Hadron Spectroscopy and Structure from Ads/CFT

SLAC-PUB-12125 September 2005

Hadron Spectroscopy and Structure from AdS/CFT

Stanley J. Brodsky1 Stanford Linear Accelerator Center Stanford University Stanford, California 94309

Abstract. The AdS/CFT correspondence between conformal field theory and string states in an extended space-time has provided new insights into not only hadron spectra, but also their light-front wavefunctions. We show that there is an exact correspondence between the fifth-dimensional coordinate of anti-de Sitter space z and a specific impact variable ζ which measures the separation of the constituents within the hadron in ordinary space-time. This connection allows one to predict the form of the light-front wavefunctions of mesons and baryons, the fundamental entities which encode hadron properties and scattering amplitudes. A new relativistic Schrödingerlight-front equation is found which reproduces the results obtained using the fifth-dimensional theory. Since they are complete and orthonormal, the AdS/CFT model wavefunctions can be used as an initial ansatz for a variational treatment or as a basis for the diagonalization of the light-front QCD Hamiltonian. A number of applications of light-front wavefunctions are also discussed.

PACS. 12.38.Aw,12.38.-t,11.25.Hf,11.90.+t,11.55.Jy

d 1 Hadron Wavefunctions in QCD i dτ generates light-front time translations, and the eigen- QCD spectrum of the Lorentz scalar HLF gives the mass spec- One of the most important tools in atomic physics is the trum of the color-singlet hadron states in QCD together Schrödingerwavefunction; it provides a quantum mechan- with their respective light-front wavefunctions. For exam- ical description of the position and spin coordinates of QCD 2 ple, the proton state satisfies: HLF | ψpi = Mp | ψpi. nonrelativistic bound states at a given time t. Clearly, it Remarkably, the light-front wavefunctions are frame- is an important goal in hadron and nuclear physics to de- independent;thus knowing the LFWFs of a hadron in its termine the wavefunctions of hadrons in terms of their rest frame determines the wavefunctions in all other frames. fundamental quark and gluon constituents. Guy de Téramondand I have recently shown how one Given thelight-front wavefunctionsψn/H (xi, k⊥i, λi),one can use AdS/CFT to not only obtain an accurate descrip- can compute a large range of hadron observables. For ex- tion of the hadron spectrum for light quarks, but also ample, the valence and sea quark and gluon distributions how to obtain a remarkably simple but realistic model of which are measured in deep inelastic lepton scattering are the valence wavefunctions of mesons, baryons, and glue- defined from the squares of the LFWFS summed over all balls. As I review below, the amplitude Φ(z) describing Fock states n. Form factors, exclusive weak transition am- the hadronic state in the fifth dimension of Anti-de Sit- plitudes [4] such as B → `νπ. and the generalized parton ter space AdS5 can be precisely mapped to the light-front distributions [5]measured in deeply virtual Compton scat- wavefunctions ψn/h of hadrons in physical space-time [1], tering are (assuming the“handbag” approximation) over- thus providing a relativistic description of hadrons in QCD laps of the initial and final LFWFS with n = n0 and at the amplitude level. The light-front wavefunctions are n = n0 + 2. The gauge-invariant distribution amplitude relativistic and frame-independent generalizations of the φH (xi,Q)defined from the integral over the transverse mo- familiar Schrödingerwavefunctions of atomic physics, but 2 2 menta k⊥i ≤ Q of the valence (smallest n) Fock state they are determined at fixed light-cone time τ = t+z/c— provides a fundamental measure of the hadron at the am- the “front form” advocated by Dirac—rather than at fixed plitude level [6,7]; they are the nonperturbative input to ordinary time t. the factorized form of hard exclusive amplitudes and ex- Formally, the light-front expansion is constructed by clusive heavy hadron decays in perturbative QCD. The quantizing QCD at fixed light-cone time [2] τ = t+z/c and resulting distributions obey the DGLAP and ERBL evo- QCD forming the invariant light-front Hamiltonian: HLF = lution equations as a function of the maximal invariant + − 2 ± 0 z P P − P ⊥ where P = P ± P . [3] The momen- mass, thus providing a physical factorization scheme [8]. + tum generators P and P ⊥ are kinematical; i.e., they In each case, the derived quantities satisfy the appropri- are independent of the interactions. The generator P − = ate operator product expansions, sum rules, and evolution

