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Conformality Loss, Walking, and 4D Complex Conformal Field Theories at Weak Coupling

Four-dimensional gauge theories with matter can have regions in parameter space, often dubbed conformal windows, where they flow in the infrared to non-trivial conformal field theories. It has been conjectured that conformality can be lost because of merging of two nearby fixed points that move into the complex plane, and that a walking dynamics governed by scaling dimensions of operators defined at such complex fixed points can occur. We find controlled, parametrically weakly coupled, and ultraviolet-complete 4D gauge theories that explicitly realize this scenario. We show how the walking dynamics is controlled by the coupling of a double-trace operator that crosses marginality. The walking regime ends when the renormalization group flow of this coupling leads to a (weak) first-order phase transition with Coleman-Weinberg symmetry breaking. A light dilaton-like scalar particle appears in the spectrum, but it is not parametrically lighter than the other excitations.

Understanding the phases of gauge theories is one of the most interesting problems in high energy and condensed matter physics. Ultraviolet(UV)-free gauge theories with matter exhibit so-called conformal windows, namely regions in parameter space where they flow in the infrared (IR) to interacting conformal field theories (CFTs). A relevant example is given by four-dimensional (4D) SU (N c ) gauge theories with N f fermions in the fundamental representation of the gauge group. At fixed N c , the conformal window spans an interval N − f ≤ N f ≤ N + f . For values of N f outside this range, IR conformality is lost and it is interesting to understand the mechanism of how this happens. The upper edge of the conformal window, N + f = 11 2 N c , is more accessible because the theory can be weakly coupled there. When N f → N + f the nontrivial fixed point collides with the Gaussian one, and the latter changes its stability for N f > N + f (i.e., the theory is no longer UV free). The lower edge is instead strongly coupled and difficult to analyze. It has been proposed that conformality is lost because two nearby fixed points merge and disappear into the complex plane [1] (see also [2]). Just below the lower edge of the conformal window, a related interesting phenomenon is expected to occur [1]: walking dynamics, namely a long range of energy scales where the renormalization group (RG) flow slows down and the theory is approximately conformal invariant, after which chiral symmetry breaking and confinement take place [3] [4]. The walking behavior would occur because the RG flow passes "between" and close to the two complex fixed points and is governed by scaling dimensions of operators in the (non-unitary) CFTs living at those fixed points [5,6]. Similar dynamics has been conjectured to take place also in three-dimensional gauge theories [7].
Conformality loss and walking in 4D strongly coupled gauge theories are still conjectural. It would be interesting to confidently establish their existence, at least in weakly coupled models. In order to claim success, several requirements should be met. In particular, these theories should be (1) unitary; (2) UV complete; (3) stable [8]. In addition, they should have a parameter that makes the full RG flow arbitrarily weakly coupled (to make the perturbative expansion reliable), and another one that allows us to tune from a regime with an IR CFT to a regime with complex fixed points and walking.
In this Letter we show how the above requirements can be fulfilled in a specific (and simple) class of models. Being weakly coupled, those models will also be calculable.
