Gauge Coupling Unification without Supersymmetry

We investigate the prospects to achieve unification of the gauge couplings in models without supersymmetry. We restrict our discussion to $SU(5), SO(10)$ and $E_6$ models that mimic the structure of the Standard Model as much as possible ("conservative models"). One possible reason for the non-unification of the standard model gauge couplings are threshold corrections which are necessary when the masses of the superheavy fields are not exactly degenerate. We calculate the threshold corrections in conservative models with a Grand Desert between the electroweak and the unification scale. We argue that only in conservative $E_6$ models the corrections can be sufficiently large to explain the mismatch and, at the same time, yield a long-enough proton lifetime. A second possible reason for the mismatch are particles at an intermediate scale. We therefore also study systematically the impact of additional light scalars, gauge bosons and fermions on the running of the gauge coupling. We argue that for each of these possibilities there is a viable scenario with just one intermediate scale.


Introduction
Although no experimental hints for a Grand Unified Theory (GUT) were observed so far, the general idea remains as an attractive and popular guideline for models beyond the Standard Model (SM). Among the reasons for the popularity of GUTs are that they allow us to understand the quantization of electric charge, the strengths of the SM coupling constants, why neutrinos are so light and quite generically contain all the ingredients needed to explain the baryon asymmetry [1]. Over the last decades the main focus of most researchers where supersymmetric GUTs, especially after the famous observation that the gauge couplings meet approximately at a common point if supersymmetric particles are present at a low scale, while they do not in the SM [2][3][4][5][6]. Since so far no hints of supersymmetric particles were experimentally observed, there was recently a revival of non-supersymmetric GUTs [7][8][9][10][11][12][13]. In such models gauge unification is possible, for example, if an intermediate symmetry between the GUT and the SM symmetry exists [14][15][16][17][18][19][20]. However, this is only one possibility out of many and our goal here is to discuss systematically the various possibilities to achieve unification of the gauge couplings in scenarios without supersymmetry.
After a short discussion of gauge unification in a more general context, we focus on the three most popular GUT groups: SU (5), SO(10) and E 6 . This restriction is necessary since there are, in principle, infinitely many groups that can be used in GUTs. The group SU (5) is the minimal simple group that contains the SM and was the group used in the original proposal by Georgi and Glashow [21]. An attractive feature of SO(10) models [22] is that the fundamental spinor representation not only contains the SM particles but also a right-handed neutrino. This additional neutrino in each generation is, for example, a crucial ingredient to realize the type-I seesaw [23][24][25][26]. Lastly, E 6 [27] is popular since it is the only exceptional group that can be used without major problems in a conventional GUT. The exceptional status is interesting because, in contrast, SU (5) is part of the infinite SU (N ) family, SO(10) of the infinite SO(N ) family and "describing nature by a group taken from an infinite family does raise an obvious question -why this group and not another? " [28]. Moreover, the fundamental representation of E 6 contains additional exotic fermions which makes it possible to construct E 6 models which solve the dark matter or strong CP puzzle [29,30].
Unfortunately it is not sufficient to specify the GUT group, since with any given group infinitely many different models can be constructed. One reason for this ambiguity is that there is no fundamental principle that fixes the scalar and fermion representations in GUTs. Moreover, for larger groups like SO (10) or E 6 there are dozens of different breaking chains from the GUT group down to G SM ≡ SU (3) C × SU (2) L × U (1) Y . Therefore it is necessary that we restrict ourselves to a finite subset of possible scenarios. For this reason, we define a subcategory consisting of all models that mimic the structure of the SM as much as possible. In the following, we call this subcategory "conservative models". Mimicking the structure of the SM exactly would mean for the particle content: • Only scalars that couple to the fermions.
• Only fermions that live in the fundamental or trivial representation of the gauge group.
• Only gauge bosons in the adjoint representation.
However, SU (5) and SO (10) scenarios that fulfill these criteria are phenomenologically nonviable and we are therefore forced to add additional representations. Still, we want to stay as closely as possible to the structure of the SM and therefore only add the minimal representations necessary. The fundamental representation of SU (5) is only 5-dimensional and therefore cannot contain all SM fermions of one generation. Therefore, we have to add an additional fermionic 10. Moreover, in SU (5) and SO(10) models the scalar representations that couple to the fermions cannot accomplish the breaking down to G SM . For this reason we add in both cases a scalar adjoint. These choices can also be understood through the embedding SU (5) ⊂ SO(10) ⊂ E 6 , since E 6 models always contain exotic fermions and no additional representations are necessary.