Submitted to European Physical Journal

Work supported in part by Department of Energy contract DE-AC02-76SF00515 2 Stanley J. Brodsky: Hadron Spectroscopy and Structure from AdS/CFT equations. However, at large x where the struck quark is far-off shell, DGLAP evolution is quenched [9], so that the fall-off of the DIS cross sections in Q2 satisfies inclusive- exclusive duality at fixed W 2. – The physics of higher Fock states such as the |uudqQi e fluctuation of the proton is nontrivial, leading to asym- e– metric s(x) and s(x) distributions, u(x) 6= d(x), and in- current trinsic heavy quarks cc and bb which have their support quark jet at high momentum [10]. Color adds an extra element of a * complexity: for example there are five-different color singlet combinations of six 3C quark representations which appear in the deuteron’s valence wavefunction, leading to quark the hidden color phenomena [11]. final state interaction An important example of the utility of light-front wavefunctions in hadron physics is the computation of polar- S ization effects such as the single-spin azimuthal asym- spectator metries in semi-inclusive deep inelastic scattering, rep- system resenting the correlation of the spin of the proton tar- proton 11-2001 get and the virtual photon to hadron production plane: 8624A06 Sp · q × pH . Such asymmetries are time-reversal odd, but they can arise in QCD through phase differences in different spin amplitudes. In fact, final-state interactions from gluon exchange between the outgoing quarks and the target spectator system lead to single-spin asymmetries Fig. 1. A final-state interaction from gluon exchange in in semi-inclusive deep inelastic lepton-proton scattering deep inelastic lepton scattering. The difference of the QCD which are not power-law suppressed at large photon vir- Coulomb-like phases in different orbital states of the proton 2 tuality Q at fixed xbj [12] (see: Fig. 1). In contrast to produces a single proton spin asymmetry. the SSAs arising from transversity and the Collins fragmentation function, the fragmentation of the quark into hadrons is not necessary; one predicts a correlation with cluding its sign has been given by Burkardt [13]. As shown the production plane of the quark jet itself. Physically, by Gardner and myself [20], one can also use the Sivers the final-state interaction phase arises as the infrared- effect to study the orbital angular momentum of gluons finite difference of QCD Coulomb phases for hadron wave by tagging a gluon jet in semi-inclusive DIS. In this case, functions with differing orbital angular momentum. The the final-state interactions are enhanced by the large color same proton matrix element which determines the spin- charge of the gluons. orbit correlation S · L also produces the anomalous mag- The final-state interaction effects can also be identified netic moment of the proton, the Pauli form factor, and with the gauge link which is present in the gauge-invariant the generalized parton distribution E which is measured definition of parton distributions [21]. Even when the light- in deeply virtual Compton scattering. Thus the contri- cone gauge is chosen, a transverse gauge link is required. bution of each quark current to the SSA is proportional Thus in any gauge the parton amplitudes need to be augmented by an additional eikonal factor incorporating the to the contribution κq/p of that quark to the proton tar- P final-state interaction and its phase [22,23]. The net effect get’s anomalous magnetic moment κp = q eqκq/p. [12, 13]. The HERMES collaboration has recently measured is that it is possible to define transverse momentum de- the SSA in pion electroproduction using transverse tar- pendent parton distribution functions which contain the get polarization [14]. The Sivers and Collins effects can be effect of the QCD final-state interactions. separated using planar correlations; both processes are ob- A related analysis also predicts that the initial-state served to contribute, with values not in disagreement with interactions from gluon exchange between the incoming theory expectations [14,15]. The deeply virtual Comp- quark and the target spectator system lead to leading- twist single-spin asymmetries in the Drell-Yan process ton amplitudes can be Fourier transformed to b⊥ and l − + + − σ = x P /2 space providing new insights into QCD dis- H1H2 → ` ` X [24,25]. Initial-state interactions also tributions [16–19]. The distributions in the