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- The Heavy Quark Potential in Two-Dimentional QCD with Adjoint Matter
- Heavy quark pair correlations in QCD
- Heavy Quark Distribution Functions from QCD
- Heavy-quark production in massless quark scattering at two loops in QCD
- QCD Corrections to Associated Higgs Boson-Heavy Quark Production
- The Heavy Quark Expansion of QCD
- Lattice QCD study of the heavy-heavy-light quark potential
- Heavy quark production near the threshold in QCD
- Heavy Quark Production in the Semihard QCD Approach at HERA and Beyond
- Determination of the renormalized heavy-quark mass in Lattice QCD
- The QCD Pomeron in Ultraperipheral Heavy Ion Collisions II. Heavy Quark Production
- Heavy Quark Production at the TEVATRON in the Semihard QCD Approach and the Unintegrated Gl
- Heavy-quark production in massless quark scattering at two loops in QCD
- The Role of the QCD Vacuum in the Heavy-Quark Bound State Dynamics
- Heavy quark production in the semihard QCD approach at THERA

UCSD/PTH 00-05

Running of the heavy quark production current and 1/|k| potential in QCD

Aneesh V. Manohar? and Iain W. Stewart?

arXiv:hep-ph/0003107v3 26 Jan 2001

Department of Physics, University of California at San Diego, 9500 Gilman Drive, La Jolla, CA 92093

Abstract

The 1/|k| contribution to the heavy quark potential is ?rst generated at one loop order in QCD. We compute the two loop anomalous dimension for this potential, and ?nd that the renormalization group running is signi?cant. The next-to-leading-log coe?cient for the heavy quark production current near threshold is determined. The velocity renormalization group result reproduces 2 the α3 s ln (αs ) “non-renormalization group logarithms” of Kniehl and Penin.

Typeset using REVTEX

? amanohar@ucsd.edu ? iain@schwinger.ucsd.edu

1

I. INTRODUCTION

For systems involving a heavy quark-antiquark pair near threshold it is useful to combine the QCD coupling constant expansion with an expansion in powers of the relative velocity v . This expansion is facilitated by using non-relativistic QCD formulated as an e?ective ?eld theory with an explicit power counting in v [1–14]. For the potential between a heavy quark and antiquark this double expansion takes the form

∞ ∞

V (p, p′ ) =

n=?2

V (n) ,

V (n) =

j =1

V (n,j ) , (1)

where V (n) ? v n ,

j V (n,j ) ? v n αs .

The even terms V (2k) are ?rst generated at tree-level (order αs ), and the odd terms V (2k+1)

2 are ?rst generated at one loop (order αs ).

Matrix elements for non-relativistic QCD systems typically depend on logarithms of the velocity v . For small v it is convenient to sum large logarithms of the form αs (mv ) ln(v ) and αs (mv 2 ) ln(v ) by using renormalization group equations in the e?ective theory. This reorganizes the series in j in Eq. (1) so that: V (n) =

j

? (n,j ) , V

where

? (n,j ) ? v n αs (m)j V

∞

[αs (m) ln(v )]k .

k =0

(2)

The simplest example of such a summation is the use of a running coupling constant, αs (?), instead of the coupling at the matching scale αs (m). For ? < m the running coupling includes a series of αs (m) ln(?/m) terms. However, it should be emphasized that the complete set of renormalization group logarithms are not determined by the simple replacement αs (m) → αs (?). A complication in summing the logarithms is the presence of two low energy scales: the typical momenta of the heavy quark ? mv (soft scale), and typical energy ? mv 2 (ultrasoft scale). Two approaches have been proposed for dealing with the presence of two scales, one stage and two stage running. With two stage running, one matches QCD onto an e?ective theory at the scale ? = m and then runs to the scale ? = mv . At ? = mv one matches onto an e?ective theory called pNRQCD [8,15] which has composite q q ? ?elds, and then considers the running to ? = mv 2 . In vNRQCD [14], the running occurs in a single stage using a velocity renormalization group. The velocity renormalization group takes into account that the scales mv and mv 2 are tied together by the heavy quark equation of motion for all 2

? < m. We use dimensional regularization and the MS scheme with both the ultrasoft scale ?U ? mv 2 and the soft scale ?S ? mv given in terms of a single subtraction point velocity ν : ?U = mν 2 and ?S = mν . The renormalization group equations are written for the variable ν . It is an interesting question as to whether both the one and two stage methods of running will sum the full set of αs ln(v ) terms. In this paper only the single stage running will be considered. ? (?2,1) and V ? (?2,2) , is The running of the Coulomb potential at one and two loops, V determined by the running coupling constant αs (?) [16] 1 . The summation of the leading logarithms for the the v 0 potential was carried out in Refs. [18,19]. In this paper we extend this analysis to the 1/|k| potential by calculating its two loop anomalous dimension. If mv 2 ? ΛQCD , the v expansion can be applied to non-relativistic QCD systems in ? production near threshold where mv 2 ? a perturbative manner. This is the case for tt 4 GeV, and is the situation that will be analyzed in this paper. Of particular interest is the Coulombic regime where v ? αs . In this regime the expansion in Eq. (1) has the form ? (?2,3) + V ? (?1,2) + V ? (0,1) + . . . ? (?2,2) + V ? (?2,1) + V V = V ? αs v2 +

2 αs v2

+

2 3 αs αs + + αs v 0 2 v v

+ ... .