We start in Section 2 with a general discussion of the renormalization group equations (RGEs) and the hypercharge normalization. In Section 3 we then discuss unification in conservative SU (5), SO (10) and E 6 models with a "Grand Desert" between the electroweak and the GUT scale. Afterwards, we discuss the impact of additional light scalars, fermions and gauge bosons on the running of the gauge couplings. Here and in the following "light" always means light when compared to the GUT scale.

The RGEs and hypercharge normalization
The RGEs for the gauge couplings up to two-loop order are where the indices i, j denote the various subgroups at the energy scale µ and The coefficients a i and b ij depend on the particle content and can be calculated manually using the formulas in Ref. [31] or, for example, with the Python tool PyR@TE 2 [32]. While these equations together with the boundary conditions [33] ω are sufficient to calculate the running of the gauge SU (2) L and SU (3) C couplings, there is an ambiguity in the running of the hypercharge coupling. This comes about since the SM Lagrangian only depends on the product of the gauge coupling constant g times the hypercharge operator Y . Therefore, we can perform the transformation (g , Y ) → (n −1 g , nY ) for any n without changing the Lagrangian. The couplings run non-parallel and it is therefore possible to pick a specific n such that ω 3C , ω 2L and ω 1Y meet at a common point.  (5), SO(10) and E 6 GUT models. We can see here that with a non-canonical normalization of the hypercharge n Y ≈ 3/4 the SM gauge couplings do meet at a point.
The choice n = 3/5 is known as canonical normalization since it follows automatically when we embed G SM in a simple group G GU T like, for example, SU (5), SO (10) or E 6 . In such models, Y corresponds to one of the generators of the enlarged gauge group and this fixes the normalization Tr (T 2 a ) = const. since it must be the same as for all other generators of G GU T . For example, in SU (5) models we usually embed the G SM representations d c = 3, 1, 1 3 n and L = 1, 2, − 1 2 n in the fundamental 5. We therefore know that the hypercharge generator reads Y = n × diag 1 3 , 1 3 , 1 3 , − 1 2 , − 1 2 . We can then fix n by using that equivalently the SU (2) L generators must correspond to SU (5) generators. Therefore, the third generator of SU (2) L is given by T 3L = diag 0, 0, 0, 1 2 , − 1 2 . Using we can conclude |n| = 3/5. It is clear that for a different choice of G GU T or a different embedding of G SM other values for n are possible [34]. However, the value n Y = 3/5 is quite generic since it follows for all realistic models where the SM is embedded in such a way that we can view it as going through an intermediate SU (5) symmetry: G GU T → SU (5) → G SM [35]. While the canonical normalization therefore seems almost inevitable, it is important to keep in mind that a different normalization of the hypercharge could, in principle, lead to successful unification of the gauge couplings, especially when we try to go beyond the standard GUT paradigm [36]. 2 In the following sections, we consider unification in explicit SU (5), SO(10) and E 6 scenarios and therefore always use n Y = 3/5. Before we can move on we have to define a criterion that tells us when the unification of the gauge couplings is successful in a given model. Through the vacuum expectation value that breaks G GU T the additional GUT gauge bosons get a superheavy mass m X . Therefore "the gauge couplings at scales much larger than m X will be approximately equal, because the breaking of the [GUT] gauge symmetry has a negligible effect when all the energies in the process are very large compared to m X . But at energy scales much smaller than m X , the gauge couplings of the SU (3), SU (2), and U (1) subgroups are very different, each running with a β-function determined by low energy physics." [38] Therefore, naively the unification condition reads ω 1Y (M GU T ) = ω 2L (M GU T ) = ω 3C (M GU T ). However, it is well known that if we use two-loop RGEs this condition must be refined and threshold corrections can alter it significantly [39]. These arise when the masses of the various superheavy particles are not exactly degenerate. The thresholds corrections are small for each individual field, but since there are generically a large number of superheavy particles in GUTs, the individual contributions can add up to non-negligible corrections. In principle it is even possible that threshold corrections are the reason that the SM gauge couplings fail to unify in models with canonical hypercharge normalization. In the following section, we discuss the impact of threshold corrections in various GUT scenarios explicitly. Some GUT gauge bosons mediate proton decay and realistic scenarios are therefore only those where the gauge couplings successfully unify at a scale that is high enough to yield a proton lifetime in agreement with the present experimental bound τ P (p → e + π 0 ) > 1.6 × 10 34 [40]. If proton decay is mediated dominantly by the superheavy gauge bosons that are integrated out at the GUT scale this experimental bound implies ω G 45 10 2(n U −15) > 16.6 , where ω G denotes the unified gauge coupling. For example, for the typical value ω G = 45 Eq. 6 yields n U > 15.6.