LF direction lead to a cos 2φ planar correlation in unpolarized Drell- σ typically display diffraction patterns arising from the Yan reactions [26]. interference of the initial and final state LFWFs [18]. The final-state interaction mechanism provides an appealing physical explanation within QCD of single-spin asymme- 2 Diffractive Deep Inelastic Scattering tries. Physically, the final-state interaction phase arises as the infrared-finite difference of QCD Coulomb phases A remarkable feature of deep inelastic lepton-proton scat- for hadron wave functions with differing orbital angular tering at HERA is that approximately 10% events are momentum. An elegant discussion of the Sivers effect in- diffractive [27,28]: the target proton remains intact, and Stanley J. Brodsky: Hadron Spectroscopy and Structure from AdS/CFT 3 there is a large rapidity gap between the proton and the made possible in any gauge by the soft rescattering. The other hadrons in the final state. These diffractive deep in- resulting diffractive contributions leave the target intact elastic scattering (DDIS) events can be understood most and do not resolve its quark structure; thus there are con- simply from the perspective of the color-dipole model: the tributions to the DIS structure functions which cannot be qq Fock state of the high-energy virtual photon diffrac- interpreted as parton probabilities [30]; the leading-twist tively dissociates into a diffractive dijet system. The ex- contribution to DIS from rescattering of a quark in the change of multiple gluons between the color dipole of the target is a coherent effect which is not included in the qq and the quarks of the target proton neutralizes the light-front wave functions computed in isolation. One can color separation and leads to the diffractive final state. augment the light-front wave functions with a gauge link The same multiple gluon exchange also controls diffrac- corresponding to an external field created by the virtual tive vector meson electroproduction at large photon vir- photon qq pair current [23,21]. Such a gauge link is pro- tuality [29]. This observation presents a paradox: if one cess dependent [24], so the resulting augmented LFWFs chooses the conventional parton model frame where the are not universal [23,30,31]. We also note that the shad- photon light-front momentum is negative q+ = q0 + qz < owing of nuclear structure functions is due to the destruc- 0, the virtual photon interacts with a quark constituent tive interference between multi-nucleon amplitudes involv- + + with light-cone momentum fraction x = k /p = xbj. ing diffractive DIS and on-shell intermediate states with a Furthermore, the gauge link associated with the struck complex phase. In contrast, the wave function of a stable quark (the Wilson line) becomes unity in light-cone gauge target is strictly real since it does not have on-energy-shell A+ = 0. Thus the struck “current” quark apparently ex- intermediate state configurations. The physics of rescat- periences no final-state interactions. Since the light-front tering and shadowing is thus not included in the nuclear wavefunctions ψn(xi, k⊥i) of a stable hadron are real, it light-front wave functions, and a probabilistic interpreta- appears impossible to generate the required imaginary tion of the nuclear DIS cross section is precluded. phase associated with pomeron exchange, let alone large Rikard Enberg, Paul Hoyer, Gunnar Ingelman and I [32] rapidity gaps. have shown that the quark structure function of the effec- This paradox was resolved by Paul Hoyer, Nils Mar- tive hard pomeron has the same form as the quark contri- chal, Stephane Peigne, Francesco Sannino and myself [30]. bution of the gluon structure function. The hard pomeron Consider the case where the virtual photon interacts with is not an intrinsic part of the proton; rather it must be con- a strange quark—the ss pair is assumed to be produced sidered as a dynamical effect of the lepton-proton interac- in the target by gluon splitting. In the case of Feynman tion. Our QCD-based picture also applies to diffraction in gauge, the struck s quark continues to interact in the hadron-initiated processes. The rescattering is different in final state via gluon exchange as described by the Wil- virtual photon- and hadron-induced processes due to the son line. The final-state interactions occur at a light-cone different color environment, which accounts for the ob- time ∆τ ' 1/ν shortly after the