed Higgs mass of 126 GeV, with the discrepancy accounted for by radiative corrections. The Standard Model-like Higgs field H is then predominantly H u .
By eq. (2.3), using tan 2β = 2/(cot β − tan β), large tan β implies in the generic case that m 2 Hu m 2 H d . 3 In the following we will take the µ parameter to be generated independently of supersymmetry breaking. Since µ and Bµ are both governed by a Peccei-Quinn symmetry, unless Bµ is merely accidentally small due to radiative corrections, the reason underlying relation (2.9) is that the effective symmetry breaking scale is below the soft mass scale, as will be discussed in more detail momentarily. In that case also µ is small: Relations (2.9), (2.10) and (2.12) are thus necessary to obtain a Fermi scale much smaller than the soft mass scale, assuming that tan β is at least moderately large and that µ and Bµ are connected. We now proceed to discuss the possible origins of these conditions.
Why should m 2 Hu be small? Choosing µ and Bµ small is technically natural, and this choice is radiatively stable. By contrast, radiative corrections to the Higgs soft masses are sizeable. In particular, as is well known, no symmetry protects m 2 Hu from loop corrections due to the large top Yukawa coupling. Condition (2.12) is technically unnatural, which is a manifestation of the usual fine-tuning problem in the MSSM. It requires large cancellations between the radiative contributions and the tree-level value of m 2 Hu . Let us discuss these in some more detail.
When considering models whose fundamental parameters are defined at the GUT scale, then the Higgs potential will receive large logarithmically enhanced quantum corrections, which need to be resummed using the MSSM renormalization group equations. In addition, there are finite corrections at the matching scale M S which we cannot neglect.
Turning first to the renormalization group running, the tree-level RG-improved Higgs potential at M S can be expressed as a function of the running Higgs mass parameters and of the running gauge couplings. The Higgs mass parameters at the scale M S depend on their GUT-scale values, but also on the GUT-scale soft masses of all fields with sizeable couplings to the Higgs sector. These are the third-generation scalars and the gauginos (with the gluino entering because of its large coupling to the stops and sbottoms). We find for tan β = 15 TeV . (2.14)

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Here the hatted quantities on the r.h.s. denote GUT-scale soft parameters, with A t normalized to the top Yukawa coupling. We have taken the GUT scale to be fixed at M GUT = 1.5 × 10 16 GeV, and omitted all terms with coefficients smaller than 0.05. The coefficients are largely insensitive to tan β, as long as tan β 10; for instance, for tan β = 30 the coefficients of the M 2 3 term are −{1.07; 1.11; 1.16} and all other coefficients differ from eq. (2.14) at most by 0.01. Another source of uncertainty is the experimental uncertainty in the top mass. We have checked that the uncertainty obtained from varying m t by 1σ around its central value of 173.2 GeV is of similar order, changing the coefficients at most by 0.01. The GUT-scale values for Yukawa and gauge couplings have been obtained using the two-loop RG code SOFTSUSY [32].
With the assumptions of large tan β and of negligible stop mixing at the GUT scale, i.e. negligible A t , the matching scale is in principle rather sharply determined by the lightest Higgs mass m h 0 . This is because the radiative corrections to m h 0 depend mainly on the stop masses (and on the RG-induced stop mixing parameter at the TeV scale). In practice however there is still a large uncertainty, partly because of the uncertainty in y t , but mostly because of the theory uncertainty in computing m h 0 from a given soft mass spectrum. We have chosen M S = 5 ± 1.5 TeV, which is in good accordance with the two-loop spectrum codes SOFTSUSY, SuSpect [33] and FeynHiggs [34][35][36][37] and also compatible with the threeloop analysis in [38] which is based on the H3M code [39].
The equivalent of eq. (2.14) for m 2 H d reads TeV .

(2.15)
While the coefficients in eq. (2.15) show a more pronounced tan β-dependence, the overall running of m 2 H d remains moderate in the range 10 tan β 40. In this region m H d | M S is therefore of the order of m H d , which is generically of the order M S .