Threshold Corrections
In this section we assume that there is a "Grand Desert" between the electroweak and the GUT scale, i.e. no particles at an intermediate mass scale. The threshold corrections, already mentioned above, can be expressed in terms of modified matching conditions [41] where Here, S, F , and V denote the scalars, fermions and vector bosons which are integrated out at the matching scale µ, t iS ,t iF , t iV are the generators of G i for the various representations, the hypercharge see Ref. [37]. and C G and C i are the quadratic Casimir operators for the groups G and G i . P GB is an operator that projects out the Goldstone bosons. The traces of the quadratic generators are known as Dynkin indices and can be found, for example, in Ref. [42]. To simplify the notation, we define η a j = ln( M j µ ), where j labels a given multiplet. Moreover, we define the GUT scale as the mass scale of the proton decay mediating gauge bosons. We can then define the following quantities that are independent of the unified gauge coupling ω G (µ) [43] ∆λ ij (µ) ≡ ω i (µ) − ω j (µ) = λ j (µ) − λ i (µ), (9) for i, j = 1, 2, 3, i = j. These quantities can be evaluated in two ways. Firstly, from the IR perspective by evolving the measured low-energy couplings up to some scale µ. Nonzero ∆λ ij (µ) indicate how much the gauge couplings fail to unify. Secondly, we can calculate the ∆λ ij (µ) from an UV perspective for any given GUT model. Here, the input needed is the mass spectrum of the superheavy particles. If for a specific GUT model the UV structure yields the values required from the IR input, the gauge couplings successfully unify. In the following, we work with ∆λ 12 and ∆λ 23 , but any other choice of two ∆λ ij would be equally sufficient. The quantities ∆λ ij (µ) are defined in Eq. (9) and indicate how much the gauge couplings fail to unify at a specific scale µ. The numbers above the line denote specific values for µ in GeV. The red part of the line indicates scales which imply a potentially dangerously short proton lifetime. The orange part implies a proton lifetime close to the present bounds, while the green part indicates a safe proton lifetime. Figure 2 shows ∆λ 23 (µ) over ∆λ 12 (µ) for a Grand Desert scenario between the electroweak and the GUT scale, as calculated from the IR input in Eq. (3). In the following sections we investigate if the needed values for ∆λ 12 and ∆λ 23 can be realized in specific GUT models. To approximate the threshold corrections in a given GUT model, we choose the masses of the superheavy particles randomly in a given range R around the GUT scale: M i = RM GU T . Previous studies used, for example, R ∈ [ 1 10 , 10] in Refs. [44,45] or R ∈ [ 1 10 , 2] in Ref. [13].

SU (5)
In SU (5) models the SM fermions of one generation live in the 5 ⊕ 10 representation. It follows from [42] 5 × 5 = 10 ⊕ 15 5 × 10 = 5 ⊕ 45 10 × 10 = 5 ⊕ 45 ⊕ 50   Figure 3. We can see that in SU (5) models with a Grand Desert gauge unification cannot be achieved if the masses of the superheavy particles are at most a factor 10 or 20 below the GUT scale.

SO(10)
In SO(10) models the SM fermions of one generation live in the 16-dimensional representation. The scalar representations with renormalizable Yukawa couplings to the SM fermions are contained in 16 × 16 = 10 ⊕ 120 ⊕ 126 .
In addition, a 45 is necessary to break SO(10) down to the SM. Again, for completeness, we consider the threshold effects when all these representations are present. The main difference regarding the threshold corrections, compared to SU (5) models, is that in SO(10) models there are additional gauge bosons which do not mediate proton decay. These do not necessarily have same mass as the proton decay mediating gauge bosons which define the GUT scale. By looking at Eq. (8) we can see immediately that such additional gauge bosons potentially have a large impact. This is confirmed by a scan with randomized mass of the superheavy fermions M i = RM GU T with R ∈ [ 1 10 , 2] and R ∈ [ 1 20 , 2] as shown in Figure 4. The decomposition of the scalar representations and the resulting threshold formulas are given in Appendix A.2. While the threshold corrections can be sufficiently large to explain the mismatch of the gauge couplings, the unification scale is too low to be in agreement with bounds from proton decay experiments (Eq. (6)) 3 .