virtual photon inter- served non-universality of diffractive parton distributions. acts with the struck quark. When one integrates over the This framework also provides a theoretical basis for the nearly-on-shell intermediate state, the amplitude acquires phenomenologically successful Soft Color Interaction(SCI) an imaginary part. Thus the rescattering of the quark model [33]which includes rescattering effects and thus gen- produces a separated color-singlet ss and an imaginary erates a variety of final states with rapidity gaps. phase. In the case of the light-cone gauge A+ = η · A = 0, The phase structure of hadron matrix elements is thus one must also consider the final-state interactions of the an essential feature of hadron dynamics. Although the (unstruck) s quark. The gluon propagator in light-cone LFWFs are real for a stable hadron, they acquire phases µν 2 µν µ ν µ ν gauge dLC (k) = (i/k + i²)[−g + (η k + k η /η · k)] from initial state and final state interactions. In addition, is singular at k+ = η · k = 0. The momentum of the the violation of CP invariance leads to a specific phase exchanged gluon k+ is of O(1/ν); thus rescattering con- structure of the LFWFs. Dae Sung Hwang, Susan Gard- tributes at leading twist even in light-cone gauge. The net ner and I [34] have shown that this in turn leads to the result is gauge invariant and is identical to the color dipole electric dipole moment of the hadron and a general rela- model calculation. The calculation of the rescattering ef- tion between the edm and anomalous magnetic moment fects on DIS in Feynman and light-cone gauge through Fock state by Fock state. three loops is given in detail for an Abelian model in the There are also leading-twist diffractive contributions references [30]. The result shows that the rescattering cor- γ∗N → (qq)N arising from Reggeon exchanges in the rections reduce the magnitude of the DIS cross section in 1 1 t-channel [35]. For example, isospin–non-singlet C = + analogy to nuclear shadowing. Reggeons contribute to the difference of proton and neu- A new understanding of the role of final-state interac- tron structure functions, giving the characteristic Kuti- 1−αR(0) 0.5 tions in deep inelastic scattering has thus emerged. The Weisskopf F2p − F2n ∼ x ∼ x behavior at small multiple scattering of the struck parton via instantaneous x. The x dependence of the structure functions reflects interactions in the target generates dominantly imaginary the Regge behavior ναR(0) of the virtual Compton ampli- diffractive amplitudes, giving rise to an effective “hard tude at fixed Q2 and t = 0. The phase of the diffractive pomeron” exchange. The presence of a rapidity gap be- amplitude is determined by analyticity and crossing to be tween the target and diffractive system requires that the proportional to −1 + i for αR = 0.5, which together with target remnant emerges in a color-singlet state; this is the phase from the Glauber cut, leads to constructive in- 4 Stanley J. Brodsky: Hadron Spectroscopy and Structure from AdS/CFT terference of the diffractive and nondiffractive multi-step massless quarks and without particle creation or absorp- nuclear amplitudes. Furthermore, because of its x depen- tion, then the resulting β function is zero, the coupling dence, the nuclear structure function is enhanced precisely is constant, and the approximate theory is scale and con- in the domain 0.1 < x < 0.2 where antishadowing is em- formal invariant. Conformal symmetry is of course bro- pirically observed. The strength of the Reggeon ampli- ken in physical QCD; nevertheless, one can use confor- tudes is fixed by the fits to the nucleon structure func- mal symmetry as a template, systematically correcting for tions, so there is little model dependence. Ivan Schmidt, its nonzero β function as well as higher-twist effects. For Jian-Jun Yang, and I [36] have applied this analysis to example, “commensurate scale relations” [45]which relate the shadowing and antishadowing of all of the electroweak QCD observables to each other, such as the generalized structure functions. Quarks of different flavors will couple Crewther relation [46], have no renormalization scale or to different Reggeons; this leads to the remarkable pre- scheme ambiguity and retain a convergent perturbative diction that nuclear antishadowing is not universal; it de- structure which reflects the underlying conformal symme- pends on the quantum numbers of the struck quark. This try of