When two fixed points collide, the operator O f governing the flow from one to the other becomes marginal. Let us denote by f the coupling associated to O f . Up to rescaling and shift, for small f its β-function reads , where y is a small parameter, possibly dependent on other couplings and parameters in the theory. For y > 0 there are two fixed points, at y = 0 they merge, and for y < 0 they become complex. In large N theories, O f should be a double-trace operator O 2 [9] (see also Appendix D of [5]). At leading order in the large N limit, but to all orders in f and other singletrace deformation couplings λ (such as the 't Hooft gauge coupling), the β-functions read [10,11][12] This applies also in the presence of several single-trace deformations and in more general large N limits, such as the Veneziano limit. If the theory flows to an IR fixed point, (1) implies that the double-trace operator O 2 will not mix with the single-trace operators with couplings λ i , and will have scaling dimension A simple model of this kind is given by an SU (N c ) gauge theory with N f Dirac fermions and N s scalars in the fundamental representation [13]. The Lagrangian is (before gauge fixing). The gauge coupling g is in the covariant derivative. As we will see, the theory is UV complete and free and hence technically natural: there exist renormalization schemes (e.g., minimal subtraction in dimensional regularization, MS) in which the scalar masses remain zero to all orders in perturbation theory. Fermion masses are protected by the SU (N f ) 2 chiral symmetry. We are interested in finding weakly coupled Caswell-Banks-Zaks (CBZ) fixed points [14]. This requires us to take a large N limit. We introduce 't Hooft couplings and take the Veneziano limit N c , N f , N s → ∞ with and λ, h, f fixed. Notice the different scaling limit of h and f with N c , reflecting the different single-and doubletrace nature of the corresponding operators. The perturbative β-functions, at two-loop order in the gauge coupling and one-loop order in the other couplings, are [15] These β-functions are in agreement with the general form (1). The two-loop coefficients are scheme dependent when multiple couplings are present; the result reported here is in MS. We study the theory at leading order in 1/N c and in a loopwise expansion, meaning that parametrically λ ∼ h ∼ f . In the CBZ limit, the coefficient Positions of the IR fixed points pj as we vary xs. The couplings are apart at xs = 0 and progressively merge (p1,2 at xs = xs while p3,4 at xs 0.8) as we increase xs. The region above the dashed lines corresponds to positive potentials.
multiplying the λ 2 term in β λ is made artificially small, justifying the use of two-loop order in the gauge but not the other couplings. In order to obtain a weakly coupled fixed point, we set and take 0 < 1. The numerical factor in front of has been chosen for later convenience. Note that can be made as small as of order 1/N c . We will use x s to parametrize a family of CBZ fixed points, working at leading order in 1/N c . The non-trivial zero of β λ is at Taking 0.1, λ is positive, of order and small. Plugging that value into β h , the latter has two zeros at Both values are real positive for 0 ≤ x s ≤ 2. Finally, plugging λ , h ± into β f , the latter has four zeros at with B = √ 6 − 3x s /4 and For x s < 2, B is real positive. On the other hand, A ± are real (and non-negative) in a smaller range: A + for while A − for x s ≤ 0.8403 (the numerical values are approximate). Outside those ranges, A ± are complex. We thus find four interacting fixed points p j (plotted in Fig. 1 as x s is varied), with couplings The stability properties under RG flow of the four fixed points are determined by the eigenvalues of the matrix ∂β j /∂c k where β = (β λ , β h , β f ) and c = (λ, h, f ). The three eigenvalues are We evaluate these eigenvalues at the fixed points. The first eigenvalue is the same at the four fixed points, namely ζ 1 = 25 λ . Since it is positive, this direction is always IR stable. The other two eigenvalues take the following simple form.
We conclude that, in the domain where such fixed points are real, p 1 has two IR-stable directions, p 2,3 have a stable and an unstable one, while p 4 has two unstable directions (besides ζ 1 ). Moreover, p 1 and p 2 merge at x s = x s where λ 3 = 0, and for larger values of x s they move into the complex plane. Similarly, p 3 and p 4 merge at x s 0.8 where λ 3 = 0 and then move to the complex plane. The linear combinations of operators that diagonalize dilations correspond to eigenvectors of the matrix ∂β j /∂c k . As expected, the double-trace operator O 2 = Tr φ † φ 2 does not mix at leading order in 1/N c with the two singletrace operators Tr F µν F µν and Tr At the values of x s where fixed points merge and ζ 3 vanishes, the double-trace operator becomes marginal, again as expected.
The scalar potential V =h Tr φ † φφ † φ +f Tr φ † φ 2 is positive definite at the fixed points. Indeed, one can prove that this is the case if and only iff +h > 0 and Mf +h > 0, where M = min(N c , N s ). In the large N limit, these conditions become h > 0 and min 1, All fixed points p 1,2,3,4 satisfy the positivity conditions, for all values of x s for which they are real (see Fig. 1).