E 6
In E 6 models, the SM fermions live in the fundamental 27-dimensional representation, which decomposes with respect to the maximal subgroup SO(10) × U (1) as The 16 1 contains, like in SO(10) models, all SM fermions of one generation plus a righthanded neutrino. In addition, we can see that the 27 contains a sterile neutrino 1 4 and additionally a vector-like down quark and a vector-like doublet, which are contained in the 10 −2 . Since these exotic fermions live in the same representation as the SM fermions, we automatically get 3 generations of them, too. These additional fermions yield potentially additional significant threshold corrections. The scalars are contained in The decomposition of these scalar representations and the resulting threshold formulas are given in Appendix A. 3. In E 6 , we not only have additional contributions from the three generations of exotic fermions, but also from a larger number of additional gauge bosons and scalars, compared to SO(10) models. Again, we estimate the possible threshold corrections by generating randomized spectra for the superheavy particles. The result is shown in Figure 5. We can see that suitable mass spectra of the large number of superheavy fields in E 6 GUTs can indeed explain the mismatch of the gauge couplings.
Next, we investigate whether the non-unification of the gauge couplings could be a hint for particles at intermediate scales. In principle, there can be additional light scalars, fermions and gauge bosons. However, in conservative SU (5) models the only possibility are additional light scalars, while in conservative SO(10) models there can be additional light scalars and gauge bosons, and only in conservative E 6 models we can have all three. For this reason, we discuss additional light scalars in the context of SU (5) models, additional light gauge bosons in the context of SO(10) models and additional light fermions in the context of E 6 models.
The idea to achieve gauge unification through additional light particles is, of course, not new. For example, to quote E. Ma [47]: "If split supersymmetry can be advocated as a means to have gauge-coupling unification as well as dark matter, another plausible scenario is to enlarge judiciously the particle content of the Standard Model to achieve the same goals without supersymmetry." Scenarios that realize this idea are discussed extensively in Refs. [48,49]. Our goal here is somewhat different since we are not adding particles solely to achieve gauge unification. Instead, we discuss if it is possible that the gauge couplings meet at a common point with the given particle content in conservative GUTs.

Additional Light Scalars
Each additional light (non-singlet) particle modifies the RGEs above the scale where it gets integrated out. However, not every modification of the RGEs necessarily brings the gauge couplings closer to unification. A convenient method to check if a given particles improves the running of the gauge couplings was put forward in Ref. [50]. In the following, we use this method and recite here the main points. Firstly, we define the quantities where Here a i are the one-loop coefficients as defined in Eq. 1. Necessary (one-loop) conditions for successful gauge unification are then [50] A 23 A 12 = 5 8 The left-hand side depends on the particle content, while the experimental input on the righthand side here is evaluated at M Z . Putting in the experimental values α −1 EM (M Z ) = 127.950 ± 0.017, α s (M Z ) = 0.1182 ± 0.0012, sin 2 θ w (M Z ) = 0.23129 ± 0.00050 [33] yields For Grand Desert scenarios, we find A 23 0.51. Therefore, a particle brings the gauge couplings closer to gauge unification if it lowers A 12 and increases A 23 or if it increases A 23 more than it increases A 12 . Moreover, from the second relation it follows that particles which lower A 12 increase the GUT scale. We therefore calculate the contributions to A 12 and A 23 for all representations contained in the 5 ⊕ 10 ⊕ 15 ⊕ 23 ⊕ 45 ⊕ 50 representation of SU (5). The result is shown in Table 1. We can see that additional light SU (2) L doublets with the same quantum numbers as the SM Higgs improve the running. However, the contribution is quite small and at least eight of them are needed to bring A 23 A 12 close to the experimental value. Similarly, while helpful, contributions from additional light scalars in the (1,3,6) and (3,2,1)    The impact of these representation on the running of the gauge couplings for various intermediate mass values is shown in Figures 6-8. We can see that no unification at a sufficiently high scale is possible with light (1, 3, 0) scalars, even if we take threshold corrections into account. The situation is better if there are light (3, 3, −2) scalars and the maximum GeV if M (6,3,−2) 10 12 GeV. Therefore, this scenario will be probed by the next generation of proton decay experiments [52].
Of course, it is also possible to consider scenarios in which more than one scalar representation is light. However, it is well known that each additional light scalar representation requires additional fine-tuning [53] and since scenarios with just one light representation are still viable, we do not discuss such scenarios any further here.