the classical theory. In general, the scale is set such picture leads to substantially different antishadowing for that one has the correct analytic behavior at the heavy charged and neutral current reactions, thus affecting the particle thresholds [47]. extraction of the weak-mixing angle θW . We find that In a confining theory where gluons have an effective part of the anomalous NuTeV result [37] for θW could mass, all vacuum polarization corrections to the gluon self- be due to the non-universality of nuclear antishadowing energy decouple at long wavelength. Theoretical [48] and for charged and neutral currents. Detailed measurements phenomenological [49] evidence is in fact accumulating of the nuclear dependence of individual quark structure that QCD couplings based on physical observables such functions are thus needed to establish the distinctive phe- as τ decay [50] become constant at small virtuality;i.e., nomenology of shadowing and antishadowing and to make effective charges develop an infrared fixed point in con- the NuTeV results definitive. Antishadowing can also de- tradiction to the usual assumption of singular growth in pend on the target and beam polarization. the infrared. The near-constant behavior of effective couplings also suggests that QCD can be approximated as a conformal theory even at relatively small momentum 3 The Conformal Approximation to QCD transfer. The importance of using an analytic effective charge [51] such as the pinch scheme [52,53] for unifying the electroweak and strong couplings and forces is also One of the most interesting recent developments in hadron important [54]. Thus conformal symmetry is a useful first physics has been the use of Anti-de Sitter space holo- approximant even for physical QCD. graphic methods in order to obtain a first approximation to nonperturbative QCD. The essential principle underlying the AdS/CFT approach to conformal gauge theories 4 Hadronic Spectra in AdS/QCD is the isomorphism of the group of Poincare’ and conformal transformations SO(2, 4) to the group of isometries Guy de Téramondand I [1,40] have recently shown how of Anti-de Sitter space. The AdS metric is a holographic model based on truncated AdS space can be used to obtain the hadronic spectrum of light quark R2 qq, qqq and gg bound states. Specific hadrons are identi- ds2 = (ηµν dx dxµ − dz2), z2 µ fied by the correspondence of the amplitude in the fifth dimension with the twist-dimension of the interpolating which is invariant under scale changes of the coordinate operator for the hadron’s valence Fock state, including in the fifth dimension z → λz and dxµ → λdxµ. Thus its orbital angular momentum excitations. An interesting one can match scale transformations of the theory in 3+1 aspect of our approach is to show that the mass param- physical space-time to scale transformations in the fifth eter µR which appears in the string theory in the fifth dimension z. The amplitude φ(z) represents the extension dimension is quantized, and that it appears as a Casimir of the hadron into the fifth dimension. The behavior of constant governing the orbital angular momentum of the ∆ φ(z) → z at z → 0 must match the twist-dimension hadronic constituents analogous to L(L + 1) in the radial 2 of the hadron at short distances x → 0. As shown by Schrödingerequation. Polchinski and Strassler [38], one can simulate confine- As an example, the set of three-quark baryons with 1 ment by imposing the condition φ(z = z0 = ). This ΛQCD spin 1/2 and higher is described in AdS/CFT by the Dirac approach, has been successful in reproducing general prop- equation in the fifth dimension [1] erties of scattering processes of QCD bound states [38, £ 2 2 2 2 2 ¤ 39], the low-lying hadron spectra [40,41], hadron couplings z ∂z − 3z ∂z + z M − L± + 4 ψ±(z) = 0. (1) and chiral symmetry breaking [41,42], quark potentials in The constants L+ = L + 1, L− = L + 2 in this equation confining backgrounds [43] and pomeron physics [44]. are Casimir constants which are determined to match the It was originally believed that the AdS/CFT mathe- twist dimension of the solutions with arbitrary relative matical tool could only be applicable to strictly confor- orbital angular momentum. The solution is mal theories such as N = 4 supersymmetry. However, if −iP ·x one considers a semi-classical approximation to QCD with Ψ(x, z) = Ce [ψ(z)+ u+(P ) + ψ(z)− u−(P )] , (2) Stanley J. Brodsky: Hadron Spectroscopy and Structure from AdS/CFT 5