In addition to the RG running of the tree-level parameters there are important finite corrections to the Higgs potential due to top-stop loops, which affect the Higgs masses (for a detailed discussion and references, see e.g. [40]). They amount to replacing m 2 Here the tadpole terms t i are computed from the minimization conditions for the full one-loop effective potential [40]. Using the one-loop results of [40], it turns out that the dominant corrections to the Higgs masses are obtained in the limit where the top Yukawa coupling is the only non-vanishing coupling, and where the stop squarks are approximately unmixed and degenerate with mass mt = M S . In the MS scheme at the renormalization

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scale M S , one finds i.e., only m 2 Hu is significantly modified by the finite corrections to the Higgs potential. In this paper we are interested in the question how electroweak symmetry breaking can occur at a scale significantly below the scale of supersymmetry breaking, i.e. how the conditions m 2 < 0 and |m 2 | M 2 S can be realized from eq. (2.11) at small |µ|. In particular, how can relation (2.12) be satisfied? An important observation is that in eq. (2.14) the scalar contributions approximately cancel for equal stop and H u masses, . This is the basis of the 'focus point' idea [17][18][19][20]. However, as the matching scale increases, the cancellation between the scalar soft mass contributions becomes less precise. The actual focussing point of the RG trajectories, where the m 0 coefficient vanishes, is only obtained for M S close to the electroweak scale.
As eq. (2.14) shows, the remaining positive contribution to m 2 Hu by scalar masses can be compensated by the negative contribution from gaugino masses. Assuming universal gaugino masses as suggested by unification, M 3 = M 2 = M 1 = M 1/2 , and taking the correction eq. (2.17) into account, one obtains for M S = 5 TeV subject to the uncertainties mentioned above. In the following we shall be interested in the case | A t | M 1/2 . A cancellation between the gaugino and the scalar contribution then occurs for a particular ratio M 1/2 /m 0 : This can also be seen from figure 1, which showsm 2 Hu (M S ) as a function of M S for different values of the ratio κ = M 1/2 /m 0 at negative, vanishing, and positive A t .
Models predicting a relation of this type therefore show some promise for obtaining a little hierarchy. In section 3 we will present an example with all the required properties: a moderate suppression for the gaugino masses and trilinear terms of roughly the correct size, and a good motivation for near-universal GUT-scale soft masses of the third generation squarks and Higgs fields. For now we still need to justify a remaining key assumption, namely that of small µ and small Bµ.
Why should µ and Bµ be small? It is well known that the higgsino mass µ plays a special role among the dimensionful parameters of the MSSM. It preserves supersymmetry, but it breaks a U(1) Peccei-Quinn (PQ) symmetry under which the Higgs bilinear is charged. The soft masses and trilinear soft terms, by contrast, break supersymmetry but preserve U(1) PQ . The Higgs soft mass mixing parameter Bµ breaks both SUSY and PQ symmetry.
For concreteness, assume that SUSY is broken by some singlet spurion X with X = F X θ 2 , and that U(1) PQ is broken supersymmetrically by some spurion Y , such that the JHEP03(2014)075

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following terms are allowed in the Lagrangian: The Kähler terms in eq. (2.20) can be absorbed in the superpotential terms by a field redefinition. The power p depends on the PQ charges of H u H d and of Y . Bare µ and Bµ terms µH u H d | θ 2 and XH u H d | θ 2 are forbidden by U(1) PQ , which also forbids the operators and Bµ is proportional to both µ and the SUSY-breaking vev, where F X /M ∼ M S is the scale of the scalar and gaugino soft mass parameters. Choosing Y such that is technically natural, since PQ breaking is a priori unrelated to SUSY breaking. The 'µ problem' is usually formulated as the need for an explanation why the SUSY-breaking soft masses are of the same order as µ. Here this is not the case: in contrast to the common SUSY model building approach, we obtain µ and the SUSY breaking soft terms from two independent scales. As soon as we allow for a little hierarchy, the µ problem becomes less severe as we will argue momentarily. Indeed the most interesting parameter choice has µ maximally separated from M S , to the extent that is allowed by experimental data. With the conditions (2.12) and (2.23), electroweak symmetry can be broken with all three terms in eq. (2.11) being of the order of the electroweak scale. The required finetuning is no worse than the fine-tuning needed in the more common case where µ is of the order of the soft breaking terms, and cancelled against a similarly largem 2 Hu . In our case we are instead cancelling large radiative contributions to them 2 Hu parameter against each other.