We inquire whether the model defines a UV complete quantum field theory, namely, whether the theory is UV free. In order to study the RG flow around the origin in the space (λ, h, f ), it suffices to use one-loop β-functions. The analysis is similar to [16]. First, we identify special flow lines that we call "radial": where ρ(µ) is a positive function of the renormalization scale µ, while γ j are constants (defined up to positive rescalings). At leading order in , four radial flows are given by γ h /γ λ h ± /λ , γ f /γ λ f ±± /λ , in terms of the IR values in (8)- (10). Extra radial flows lie on the plane λ = 0 (i.e., have γ λ = 0) with γ h = 0 or γ f /γ h = − 1 + x s ± 1 − 10x s + x 2 s /2. Then, we introduce spherical coordinates (r, θ, ϕ) in the space of couplings, setting λ = r cos θ , h = r sin θ sin ϕ , f = r sin θ cos ϕ (18) with θ ∈ [0, π 2 ] (λ ≥ 0) and ϕ ∈ [0, 2π). Correspondingly, we define radial and angular β-functions β r and β θ , β ϕ . Since the one-loop β-functions in (5) are homogeneous in the couplings, the angular functions β θ , β ϕ are proportional to r and can be studied separately from β r . Their fixed points are precisely the radial flows discussed above.
We plot the UV angular flows, for different values of x s , in Fig. 2. The angular flow takes place on a hemisphere at fixed r, and we use (θ, ϕ) as two-dimensional polar coordinates. The gray shaded region is where β r > 0. The region above the dashed line is where the potential V is positive definite. Radial flows are represented by dots: white dots are radial flows in the λ = 0 plane; blue, yellow, green and red dots are the other ones (that, for → 0, correspond to the IR fixed points p j in Fig. 1). The red dot is the UV-attractive radial flow that makes the theory UV free. The theory is UV free for small values of x s as long as 0.1, and is UV free up to the IR merging point x s = x s for 0.085. Near the merging point, the coupling constants are expected to run slowly and enter a walking regime [1]. It was pointed out in [5] that a proper invariant description of the walking regime is provided by the CFT data of so-called complex CFTs, namely the CFTs that appear for imaginary values of the couplings. In our model the fixed points p 1 and p 2 become complex when x s > x s and define two complex CFTs C and C. Theory C contains the double-trace operator O 2 with ∆ O 2 = 4 + i|ζ 3 |, where ζ 3 = 8λ A + is purely imaginary for x s > x s . The "conjugate" operator with ∆ O 2 = 4 − i|ζ 3 | is instead in the CFT C. We notice that there exists an (unphysical) RG flow for imaginary RG time that connects C to C. This is induced by a deformation δf O 2 of C. At large N , β δf = i|ζ 3 | δf +α δf 2 (with α a real constant) to all orders in conformal perturbation theory [9]. The fixed point at δf = 0 is C while the one at δf = −i|ζ 3 |/α is C [5].
The walking regime is controlled by |ζ 3 | and the RG flow of the double-trace coupling f . When |ζ 3 | 1, in the walking regime λ ≈ λ and h ≈ h + . By redefining f → f 0 /4 − λ B, the β-function reads β f0 ≈ f 2 0 + |ζ 3 | 2 /4, with solution f 0 (µ) ≈ |ζ 3 |/2 tan |ζ 3 |/2 log µ/Λ , Λ being an integration constant. The ratio of scales where the walking regime occurs is approximately given by exp 2π/|ζ 3 | [17]. We illustrate this behavior in Fig. 3, where we plot the RG flow of f + h for various values of x s > x s , when there is no IR-stable fixed point and radiative symmetry breaking occurs in the IR through dimensional transmutation. The red line corresponds to the walking regime for x s − x s 1 (while the dashed blue line is an IR-stable flow for x s < x s ).