(3)

If the αs ln(v ) dependence is treated perturbatively these terms are referred to as the leading order (LO), next-to-leading order (NLO), and next-to-next-to-leading order (NNLO) potentials. Note that since the 1/|k| potential ?rst occurs at one loop, it only contributes at NNLO. When the series in αs ln v are summed, the terms in Eq. (3) will be referred to as leading-log (LL), next-to-leading log (NLL) and next-to-next-to-leading log (NNLL), respectively. In the Coulomb regime, the Coulomb potential must be kept to all orders. Each additional Coulomb insertion gives a αs /v 2 plus a factor of v (from the potential loop), so each new Coulomb interaction costs a factor of αs /v ? 1. ?, a non-relativistic expansion must also be made To study the threshold production of tt for the electromagnetic production current2 ? γi t = t

p ? i ? c1 ψp σ χ?p ?

c3 c2 ? ψp p · σ pi χ? ψ ? p2 σ i χ? ?p ? ?p + . . . . 2 2m m2 p

(4)

1 At 2 We

three loops ultrasoft gluons can contribute to the running of the static potential [17]. will ignore e?ects associated with the top quark width. 3

The ?elds ψ ? and χ? create non-relativistic top quarks and antiquarks respectively. The c1 term contributes at order v 0 , and the c2 and c3 terms contribute at order v 2 . The current on the LHS of Eq. (4) is conserved, and has no anomalous dimension in QCD. However the non-relativistic current operators on the RHS are scale dependent in the e?ective theory, and the coe?cients cj therefore depend on logarithms of ?. The coe?cients cj each have an

2 expansion in αs . The matching at ? ? m is known to order αs for c1 [20,21], and to order

αs for c2 and c3 [7], so the production current is known to NNLO with partial N3 LO results. At LL order, one needs the tree-level matching c1 = 1 at ? = m, and the v 2 coe?cients c2 and c3 can be set to zero. There is no one loop anomalous dimension for the operator

? i ? ψp σ χ?p , so the LL result is that c1 = 1 at all ν .

At NLL order, we need the one loop matching for c1 at ? = m, and the two loop running for c1 . The coe?cients c2,3 ?rst enter at NNLL, at which order one would also need the three-loop anomalous dimension for c1 . At two loops, the anomalous dimension for c1 was computed at the matching scale ? = m [20,21] ? ? c 1 (? ) ?? = ?CF 1 1 2 CF + CA αs (m) , 3 2 (5)

?=m

by studying the two loop matching condition for c1 . For ? < m the anomalous dimension no longer has the simple form Eq. (5), but depends on the running of the quark potential. This anomalous dimension was computed in Ref. [14], and depends on the running values ? (?2,1) ]2 , V ? (?2,1) × V ? (0,1) , and V ? (?1,2) (see Eq. (42) below). It is interesting that the structure [V of this result implies that determining the RHS of Eq. (5) for ? < m requires the LL values ? (?2,1) and V ? (0,1) , but the NLL value of V ? (?1,2) . The one loop running of V ? (?2,1) is well of V ? (?2,2) was computed in Refs. [18,19]. The two loop running known, and the running of V ? (?1,2) is computed in this paper. Using the running of these terms in the potential, of V we arrive at a complete NLL expression for c1 . The running of the non-relativistic scalar current is also brie?y discussed. In section II the e?ective theory is reviewed. We explain how reparameterization invariance ?xes the value of the lowest order coupling of an ultrasoft gluon to the Coulomb potential. The details of the computation of the two loop anomalous dimension for the 1/|k| potential are given in section III, and in the appendices. In section III we give a derivation of the anomalous dimension using on-shell potentials, while in appendix B we repeat the derivation in the presence of o?-shell potentials. Readers not interested in the technical details can skip to section IV, where our results are discussed. In section IV we expand 4

our renormalization group improved results in powers of αs to compare to ?nite order calculations in the literature. For the color singlet 1/|k| potential the ?rst αs ln(v ) term in the series was computed in Ref. [15], and our result for this term agrees with theirs. In

3 Ref. [22], Kniehl and Penin computed the αs ln2 (αs ) terms in the wavefunction at the origin

which they refer to as “non-renormalization group logarithms”, since they do not involve factors of the β -function for αs . We show that the second term in the series generated by our NLL production current agrees with the result in Ref. [22]. Thus, the solution of the renormalization group equations in the velocity renormalization group method does include these logarithms. Finally, we discuss our result for the NLL 1/|k| potential and production current.

II. THE vNRQCD LAGRANGIAN

The vNRQCD e?ective Lagrangian has the form [14] L = Lu + Lp + Ls . (6)

The ultrasoft Lagrangian Lu involves the ?elds ψp which annihilate a quark, χp which annihilate an antiquark, and A? which annihilate and create ultrasoft gluons. The potential Lagrangian Lp contains operators with four or more quark ?elds including the quark-antiquark potential. Finally, the soft Lagrangian Ls contains all terms that involve soft particles which have energy and momenta of order mv . The terms we need in the ultrasoft Lagrangian include 1 Lu = ? F ?ν F?ν + 4 +

p ? iD 0 ? ψp p

p4 (p ? iD)2 ψp + 2m 8m3 (7)

χ? p

(p ? iD)2 p4 iD ? + χp . 2m 8m3

0

? 0 0 0 ? 0 The covariant derivative is D ? = ? ? + ig?? U A = (D , ?D), so that D = ? + ig?U A ,

D = ? ? ig?? U A, and involves only the ultrasoft gluon ?elds. The ultrasoft scale parameter ?U = mν 2 , where ν ? v is the subtraction velocity. This v scaling for ?U is required for a consistent power counting in d dimensions [23]. The covariant derivative on ψp and χp ? A for the 3 and ? contain the color matrices T A and T 3 representations, respectively. The Lagrangian Lp includes both the traditional quark potential and ultrasoft corrections to this potential which we will denote by Lpu : 5

p

p′

-p

-p′

FIG. 1. QCD diagrams for tree level matching.