Remarkably, if the conditions (2.23) are satisfied withm 2 Hu sufficiently small, then the electroweak scale is parametrically given not by M S but by µ. This is most easily seen by settingm 2 Hu = 0, m H d = ηM S , Bµ = ζ|µ|M S at the scale M S , with η and ζ of the order one (or at least small compared to M S /µ -in the next section we will consider a model where ζ ∼ 1/κ, with κ ≈ 0.25 as in eq. (2.19)). One then obtains

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For ζ 2 > η 2 the Higgs mass matrix eq. (2.24) has a negative eigenvalue even though the diagonal entries are both positive. In fact, for ζ 2 η 2 the electroweak scale is given by a seesaw-type formula, A very similar pattern has previously been investigated in the context of gauge-mediated supersymmetry breaking, where the hierarchy between m H d (or equivalently M S ) and |µ| is not due to a PQ symmetry but due to a loop factor [41,42]. Let us emphasize that a sufficiently large value of Bµ, and therefore ζ, is crucial for electroweak symmetry breaking, which takes place irrespective of the sign of m 2 Hu . As already emphasized we have no symmetry reason form 2 Hu = 0. In the more general case m 2 Hu M 2 S , electroweak symmetry breaking imposes a lower bound on |µ| 2 , Hu . (2.27) Note that there is also a phenomenological lower bound on |µ|: since tan β is parametrically given by m 2 H d /Bµ ∼ η 2 M S /(ζ|µ|), and should not exceed a value ≈ 60 in order to avoid non-perturbative Yukawa couplings, the hierarchy between µ and M S cannot be too large. Thus, for fixed M S , µ is bounded from below. The most relevant bound for the model of the next section will however turn out to be the direct experimental lower limit |µ| 100 GeV from chargino searches at LEP.
At this point let us briefly return to the µ problem. If we setm 2 Hu = 0 and ignore the associated fine-tuning for a moment, it is clear from the Higgs mass matrix eq. (2.24) and from eq. (2.26) that the soft mass scale may be decoupled from the scale of electroweak symmetry breaking (which is essentially given by µ). In a hypothetical universe with very light down-type quarks, there would also be no restriction on the ratio M S /µ ∼ tan β, so M S could in principle be very large, and the µ problem would be circumvented. Realistically, however, this line of reasoning is invalidated to some extent by the experimentally known bottom and top quark masses. The known value of m b leads to an upper bound on tan β, while the known value of m t implies that the top Yukawa coupling is large, and that a relation such asm 2 Hu = 0 will therefore be spoiled by large loop corrections. These two arguments point towards a soft mass scale M S which is not too far above the electroweak scale; the 126 GeV Higgs mass further fixes the 'little hierarchy' to amount to 1-2 decades. In summary, the µ problem is still present, but somewhat alleviated when allowing for a little hierarchy between M S and the Fermi scale (as seems to be forced upon us by LHC data).

Supersymmetry breaking in higher-dimensional GUTs
We shall now present an explicit example which realizes the conditions for a seesaw-type pattern of electroweak symmetry breaking discussed in the previous section. Consider a six-dimensional (6d) GUT model, with the third quark-lepton generation and the Higgs fields located in the bulk and the first two families localized at 4d branes or orbifold fixed

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points. Such a model has been derived as an intermediate step [43] in a compactification of the heterotic string to the supersymmetric standard model in four dimensions [44,45]. Supersymmetry is supposed to be broken by the F -term of a chiral superfield located at some fixed point.