Additional Light Gauge Bosons
While in conservative SU (5) models the only possibility to achieve gauge unification is through additional light scalars, in SO(10) and E 6 models there can be additionally light gauge bosons, too. This is the case when there is at least one intermediate symmetry between G SM and G GU T . Since, the E 6 scalar representations that couple to fermions contain no singlet under any viable maximal subgroup other than SO(10), we discuss in the following only breaking chains that start with G GU T = SO (10). Moreover, we restrict ourselves to scenarios with exactly one intermediate symmetry. A thorough discussion of breaking chains with two intermediate symmetries can be found in Ref. [20]. 4 The breaking of SO(10) down to the SM gauge group is achieved by SM singlets in the 10 ⊕ 120 ⊕ 126 ⊕ 45 scalar representation. There are no SM singlets in the 10 and 120 and therefore all superheavy VEVs must come from the 126 or 45 representation. 10 15.9 GeV is possible for M (6,3,−2) 10 12 GeV. This scenario will therefore be probed by the next generation of proton decay experiments [52].
The singlet in the 126 breaks SO(10) down to SU (5). Since in such a scenario the gauge couplings already have to unify at the intermediate SU (5) scale there is no improvement compared to the scenarios discussed in the previous section.
There are two SM singlets in the adjoint 45 and they can break Here SU (5) denotes the flipped SU (5) embedding [55,56]. The breaking of the intermediate symmetry down to SU  [58,59]. This breaking chain was analyzed extensively in Refs. [13,60]. Hence, in the following we put our focus on the first and second breaking chain in Eq. (19). Before we can evaluate the RGE running in a scenario with intermediate symmetry, we need to specify the scalar spectrum. For this purpose we use the extended survival hypothesis, which states that "Higgses acquire the maximum mass compatible with the pattern of symmetry breaking." [61]. This a hypothesis of minimal fine tuning since only those scalar fields are light that need to be for the symmetry breaking [53]. In addition, we need to make sure that the Yukawa sector is rich enough to be able to reproduce the SM fermion observables. For this reason, at least one additional SU (2) L scalar doublet must be kept at the intermediate scale [62]. 5 The VEV that breaks SU (4) C × SU (2) L × U (1) R down to the SM gauge group lives in the (10, 1, −1) ⊂ 126 representation of the intermediate group and therefore has a mass of the order M 421 . The SM Higgs lives in the (1, 2, 1 2 ) ⊂ 10 representation. Since at least one additional doublet is needed to generate the flavour structure of the SM, we assume that the (15, 2, 1 2 ) ⊂ 126 has a mass of the order M 421 , too. With this particle spectrum, the RGE coefficients above the intermediate scale read Below M 421 the RGEs are the Standard Model ones. The matching condition for the hypercharge U (1) Y without threshold corrections reads [18] With this information at hand, we can solve the RGEs and find From similar results previous studies concluded that this breaking chain "is definitely ruled out" [18] since such a low value for M SO(10) implies a proton lifetime in conflict with experimental bounds. However, as already discussed in Section 3, results such as the one in Eq. (26) can be modified significantly by threshold corrections. These depend on the detailed mass spectrum of the superheavy particles and can be estimated by generating the masses of the various multiples randomly M i = RM j , where j ∈ {421, SO(10)}, within a given range, for example, R ∈ [ 1 10 , 2] or R ∈ [ 1 20 , 2]. The decomposition of the relevant scalar representations and the resulting threshold formulas are given in Appendix A.4. The result of such a scan with randomized mass spectra is shown in Figure 9. We find that within these ranges the proton lifetime can be at most τ max = 6.15 × 10 32 yrs.; R ∈ [1/10, 2] τ max = 7.33 × 10 33 yrs.; R ∈ [1/20, 2] .
We therefore conclude that this breaking chain is ruled out even if we take threshold corrections into account.
Again, below the intermediate scale the RGEs are the Standard Model RGEs. The matching condition for the hypercharge U (1) Y without threshold corrections for this breaking chain reads [18] Solving the RGEs yields Therefore, in the absence of threshold corrections this breaking chain is not yet challenged by the experimental bounds on proton decay. Nevertheless, for completeness we investigate  Table 7. We can see here that vector-like lepton doublets (1, 2, 3) improve the running of the gauge couplings, while vector-like quarks (3, 1, −2) make the situation worse. In addition, we can see that at the one-loop level the impact of the vector-like E 6 quarks and leptons on the RGE running cancel exactly. While the contributions of the individual fermions on the running is quite small, it can be significant since there are three generations of them. 6 To achieve gauge unification using the exotic E 6 fermions, we therefore need a scenario with a large mass splitting between the vector-like leptons and quarks. This is indeed possible since the 45 ⊂ 351 contains two SM singlets and one of them gives a mass solely to the vector-like quarks, while the other one yields a mass term for the vector-like leptons. Hence, it is possible that the exotic quarks are much heavier than the exotic leptons. This is known as the Dimopoulos-Wilzeck structure [64,65]. In the following, we assume that all vector-like quarks are sufficiently heavy to only have a negligible influence on the RGEs and focus solely on the exotic lepton doublet.