Lp = ?

p,p′

? ? ? Vαβλτ (p, p′ ) ?2 S ψp′ α ψp β χ?p′ λ χ?p τ

+ Lpu .

(8)

The terms we need in Lpu are ?xed by reparameterization invariance [24] and will be described below. The on-shell potential V (p, p′ )αβλτ has an expansion in αs and v , and α, β, λ, τ denote color and spin indices. We will use the color basis in which the poten? . The tree level diagrams in tial V is written as a linear combination of 1 ? 1 and T ? T Fig. 1 generate terms of O(v 2k αs ) in the QCD potential. The order v ?2 Coulomb potential is ? A ) Vc + (1 ? 1) Vc , V (?2) = (T A ? T k2 k2

(T,1) where the coe?cients Vc have an expansion in αs . The order v 0 potential includes (T ) (1)

(9)

V (0)

(T ) 2 ′2 (T ) ? A ) ? V2 + Vr (p + p ) + Vs S2 + VΛ Λ(p′ , p) + Vt T (k)? = (T A ? T m2 2 m2 k2 m2 m2 m2

?

(T )

(T )

(T )

?

where k = p′ ? p and S= σ1 + σ2 , 2

V V (1) +(1 ? 1) ? 2 2 + s 2 S2 ? , m m Λ(p′ , p) = ?i

?

(1)

?

(10)

S · (p′ × p) , k2

T (k) = σ 1 · σ 2 ?

3 k · σ1 k · σ2 . k2

(11)

Matching the two diagrams in Fig. 1 to the v ?2 and v 0 potentials at ? = m gives

(T ) Vc = 4παs (m) , (T ) Vr = 4παs (m) , (T ) Vs =? (1) Vs

VΛ = ?6παs (m) ,

(1) Vc = 0,

(T )

Vt = 0,

(T )

=?

(1)

παs (m) , 3

1 4παs (m) + π αs (m) , 3 Nc 2 (Nc ? 1) = π αs (m) , 2 2Nc (12)

V2

(T )

V2 = 0 .

The LL values for the coe?cients of the V (?2) and V (0) potentials will be needed below and are summarized in Appendix A. They are obtained by using the tree-level matching values in Eq. (12) and running using the one loop anomalous dimensions computed in Ref. [19]. 6

The order 1/v potential includes V

(?1)

π2 (T ) ? A ) + V (1) (1 ? 1) . = Vk (T A ? T k m |k|

(13)

Tree level matching gives V (?1) = 0, and V (?1) has zero one loop anomalous dimension [19], so V (?1) = 0 at LL order as well. At one loop in QCD, order 1/v potentials of the form in Eq. (13) are generated. The one loop matching of the on-shell potential at ? = m gives [23] Vk

(T ) 2 = αs (m)

7CA Cd , ? 8 8

2 Vk = αs (m)

(1)

C1 . 2

(14)

2 2 2 The color group theory factors are CF = (Nc ? 1)/(2Nc ), CA = Nc , C1 = (Nc ? 1)/(4Nc ),

and Cd = Nc ? 4/Nc . For the color singlet channel Eq. (14) agrees with Refs. [25,26]. In the language of the threshold expansion [10] the value of the coe?cients in Eqs. (12) and (14) are from integrating out o?-shell potential gluons at the hard scale ? ? m where ν = 1 [23]. In the next section we will compute the two loop anomalous dimension for V (?1) , and determine the NLL value of the coe?cients in Eq. (13). In addition we need ultrasoft corrections to the potential which are contained in Lpu . Reparameterization invariance [24] restricts the form of some of these terms by requiring that only the linear combination p ? iD can appear. Here the covariant derivative acts on ? a quark or antiquark ?eld with label p. The reparameterization invariant form of the T ? T Coulomb potential operator is

? A ?A χ? ψp ′ T ψp ?p′ T χ?p

(p′ ? p)2

→

TA 1 ? ?A ψp χ? ψp′ ? ?p′ T χ?p ′ 2 2 (p ? p + iD) ?A T 1 ? A ψp χ? + ψp χ?p , ′ T ′ ? ?p 2 (?p′ + p + iD )2

(15)

? ? → ← ? where D = D + D . Terms in the v expansion are then generated by expanding Eq. (15)

with D ? p′ ? p. As written the ordering of color generators in Eq. (15) is ambiguous. ? → The correct ordering in the expansion is to write factors of D to the right of the T A , and ← ? factors of D to the left of the T A . Expanding Eq. (15) and keeping only the terms that we will need gives Lpu

(T ) ABC 2i Vc f ? ? A ? ? C ?B = ?2 S ?U k · (g A ) ψp′ T ψp χ?p′ T χ?p 4 k ? ? ? 2 ( k · ? )2 A ? i k · ? ? (T ) 2? ?A ? + 2 T ψp χ? +Vc ?S ψp′ ?p′ T χ?p 4 4 6 k 2k k ? ? ? ( k · ?) 2 ? A ?2 ?ik · ? ? A (T ) 2? ? T χ?p , ? 4 +2 +Vc ?S ψp′ T ψp χ?p′ k4 2k k6

(16)

7

→

FIG. 2. Matching for the operator attaching an ultrasoft gluon to a potential interaction.