When the IR-stable fixed point moves in the complex plane, the RG flow continues until, at some energy scale, all N s scalars condense with color-flavor locking pattern: This pattern follows from the fact that the single-trace coupling h is positive when the coupling z ≡ f + h becomes negative [18]. We can determine v by computing the effective potential. For our purposes, it will be enough to approximate it by means of the tree-level RG improved potential, evaluated at the scale Λ IR where z = 0 (see Fig. 3) and no large logs appear. Around the vacuum expectation value (VEV) (19) the doubleand single-trace couplings combine into z. Around z ≈ 0 we have This potential has a minimum at v/Λ IR = e − 1 4 , where V eff (v) < 0. By adding a tiny UV mass term for the scalars, m 2 ∼ λ 2 Λ 2 IR /N c , we explicitly see that the phase transition is (weakly) of first order, which is the typical case occurring in radiative symmetry breaking induced by dimensional transmutation.
The scalar VEV (19) breaks the gauge group to SU (N c − N s ). Scalars acquire a tree-level squared mass of order hv 2 /N c , gluons of order λv 2 /N c , while the scalar parametrizing the radial fluctuation of v gets a oneloop squared mass schematically of order (h 2 + λ 2 )v 2 /N c [19]. The latter is proportional to the β-function of z at z = 0, which is not parametrically small in the parameter x s − x s . In the walking regime, the scale Λ IR can be made arbitrarily low. However, the gluon-to-scalar mass ratio remains constant. It has been conjectured, in the context of technicolor models, that a scalar particledenoted technidilaton-is parametrically lighter than the other resonances, and corresponds to the pseudo-Nambu-Goldstone boson of the spontaneously broken conformal symmetry [3]. In our weakly coupled description of walking, the radial fluctuation is the lightest excitation, but it cannot be made parametrically lighter than the others when x s → x s . This is in agreement with the absence of spontaneous breaking of conformal symmetry, as conformality is broken explicitly. Let us discuss the effect of higher order corrections and finite N models. Higher loop corrections to (5) correct the location of the fixed points to g = g 1 + l=2 δ l g , where g 1 = O( ) (for sufficiently small) is any of the values in (8) Since the interesting region at large N c occurs for N s N c , at finite N c we consider small N s . We choose N f (N c ) such that the theory is the most weakly coupled one and perturbative computations are expected to make sense. The qualitative analysis is the same as in the large N case. For each value of N s , there is a maximal integer value N c at and below which the IR-stable fixed point has merged to another one: conformality is lost for N c ≤ N c . For N s = 2, 3, 4, we find N c = 25, 39, 53, corresponding to x s 0.08, 0.077, 0.075. Note how the large N value x s 0.073 is quickly approached. For N c > N c , there are UV-free RG flows leading to the stable IR fixed point. For N s = 1 the single-and double-trace quartic couplings combine in the single coupling z = N c f +h /16π 2 . Independently of N f , for N c ≥ 3 we always find two real fixed points z ± and UV-free RG flows, while for N c = 2 the z ± are complex and the theory is not UV free.
Summarizing, we have shown explicit, weakly coupled, and UV complete 4D gauge theories where a conformal window ends by merging of two fixed points and a walking regime appears, after which dynamical symmetry breaking occurs. Models of this kind could also have phe-nomenological applications. In particular, UV complete gauge theories with walking regime, near the edge of their conformal window, are interesting candidates for possible composite Higgs models. In the context of natural theories, fundamental scalars should be avoided, and the dynamics should occur at strong coupling, as in QCD. Although we have shown that a dilaton-like scalar particle is not parametrically lighter than the other excitations, yet we generally expect it to be the lightest resonance and as such could be a clear collider signature for models of this kind.
We thank Hrachya Khachatryan for collaboration at the early stages of this project. We also thank Lorenzo Di Pietro and Slava Rychkov for discussions. F.B. is supported in part by the MIUR-SIR Grant No. RBSI1471GJ. M.S. acknowledges support from the Simons Collaboration on the Nonperturbative Bootstrap.