Another crucial observation is that the Yukawa couplings of the exotic fermions and those of the SM fermions have a common origin since the Yukawa sector above the E 6 scale reads It is therefore reasonable to assume that there is a splitting among the three exotic fermion generations which is of comparable size as the splitting among the SM generations, i.e. m 2L /m 3L 10 −2 , m 1L /m 3L 10 −4 . The RGE coefficients for the SM supplemented with one, two and three vector-like lepton doublets are In summary, we have demonstrated that unification of the gauge couplings is possible in conservative GUT scenarios without supersymmetry.
We have shown that one possible explanation for the observation that the SM gauge couplings do not meet at a common point are large threshold corrections. These are necessary when the superheavy fields do not have exactly degenerate masses. We calculated the magnitude of these corrections in conservative SU (5), SO(10) and E 6 models with a Grand Desert between the electroweak and the GUT scale. We found that they can be large enough only in E 6 models. The E 6 scale can be as high as M max In Section 4, we calculated the impact of additional light scalar fields on the running of the gauge couplings. We argued that in conservative SU (5) scenarios the only representations that can significantly help to achieve gauge unification are (1, 3, 0), (3, 3, −2) and (6, 3, −2). While it is possible to achieve unification through suitable mass values for each of these representations (at least if we take threshold corrections into account), only for the (6, 3, −2) this happens at a scale high-enough to be in agreement with bounds from proton decay experiments. In Section 5, we investigated scenarios with additional light gauge bosons. In conservative SO(10) GUTs the only scenarios with just one intermediate symmetry and improved running of the gauge couplings go through an SU (3) C × SU (2) L × SU (2) R × U (1) X or SU (4) × SU (2) L × U (1) R stage 7 . We calculated that the second possibility is already ruled out through proton decay experiments, even if we take threshold corrections into account. For the scenario with SU (3) C × SU (2) L × SU (2) R × U (1) X intermediate symmetry, we found that the proton lifetime can be as long as τ max 5.24 × 10 44 yrs. Finally in Section 6, we discussed the impact of additional light fermions in the context of conservative E 6 models. We argued that light vector-like E 6 leptons improve the running, while the vector-like E 6 quarks make the situation worse. Including threshold corrections plus the heaviest lepton generation around m 3L 10 14 GeV (and mass splittings m 2L /m 3L 10 −2 , m 1L /m 3L 10 −4 ), we found that the E 6 scale can be as high as A Decomposition of the Scalar Representations and Threshold Formulas in Grand Desert Scenarios Table 1: Decomposition with respect to SU (3) C × SU (2) L × U (1) Y of the scalar representations in conservative SU (5) GUTs. Goldstone bosons are labelled by ξ i , SM singlets by s i and all other fields by ϕ i . The hypercharges are given in the normalization of Ref. [42]. The numbers in the A 23 and A 12 columns indicate whether the fields can help to achieve gauge unification or not. For further explanations, see Section 4. 5 Here, P SV denotes the Pati-Salam gauge bosons in the (3, 1, −4) and W R the right-handed W ± R in the (1, 1, −6).  Table 2: Decomposition of the scalar 10 representation of SO(10) with respect to the subgroups SU (5) and SU (3) C × SU (2) L × U (1) Y . For further details, see Table 1. Here, P SV denotes the Pati-Salam gauge bosons in the (3, 1, −4), W R the right-handed W ± R in the (1, 1, −6). In addition, E i are the additional E 6 gauge bosons in the (1, 2, −3), (3, 1, 2), (1, 1, 6), (3, 1, −4) respectively. D i and L i denote the three generations of vector-like quarks and leptons. (3, 2, 1) Σ 8 Table 6: Decomposition of the scalar 27-dimensional representation of E 6 with respect to the subgroups SO(10), SU (5) and SU (3) C × SU (2) L × U (1) Y . For further details, see Table 1.