? ? → ← ? where ? = ? + ? . The ?rst term couples an ultrasoft gluon to a four quark operator.

The terms in the second and third lines in Eq. (16) contain order 1/v and v 0 terms from the multipole expansion of the Coulomb potential. The ?rst term could also have been determined from the on-shell matching calculation shown in Fig. 2. However, by determining the terms in Eq. (16) using reparameterization invariance rather than matching we know that the coe?cients remain equal to Vc to all orders in perturbation theory. This saves us from the extra work that would be involved in computing the anomalous dimensions for these terms in Lpu . The terms in the soft Lagrangian include Ls =

q ? ?g 2 ?2 S p,p′ ,q,q ′ ν ? +? ?q / q ?q + c ?q q 2 cq q ? Aν q ? q Aq 2

(17)

1 1 ν (σ) ν (σ) ψp′ ? [A? ψp′ ? {A? q ′ , Aq ]U?ν ψp + q ′ , Aq }W?ν ψp 2 2

(σ) ?) . ψp ) (? ?q′ γ ? T B ?q ) + (ψ → χ, T → T +ψp′ ? [? cq′ , cq ]Y (σ) ψp + (ψp′ ? T B Z?

The ?elds A? q and cq are the soft gluon and ghost ?elds, and ?q is a massless soft quark ?eld with nf ?avor components. U , W , Y , and Z are functions of (p, p′ , q, q ′) and matrices in spin and the index σ denotes the relative order in the v expansion. For Feynman gauge and the case p2 = p′ 2 these functions were derived in Ref. [14,19]. Beyond one loop terms proportional to (p2 ? p′ 2 ) will be needed in Ls , since besides its soft energy q 0 ? mv the Aq gluons can carry away a residual energy of order mv 2 . The LL values for the functions U , W , Y , and Z can be found in Appendix A of Ref. [23]. In addition, some NLL contributions to Ls will be needed and will be discussed in section III A. These additional contributions are obtained from one loop matching with two-loop renormalization group improvement. As an aside, note that it is not necessary to consider the ultrasoft renormalization of the vertices given in the soft Lagrangian in Eq. (17). One might think that diagrams such as

(18) 8

would e?ect the running of the coe?cients in the soft Lagrangian. Diagrams analogous to the one in Eq. (18), but with only soft gluons and quarks generate the running of the coe?cient functions in the soft Lagrangian3 in Ref. [19]. However, the graph in Eq. (18) has only one heavy quark, so a distinction between soft and ultrasoft gluons is unnecessary at this point. Noting that the soft vertices will always occur in pairs, it is in fact consistent to only dress pairs of the soft vertices by ultrasoft gluons:

(19) Since these diagrams involve two heavy quarks, both types of gluons can occur. Since in the end it is only graphs such as Eq. (19) with two soft vertices that are relevant for constructing the theory, it is consistent to include the ultrasoft renormalization of soft vertices as a contribution to the four-quark operator in Eq. (19), rather than treating the subgraph as a contribution to the soft vertex, as in Eq. (18). Along with the diagrams in Eq. (19) there are graphs in which the ultrasoft gluon is exchanged between the two heavy quarks.

Ref. [19] the running of Ls was calculated by examining loops with soft gluons that contribute to the Compton scattering process prior to integrating out the soft quarks. There it was noted that all ultraviolet divergent diagrams are in one-to-one correspondence with graphs in HQET, so that the running of this Lagrangian could be obtained from the known running in HQET [27]. 9

3 In

III. TWO LOOP ANOMALOUS DIMENSION FOR V (?1)

To calculate the NLL anomalous dimension for the 1/|k| potentials we need to consider

3 graphs in the e?ective theory of order4 αs /v . These diagrams come in two classes, those

with soft gluons, and those with a single ultrasoft gluon. The total anomalous dimension for the 1/|k| potential is γ (1,T ) = νd/dν Vk

(1,T )

. Since ?S = mν and ?U = mν 2 , γ (1,T ) can be

written as the sum of a soft and ultrasoft anomalous dimension γ (1,T ) = γS where γS

(1,T ) (1,T )

+ 2 γU

(1,T )

,

(1,T )

(20) . In the remainder of this section

= ?S ?/??S Vk

(1,T )

and γU

(1,T )

= ?U ?/??U Vk

we discuss the computation of these two loop anomalous dimensions in detail. The calculation is split into two parts, graphs with soft vertices and graphs with ultrasoft vertices. Graphs with soft gluons only contribute to γS , while those with an ultrasoft gluon contribute to both γS and γU .