N (2600) 8 (a) (b) ∆ (2420) N (2250) )

2 ∆ 6 N (2190) (1950) ∆ N (1700) (1920) ∆ (1910)

(GeV N (1675) N (1650) ∆ (1905) 4 N (1535) N (2220) N (1520) ∆ ∆ (1232) (1930) 2 N (1720) 56 N (1680) ∆ (1700) 70 ∆ (1620) N (939) 0 0 2 4 6 0 2 4 6 1-2006 8694A14 L L

Fig. 2. Predictions for the light baryon orbital spectrum for ΛQCD = 0.25 GeV. The 56 trajectory corresponds to L even P = + states, and the 70 to L odd P = − states.

2 2 with ψ+(z) = z J1+L(zM) and ψ−(z) = z J2+L(zM). ativistic description of hadrons in QCD at the amplitude The physical string solutions have plane waves and chiral level. We derived this correspondence by noticing that the spinors u(P )± along the Poincar´ecoordinates and hadronic mapping of z → ζ analytically transforms the expression µ 2 invariant mass states given by PµP = M . A discrete for the form factors in AdS/CFT to the exact Drell-Yan- four-dimensional spectrum follows when we impose the West expression in terms of light-front wavefunctions. In + boundary condition ψ±(z = 1/ΛQCD) = 0. One has Mα,k = the case of a two-parton constituent bound state the cor- − respondence between the string amplitude Φ(z) and the βα,kΛQCD, M = βα+1,kΛQCD, with a scale-independent α,k e mass ratio [40]. The βα,k are the ﬁrst zeros of the Bessel light-front wave function ψ(x, b) is expressed in closed eigenfunctions. form [1]

Figure 2(a) shows the predicted orbital spectrum of ¯ ¯ 2 ¯ ¯2 R3 |Φ(ζ)| the nucleon states and Fig. 2(b) the ∆ orbital resonances. ¯ψe(x, ζ)¯ = x(1 − x) e3A(ζ) , (3) The spin 3/2 trajectories are determined from the cor- 2π ζ4 responding Rarita-Schwinger equation. The data for the 2 2 baryon spectra are from S. Eidelman et al. [55]. The in- where ζ = x(1 − x)b⊥. Here b⊥ is the impact separation ternal parity of states is determined from the SU(6) spin- and Fourier conjugate to k⊥. The variable ζ, 0 ≤ ζ ≤ −1 flavor symmetry. ΛQCD, represents the invariant separation between point- like constituents, and it is also the holographic variable Since only one parameter, the QCD mass scale ΛQCD, is introduced, the agreement with the pattern of physi- z in AdS; i.e., we can identify ζ = z. The prediction for cal states is remarkable. In particular, the ratio of ∆ to the meson light-front wavefunction is shown in Fig. 3. We nucleon trajectories is determined by the ratio of zeros can also transform the equation of motion in the fifth di- of Bessel functions. The predicted mass spectrum in the mension using the z to ζ mapping to obtain an effective truncated space model is linear M ∝ L at high orbital an- two-particle light-front radial equation gular momentum, in contrast to the quadratic dependence · 2 ¸ M 2 ∝ L in the usual Regge parametrization. d 2 − 2 + V (ζ) φ(ζ) = M φ(ζ), (4) Our approach shows that there is an exact correspon- dζ dence between the fifth-dimensional coordinate of anti-de 2 2 Sitter space z and a specific impact variable ζ in the light- with the effective potential V (ζ) → −(1 − 4L )/4ζ in the − 3 front formalism which measures the separation of the con- conformal limit. The solution to (4) is φ(z) = z 2 Φ(z) = 1 stituents within the hadron in ordinary space-time. The Cz 2 JL(zM). This equation reproduces the AdS/CFT amplitude Φ(z) describing the hadronic state in AdS5 can solutions. The lowest stable state is determined by the be precisely mapped to the light-front wavefunctions ψn/h Breitenlohner-Freedman bound [56] and its eigenvalues by of hadrons in physical space-time[1], thus providing a rel- the boundary conditions at φ(z = 1/ΛQCD) = 0 and given 6 Stanley J. Brodsky: Hadron Spectroscopy and Structure from AdS/CFT