In the following we shall restrict our discussion to the case of strong coupling at the cutoff scale. The couplings of the supersymmetry breaking brane field to Higgs, matter and gauge fields can then be estimated by means of 'naive dimensional analysis' (NDA) following [51]. The localization of the fields fixes the structure of the Lagrangian where y i are the positions of the 4d branes, and W α , Φ and φ denote bulk gauge fields, bulk chiral fields, and brane chiral fields, respectively. Matching 6d and 4d theories at the compactification scale, the gauge couplings and Planck masses are related by where V 2 is the volume of the two compact dimensions. 5 In order to define the theory one has to introduce a UV cutoff Λ. If loop corrections at the scale Λ are suppressed by , the Lagrangian eq. (3.1) can be expressed in terms of dimensionless fields W α /Λ 3/2 , Φ/Λ and φ/Λ, The fields W α , Φ and φ are assumed to have canonical kinetic terms in 6d and 4d, respectively, and the rescaled fields W α , Φ and φ have canonical dimensions in 4d. According to NDA the Lagrangian (3.1) now takes the form where all couplings are O(1) and D = 2 D π D/2 Γ(D/2) is a geometrical loop factor, with Strong coupling at the cutoff scale Λ corresponds to 1. 5 In the considered GUT model one has V2 = 2π 2 R5R6, where R5 and R6 are the radii of the orbifold.
The model has a Wilson line in the direction of R6 which breaks the GUT symmetry. With R5 ≥ R6, the mass of the lowest lying Kaluza-Klein state is 1/(2R5). Identifying this mass with the GUT scale MGUT 1 × 10 16 GeV, one obtains V −1/2 2 5 × 10 15 GeV (see [46]).

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In our 6d GUT model, the couplings of the SUSY breaking brane field X to the bulk fields are given by 6 where H u , H d , W α , Q 3 , U 3 , D 3 , L 3 and E 3 denote Higgs fields, gauge fields and third generation quark and lepton fields, respectively. H u is part of the 6d gauge multiplet, Q 3 and U 3 belong to the same hypermultiplet, and the cubic term Q 3 H u U 3 is part of the 6d gauge interactions. 7 From the gauge kinetic term one reads off the gauge coupling The mass parameter µ is an additional free parameter which can be much smaller than the cutoff scale Λ due to an accidental PQ symmetry as discussed in section 2. From eqs. (3.3) and (3.7) one obtains the Lagrangian for canonically normalized bulk fields, (3.9) Finally, the replacement Φ(x, y) → V −1/2 2 Φ(x) yields the couplings of canonically normalized zero modes, (3.10) In eq. (3.7) we have assumed a universal coupling of the SUSY breaking field to bulk fields. The focus point cancellation discussed in section 2 requires approximately equal mass terms of H u , Q 3 and U 3 at a level of about 5%. In the considered model the equality of mass terms is guaranteed by a symmetry only for U 3 and E 3 , which belong to the same JHEP03(2014)075 SU(6) hypermultiplet in six dimensions. For all other fields a dynamical reason is needed. The couplings of brane and bulk fields depend on the profile that the bulk fields aquire in connection with the stabilization of the compact dimensions. These profiles depend on the presence of localized Fayet-Iliopoulos (FI) terms [47]. Such FI-terms are also crucial to reconcile the tree-level gauge-top unification of the model, y t = g 4 (cf. eq. (3.10)), with the large values of tan β considered in section 2 [46]. It is conceivable that the FI terms present in the model [43] lead to approximately equal mass terms, but a detailed study of the compactification dynamics is beyond the scope of this paper.
Replacing now the brane field X by its SUSY breaking vacuum expectation value F X , we obtain from eq. (3.10) the wanted mass parameters of the zero modes for gaugino fields, Higgs and higgsino fields and third generation scalar quark-lepton fields, where y t = g 4 , and A further important parameter is the higgsino mass µ. If µ is generated independently of supersymmetry breaking, generically one would expect µ ∼ M S / tan β, as discussed in section 2. In the model of section 3, since Bµ is enhanced by a factor 1/κ, we estimate µ ∼ κM S / tan β, which implies that for M S = 5 ± 1.5 TeV and moderately large tan β, the µ parameter should actually be close to the electroweak scale (|µ| 100 GeV being excluded by chargino searches). A soft upper bound can be estimated by conservatively setting tan β = 5, κ = 1/3 and M S = 6.5 TeV, which yields µ 450 GeV.