A. Soft contributions

3 The order αs /v diagrams containing soft gluons that contribute to the anomalous di-

mension are shown in Fig. 3. The sum of diagrams forms a gauge invariant set. The two loop graphs in Figs. 3a and 3b involve an iteration of a potential and a soft loop. The vertices in these graphs are of LL order (tree level matching with one loop running) and are given in Ref. [23]. In Figs. 3a and 3b, counting powers of v from the propagators and from the loop measures gives a v 1 , so the sum of powers of v for the three (amputated) vertices must give an overall 1/v 2 . The v scaling for the two soft vertices is σ + σ ′ ? 2. In Fig. 3 we show two possibilities: a) has one V (?2) insertion and two soft vertices from Eq. (17) such that σ ′ + σ = 2, and b) has one insertion of a V (0) potential from Eq. (10) and two soft vertices such that σ ′ = σ = 0. We could also have a V (?1) potential plus two soft vertices where σ + σ ′ = 1; however this diagram is identically zero. The graphs where the potential and soft loop are exchanged simply give a factor of 2.

is the size (in v ) of the amputated diagrams, so in contrast to the general power counting formula in Ref. [14] we are not including the powers of v generated by external lines. 10

4 This

σ Vc V(0)

0

(a)

0

σ′

1

(b)

0

1

0

(c)

(d)

(e)

FIG. 3. Order α3 s /v graphs containing soft gluons, ghosts, or massless quarks which are all denoted by a zigzag line. In (a) the dot denotes the Coulomb potential, while in (b) the dot denotes the order v 0 potential. The boxes denote soft vertices with insertions of the functions U (σ) , W (σ) , Y (σ) , or Z (σ) . In (a) the indices σ + σ ′ = 2. In (c), (d), and (e) the ? vertex is obtained from the one loop matching in Fig. 4.

The one loop graphs in Fig. 3c, 3d, and 3e involve additional vertices in Ls , denoted ?, which are of NLL order (from one loop matching with two loop running). The one loop matching calculation for these vertices is sketched in Fig. 4. There are a large number of diagrams in the full theory (graphs on the left hand side), so only a few representative examples have been shown. To obtain the values for the operators on the right hand side we subtract purely soft e?ective theory diagrams from those in the full theory. To see how these operators arise, it is useful to recall that in the threshold expansion [7,11] soft heavy quarks have a propagator 1 1 = P ? iπδ (q0 ) , q0 + i? q0 (21)

where P stands for the principal value. In our approach, o?-shell potential gluons and soft quarks are integrated out at the scale m when constructing the e?ective theory. When integrating out the soft heavy quarks the principal value term in Eq. (21) goes directly into a coe?cient in the soft Lagrangian since this term is consistent with the scaling in the soft 11

a)

+

+ ...

→ →

1

b)

+

+ ...

1

FIG. 4. Contributions to the soft Lagrangian from one loop matching. In the full theory diagrams on the left the thick lines are massive quarks, while the thin lines are massless quarks. The matching in a) gives αs corrections to the functions U (1) , W (1) , Y (1) , and Z (1) in Eq. (17). The matching in b) induces new operators that involve the scattering of soft gluons, ghosts, or light quarks o? of a four fermion potential.

regime, q0 ? mv . For instance, in Eq. (17), U00 = 1/q0 . The delta function contribution in Eq. (21) is associated with the potential regime since q0 ? 0. When the delta function appears in a loop in the full theory (or threshold expansion) it forces gluons in the loop to have zero energy, or in other words to become potential gluons. It is these contributions which do not appear in the soft e?ective theory diagrams and must be made up by the operators shown on the right hand side of Fig. 4. The total contribution to the anomalous dimensions from the soft diagrams in Fig. 3 is γS

(T )

(0)

=?

β0 (7CA ? Cd ) 3 8 C A (C A + C d ) 3 αs (mν ) ? αs (mν ) , 8π 3π β0 C1 3 16CA C1 3 αs (mν ) + αs (mν ) , 2π π (22)

γS = ?

(1)

where β0 = 11CA /3 ? 4TF nf /3, nf is the number of massless soft quarks, and Vc (ν ) = 4παs (mν ) was used. In Eq. (22) the terms proportional to β0 can be inferred from Eq. (14). They simply turn the αs (m)’s in the matching result into running αs ’s. At one and two loops terms proportional to the β -function for αs completely determine the soft anomalous dimension for the Coulomb potential. However, the 1/|k| potentials have additional contributions because the soft diagrams in Fig. 3c, 3d, and 3e have infrared divergences. The IR divergences from purely soft diagrams are not true IR divergences in the e?ective theory. For instance, in general they do not match up with IR divergences in QCD. The true IR divergences are from momenta < mv 2 , and the desired ultraviolet divergences are from momenta ≥ m. Instead, the soft IR divergences are from momenta < mv , and match up with 12

ultrasoft UV divergences that are from momenta ≥ mv to carry these UV divergences up to the hard scale. Writing the soft IR divergence 1 ?IR = 1 ?U V ? 1 ?U V ? 1 ?IR , (23)

the ?rst term contributes to the anomalous dimension in Eq. (22). The 1/?UV ? 1/?IR term can be ignored since it simply takes the corresponding ultrasoft UV divergence up to the hard scale m.5 Thus, to compute γS , all divergences from soft loops should be treated as UV divergences. The terms not proportional to β0 in Eq. (22) can be inferred from the result of the ultrasoft calculation in Eq. (30) of the next section. Despite the fact that Eq. (22) can be inferred without a direct calculation it is worthwhile to examine the diagrams in Fig. 3. Consider the graphs in Figs. 3a and 3b in Feynman gauge. The sub-loop with soft gluons is divergent, while the remaining potential loop is convergent. There is also a set of one loop diagrams (not shown) where the soft sub-loop is replaced by the one loop counterterms for V derived in Ref. [19]. We ?nd that these counterterm graphs exactly cancel against a set of divergences in Fig. 3a and 3b. For Fig. 3b there is an exact cancellation, and so there is no operator mixing between V (0) and V (?1) . However, there are divergences that appear in Fig. 3a that have no corresponding counterterm graphs. Consider the soft gluon case (the ghost and soft quark cases are similar). After performing the k 0 integration the loop integral for Fig. 3a is d