Fig. 3. AdS/QCD Predictions for the L = 0 and L = 1 LFWFs of a meson

in terms of the roots of the Bessel functions: ML,k = βL,kΛQCD. Normalized LFWFs follow from (3) p ¡ ¢ e −1 ψL,k(x, ζ) = BL,k x(1 − x)JL (ζβL,kΛQCD) θ z ≤ ΛQCD , Fig. 4. AdS/QCD Predictions for the pion form factor. (5) − 1 where BL,k = π 2 ΛQCD J1+L(βL,k). The resulting wavefunctions (see: Fig. 3) display confinement at large inter- twist perturbative QCD prediction for the pion form fac- quark separation and conformal symmetry at short dis- tor by a factor of 16/9 compared to the prediction based tances, reproducing dimensional counting rules for hard on the asymptotic form, bringing the PQCD prediction exclusive processes in agreement with perturbative QCD. close to the empirical pion form factor [58]. The hadron form factors can be predicted from over- Since they are complete and orthonormal, the AdS/CFT lap integrals in AdS space or equivalently by using the model wavefunctions can be used as an initial ansatz for Drell-Yan-West formula in physical space-time. The pre- a variational treatment or as a basis for the diagonal- diction for the pion form factor is shown in Fig. 4. The ization of the light-front QCD Hamiltonian. We are now form factor at high Q2 receives contributions from small in fact investigating this possibility with J. Vary and A. Harindranath. The wavefunctions predicted by AdS/QCD ζ, corresponding to small b⊥ = O(1/Q) ( high relative have many phenomenological applications ranging from k⊥ = O(Q) as well as x → 1. The AdS/CFT dynamics is thus distinct from endpoint models [57] in which the exclusive B and D decays, deeply virtual Compton scat- LFWF is evaluated solely at small transverse momentum tering and exclusive reactions such as form factors, two- or large impact separation. photon processes, and two body scattering. A connection The x → 1 endpoint domain is often referred to as between the theories and tools used in string theory and a ”soft” Feynman contribution. In fact x → 1 for the the fundamental constituents of matter, quarks and glu- struck quark requires that all of the spectators have x = ons, has thus been found. k+/P + = (k0 + kz)/P + → 0; this in turn requires high The application of AdS/CFT to QCD phenomenology longitudinal momenta kz → −∞ for all spectators – un- is now being developed in many new directions, incor- less one has both massless spectator quarks m ≡ 0 with porating finite quark masses, chiral symmetry breaking, asymptotic freedom, and finite temperature effects. Some zero transverse momentum k⊥ ≡ 0, which is a regime of measure zero. If one uses a covariant formalism, such as recent papers are given in refs. [59–68]. the Bethe-Salpeter theory, then the virtuality of the struck 2 2 2 k⊥+m Acknowledgments quark becomes infinitely spacelike: kF ∼ − 1−x in the endpoint domain. Thus, actually, x → 1 corresponds to Work supported by the Department of Energy under high relative longitudinal momentum; it is as hard a do- contract number DE–AC02–76SF00515. The AdS/CFT main in the hadron wavefunction as high transverse mo- results reported here were done in collaboration with Guy mentum. de Téramond. It is also interesting to note that the distribution amplitude predictedp by AdS/CFT at the hadronic scale is φ (x, Q) = √4 f x(1 − x) from both the harmonic os- π 3π π cillator and truncated space models is quite different than the asymptotic distribution amplitude predicted from the References PQCD evolution√ [6] of the pion distribution amplitude φπ(x, Q → ∞) = 3fπx(1 − x). The broader shape of the 1. S. J. Brodsky and G. F. de Teramond, Phys. Rev. Lett. 96, pion distribution increases the magnitude of the leading 201601 (2006) [arXiv:hep-ph/0602252]. Stanley J. Brodsky: Hadron Spectroscopy and Structure from AdS/CFT 7

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