In summary, the mass spectrum we predict is characterized by heavy third-generation squarks and sleptons, heavy extra Higgs bosons, gluino masses starting from about 2 TeV, higgsino-like charginos and neutralinos with electroweak-scale masses, and squarks and sleptons which are either extremely heavy (B) or generated by gaugino mediation (A). In the latter case, standard SUSY searches for jets and missing energy, as well as searches for direct slepton production, will be promising channels at LHC-14. In any case, the light higgsinos can be searched for and measured at a linear collider [54][55][56]. Table 1 shows a number of superpartner mass spectra. The first three columns correspond to three different values of M S in scenario (A). For a relatively low matching scale M S = 3.5 TeV, gluinos and squarks should be found during the next LHC run, and sleptons should also be easy to see as the slepton masses are already at the border of the present exclusion bounds [57,58] figure 1. Note that the relation between M S and M 3 for fixed κ is only approximately linear. As before, tan β = 15, M GUT = 1.5 × 10 16 GeV. We have indicated the range of M S preferred by the Higgs mass (which we took to be 5 ± 1.5 TeV). We have also indicated the predictions for M 3 as a function of M S , for the two cases A t = ±M 1/2 (black strips), and the minimal and maximal M 3 which can be obtained (dashed horizontal lines), when restricting |m Hu | to be of the order of the electroweak scale as in figure 1. One finds 1.8 TeV M 3 4.9 TeV.
challenging, but squarks and gluinos may still be accessible at high integrated luminosities. The third case of M S = 6.5 TeV places squarks and gluinos out of LHC reach.
The last column of table 1 shows a spectrum for the case that the first-and secondgeneration scalar masses are non-vanishing at the GUT scale and given by M soft = 30 TeV (scenario (B) above). In this case the overall soft mass scale also for the third generation and the gluinos is higher. The reason is that we are keeping M S = 5 TeV fixed, and the first two squark generations significantly decrease the stop masses when running down from the GUT scale through two-loop effects, up to a point where the stop mixing contribution to the lightest Higgs mass can become very significant [54,[59][60][61]. This case is not covered by our semi-analytic discussion in section 2, which does not account for possible large contributions to the running from the first two generations, but can nevertheless be dealt with numerically. As is evident from table 1, all states are too heavy to be seen at colliders in the foreseeable future, with the possible exception of the higgsinos.
Finally, the matching scale M S also determines the gravitino mass. From eq. (3.19) one obtains 40 GeV m 3/2 80 GeV . (4.2) Here we have chosen the 6d Planck mass as the cutoff scale, and we have varied m 0 between 4 TeV and 8 TeV according to table 1. The starting point of our discussion has been the compatibility of the measured Higgs boson mass, and the associated large matching scale M S , with a Fermi scale significantly Table 1. Example mass spectra computed with SOFTSUSY 3.3.10 [32] for different matching scales. The parameters are tan β = 15, A t,b = 0, M 1/2 = (1, 1.6, 2.25, 2.45) TeV, m 0 = (4.35, 6.0, 7.6, 7.7) TeV for the third generation and the Higgs fields. For the three columns on the left, the GUT-scale scalar soft masses of the first two generations vanish, whereas for the rightmost column they arem 0 = 30 TeV. All masses in the table are in units of GeV. smaller than M S . We have shown that for a small higgsino mass µ, not controlled by supersymmetry breaking, and universal Higgs and stop masses at the GUT scale, a small Fermi scale arises for suitable relations between gaugino and scalar masses. It is interesting that a simple example can be obtained within the context of a higher-dimensional GUT model. The matching scale, together with the related gaugino-scalar mass ratio, and the value of tan β determine the superparticle mass spectrum. If the matching scale turns out to be lower than about 5 TeV, this scenario will be probed by the upcoming next LHC run, with searches for gluinos, squarks and also sleptons being promising channels. Moreover, our setup favours light higgsinos, which can be searched for at a linear collider. The lightest superparticle is the gravitino. [5] ATLAS collaboration, Search for strongly produced supersymmetric particles in decays with two leptons at √ s = 8 TeV, ATLAS-CONF-2013-089 (2013).