d?1 (σ) U?ν U ?ν (σ ) , d t 2 0 2 t [(t ) ? (t + q ? p′ )2 ] d

′

1 q 2 (E ? q /m)(p ? q)2

(24)

where p and p′ are the momenta of the incoming and outgoing quarks, E = p2 /m and in Eq. (24) the U ’s depend on q, t, p′ and t0 . For the divergences of interest performing the t integral (the soft loop) in d = 4 ? 2? dimensions gives a factor of (p′ 2 ? q2 )2 + ... , m2 (p′ ? q)4+2? ? (25)

where the ellipsis denote order ?0 terms. The remaining loop integration is ?nite. For the one loop graph that corresponds to the soft sub-loop, the loop momenta q in Eq. (25) is

result, that there are no true IR divergences in the soft regime has not been proven to all orders in perturbation theory. However, its is likely that all IR divergences can be attributed to ultrasoft and collinear gluons in the spirit of the Coleman-Norton theorem [28], plus IR divergences associated with the Coulomb regime that are reproduced by iterations of the potential. 13

5 This

replaced by p′ , and this diagram vanishes on-shell by energy conservation so no counterterm is generated. Performing the ?nal integration and including the factor of 2 from the left-right symmetric graph gives

(T ) 2 (?S ) αs (? S ) Fig. 3a = i Vc ? 2 β0 ?2 S ?AT ? B ) 1 + 2 ln ?S + . . . . (T A T B ? T 32 m|k| ? |k|2

(26)

The divergence in Eq. (26) contributes to the anomalous dimension for Vk . This seems slightly unusual because it was generated by a sub-divergence, whereas usually only the overall divergence in a diagram is relevant. In this diagram the loop integral with soft gluons generates a 1/? pole, and the remaining potential loop integral generates the 1/|k| factor. The corresponding diagrams in QCD include graphs such as the vacuum polarization of one of the gluons in the box diagram. In this full theory graph the subdivergence due to the vacuum polarization insertion would be canceled by a counterterm. However, in the e?ective theory this divergence is instead absorbed into the coe?cients of terms in the quark potential because the potential gluon components have been integrated out. Since matching the full theory box diagram gives a contribution to the 1/|k| potential, it is not surprising that gluon vacuum polarization in the box graph contributes to the anomalous dimension of this potential. An alternative to the approach used to derive Eq. (26) is to use o?-shell matching and running. In this case the soft anomalous dimension analysis will be di?erent (since, for instance, the o?-shell potential is gauge dependent). This approach is discussed in Appendix B, where it is shown that the ?nal answer for physical observables is unchanged. The diagrams in Figs. 3c, 3d, and 3e are tedious to evaluate due to the large number of diagrams necessary for the matching calculation in Fig. 4.6 Since the graphs in Figs. 3c, 3d, and 3e are one-loop diagrams there is no cancellation from counterterms. In Feynman gauge Fig. 3c, d, e = i

? 3 π 2 ?2 1 S αs (?S ) 4 ?A) C1 TF nf (1 ? 1) + CA TF nf ? Cd TF nf (T A ? T m|k| 4π ? 3 3 37 65 2 7 ? A ) . (27) + CA C1 (1 ? 1) ? CA Cd + C A (T A ? T 3 4 12

Only the terms proportional to nf in Eq. (27) have been checked by direct calculation. Also, in Eq. (27) we have assumed that the ? operators simply run with the strong coupling

fact once a contribution to ? has been identi?ed it is simpler to directly evaluate the two-loop diagram obtained by combining the steps in Fig. 4 and Fig. 3. 14

6 In

(a) 1 (e) 1 2 2

(b) 1 (f) 1 2 2

(c) 1 (g) 1 2 2

(d) 1 (h) 1 2 2

FIG. 5. Order α3 s /v two loop graphs with an ultrasoft gluon and two potential insertions. The topologies shown give several di?erent classes of diagrams depending on the vertices used as explained in the text. The diagrams obtained by ?ipping the graphs left-to-right and up-to-down are to be understood.

constant, αs (mν ). To motivate this, recall that a theory of propagating soft quarks and gluons has the same singularity structure as Heavy Quark E?ective Theory (HQET). The operators that are generated in Fig. 4 correspond to diagrams in HQET with insertions of ?2 /(m) or a p · A/m vertex. Since these operators do not run in HQET the operators that are constructed in Fig. 4 should also simply run with the strong coupling constant.

B. Ultrasoft contributions

3 Next consider the order αs /v diagrams with ultrasoft gluons. At one loop we have

a single insertion of the V (?1) potential dressed by an ultrasoft gluon with gA0 couplings. These diagrams are obviously zero in Coulomb gauge and in Feynman gauge it was shown in Ref. [14] that, with any potential, the sum of this set of one loop diagrams is also identically zero. At two loops in an arbitrary gauge there are many possible contributions. There are diagrams with two V (?2) vertices, and an ultrasoft tadpole generated by the seagull A2 operator attached to one of the quark lines. These graphs do not have logarithmic divergences and therefore do not contribute to the anomalous dimension. There are also diagrams that are zero because they are odd in an ultrasoft momenta which we can omit. Next consider the topologies shown in Fig. 5. Several classes of diagrams are generated depending on the vertices used: 1. vertex 1 and 2 are V (?2) , and the ultrasoft gluon couples with p · A/m, 2. vertex 1 and 2 are V (?2) , the ultrasoft gluon couples with gA0 , and there are two insertions of p · ?/m on quark lines, 3. vertex 1 and 2 are V (?2) , the ultrasoft gluon couples with gA0, and there is one insertion of ?2 /m on a quark line, 15

4. vertex 1 and 2 are V (?2) , the ultrasoft gluon couples with gA0, and there is one insertion of p4 /m3 on a quark line (together with the expansion of factors of the energy that appear in lower order diagrams which should be viewed as corrections to the e?ective theory states, see Refs. [7,23]), 5. vertex 1 is V (?2) , vertex 2 is V (0) and the ultrasoft gluon couples with gA0 , 6. vertex 1 is the order 1/v potential from the multipole expansion of the Coulomb potential given in Eq. (16), vertex 2 is V (?2) , and the ultrasoft gluon couples with gA0 vertices. 7. vertex 1 is the order v 0 potential in Eq. (16), vertex 2 is V (?2) , there is one insertion of p · ?/m on a quark line, and the ultrasoft gluon couples with gA0 vertices. 8. vertex 1 and 2 are v 0 potentials from Eq. (16), and the ultrasoft gluon couples with gA0 vertices. Insertions of operators with ?’s only need to be considered on quark propagators where the multipole expansion was used; together with the graphs in cases 6, 7, and 8 they build up the sub-leading terms in the multipole expansion. The graphs in cases 1, 2, and 5 do not give any contribution to the two loop anomalous dimension. The reason is that all ultraviolet divergences are exactly canceled by one loop counterterm graphs (these counterterms are generated by one loop graphs having one potential insertion dressed by an ultrasoft gluon, and in Feynman gauge were calculated in Refs. [14,19]). The graphs with the topology in Fig. 5c,d are ultraviolet ?nite. For the remaining diagrams we can identify the corresponding counterterm graph by simply shrinking the smallest loop containing the ultrasoft gluon to a point. The only subtlety occurs in Fig. 5h which has overlapping potential and ultrasoft loop integrals. For heavy scalars this graph was analyzed in Ref. [10] with the threshold expansion, while in an e?ective theory for heavy fermions this diagram was analyzed in Ref. [29] for the case where the ultrasoft gluon is massive and couples with derivatives at the vertices. Since the nature of the overlapping integrals does not depend on the structure of the numerator or on having a massive gluon, this analysis will not be repeated here. In the e?ective theory this diagram comes with the appropriate factor of 2, so that it is canceled by the two one loop counterterm graphs that correspond to either making the loop integral on the right large or making the loop integral on the left large. Note that for a φ3 relativistic theory in d = 6 [30], the sub-divergences for this diagram are also canceled in this way, but leave an overall divergence. For the non-relativistic e?ective theory diagram this overall divergence is not present.

16

For the graphs in case 4, the sum of insertions on quark lines inside the loop shared by the ultrasoft gluon are ?nite. The graphs with insertions on quark lines outside this loop are ultraviolet divergent, but are exactly canceled by the counterterm diagrams that correspond to shrinking the ultrasoft loop to a point. Therefore, the graphs in case 4 also do not contribute to the anomalous dimension. In a general gauge the graphs in cases 3, 6, 7, and 8 will contribute to the anomalous dimension. There are also additional graphs with the vertex in Eq. (15) which involves the coupling of an ultrasoft Ai gluon to a potential vertex. Together this set of graphs gives a gauge invariant contribution to the anomalous dimension, so we can simplify their computation by choosing the most convenient gauge. We will choose Coulomb gauge since the graphs in cases 3, 6, 7, and 8 involve ultrasoft A0 gluons and vanish in this gauge. The result for the in?nite part of the the remaining diagrams in Coulomb gauge is:

= 0,

? (T ) 2 ?i αs (?U)?2 1 S [Vc ] ?A , C A C 1 1 ? 1 ? C A (C A + C d )T A ? T 8π m |k| ? 4

(28a)

=

(28b)

=

? (T ) 2 ?i αs (?U)?2 S [Vc ] CA C1 1? 1, 8π m |k| ? 3

(28c)

=

? (T ) 2 2 1 ?i αs (?U)?2 S [Vc ] ? A . (28d) C A C 1 1 ? 1 ? C A (C A + C d )T A ? T 8π m |k| ? 3 12

Equations (28b,c) include the factor of four from their left-right and up-down mirror graphs. In the graphs in Eq. (28) the factor

? 4? ? ?2 1 ?2 ?2 ?2 U ?S S S U + ln = + ln |k| ? E2 ? |k|1+2? E 2? |k|2

(29)

occurs, where E = p2 /m. The ?rst term is included in the result displayed in Eq. (28), and the remaining terms are not shown. For ν ? v , we have ?S ? |k | ? mv , ?U ? E ? mv 2 , so the soft and ultrasoft scale factors correctly minimize possible large logarithms in the e?ective theory. From the sum of diagrams in Eq. (28) we have the following result for the soft and ultrasoft anomalous dimensions of the order 1/|k| potentials: 17

γ S = γ U = C A (C A + C d ) γS = γU = ?CA C1

(1) (1)

(T )

(T )

(T ) αs (mν 2 ) [Vc (ν )]2 , 12π 3

(T ) αs (mν 2 ) [Vc (ν )]2 . 2π 3

(30)

Recall that the soft and ultrasoft anomalous dimensions are given by di?erentiating with respect to ln ?S and ln ?U respectively. It is interesting to ask how the result in Eq. (30) would be reproduced if terms that vanish by the equations of motion were included in our e?ective Lagrangian. It is possible to include a term in our e?ective Lagrangian which makes the graph in Eq. (28b) give no contribution to the anomalous dimension, but the ?nal result for observables remains invariant. This example is discussed in Appendix B.

IV. RESULTS

In this section the NLL heavy quark 1/|k| potential and production current are discussed. After presenting the renormalization group improved results, we re-expand to compare to the ?nite order results in Refs. [15] and [22]. We also discuss the behavior of the NLL 1/|k| potential and the NLL production current as we run down from ν = 1 to ν = v , where v is the Coulombic velocity.

A. The NLL 1/|k| potentials

The total soft and ultrasoft anomalous dimensions for the on-shell 1/|k| potentials are obtained by adding Eqs. (22) and (30). Using the LL coe?cient for the Coulomb potential, Vc (ν ) = 4παs (mν ), we ?nd γS

(T )

=?

γS γU

(1)

(T )

γU

(1)

1 8 β0 (7CA ? Cd ) [αs (mν )]3 ? CA (CA + Cd ) [αs (mν )]3 8π 3π 4 + CA (CA + Cd ) αs (mν 2 )[α(mν )]2 , 3π 1 16 8 = ? β0 C1 [αs (mν )]3 + CA C1 [αs (mν )]3 ? CA C1 αs (mν 2 )[αs (mν )]2 , 2π π π 4 CA (CA + Cd ) αs (mν 2 )[αs (mν )]2 , = 3π 8 = ? CA C1 αs (mν 2 )[αs (mν )]2 . π 18

(31)

In full QCD (taking the QCD scale parameter ? = m), the ?rst logarithm generated by the ultrasoft anomalous dimension corresponds to a ln(E/m), while the ?rst logarithm generated by the soft anomalous dimension corresponds to a ln(|k|/m). For the velocity renormalization group, the total anomalous dimension is simply γS + 2γU : ν ? (T ) 1 8 Vk (ν ) = ? β0 (7CA ? Cd ) [αs (mν )]3 ? CA (CA + Cd ) [αs (mν )]3 (32) ?ν 8π 3π 4 + CA (CA + Cd ) αs (mν 2 )[α(mν )]2 , π ? (1) 1 16 24 ν Vk (ν ) = ? β0 C1 [αs (mν )]3 + CA C1 [αs (mν )]3 ? CA C1 αs (mν 2 )[αs (mν )]2 . ?ν 2π π π

Note that no other 1/v potentials are generated for ν < 1 by operator mixing. Integrating Eq. (32) using the one loop β -function for αs and the one loop boundary condition in Eq. (14) gives Vk (ν ) = (7CA ? Cd ) 2 (7CA ? Cd ) 8 CA (CA + Cd ) 2 (z 2 ? 1) αs (m) (33) αs (m) + + 8 8 3β0 8 C A (C A + C d ) 2 + z ? 1 ? 2 ln(w ) αs (m) , β0 48CA C1 2 C1 2 C1 16 CA C1 (1) 2 (z 2 ? 1) αs (m) ? Vk (ν ) = αs (m) + ? αs (m) z ? 1 ? 2 ln(w ) , 2 2 β0 β0

(T )

where αs (mν ) , z= αs (m)

2 and C1 = CA CF /2 ? CF gives

αs (mν 2 ) 1 w= = . αs (mν ) 2?z

(34)

Projecting onto the color singlet channel, V (s) = V (1) ? CF V (T ) , and setting Cd = 8CF ? 3CA

2 2 CF 8 C A C F (C A + 2 C F ) CF 2 2 (z 2 ? 1) αs (m) ? CF CA αs (m) + ? CF CA ? 2 2 3β0 8 C A C F (C A + 2 C F ) 2 ? z ? 1 ? 2 ln(w ) αs (m) . (35) β0 (o) (1) (T )

Vk (ν ) =

(s)

The projection onto the color octet channel is Vk = Vk + (CA /2 ? CF )Vk . Logarithmic corrections to the color singlet V (?1) potential were also considered by Brambilla et al. [15] using pNRQCD, but were not resummed. Brambilla et al. have

2 Vk (ν ) = ?CF CA αs (r ) ? (s)

4 C A C F (C A + 2 C F ) αs (?)αs (r )2 ln(?r ) . 3π

(36)

To compare this expression to ours: α(r ) → α(mν ), r → 1/(mν ) and ? = ?U = mν 2 since r corresponds to the soft scale and ? corresponds to the ultrasoft scale. Expanding Eq. (36) in αs (m) gives 19

2 Vk (ν ) = ?CF CA αs (m) +

(s)

β0 CF CA 3 αs (m) ln[1/(mr )] π 4 C A C F (C A + 2 C F ) 3 αs (m) ln(?r ) + . . . . ? 3π

(37)

To compare this to our result we expand the resummed logarithms in Eq. (35): Vk (ν ) =

(s) 2 2 β0 CF CA 3 β0 CF CF 2 3 ? CF CA αs (m) + αs (m) ln(ν ) ? αs (m) ln(ν ) 2 π 2π 4 C A C F (C A + 2 C F ) ? αs (m)3 ln(ν ) + . . . . 3π

(38)

In Eq. (38), the ?rst and second ln(ν ) terms are entirely from the soft anomalous dimension in Eq. (31), while the third ln(ν ) term is from a combination of the ultrasoft and soft anomalous dimensions. The ?rst ln(ν ) term in Eq. (38) agrees with the ln[1/(mr )] = ln(ν ) term in Eq. (37), and the third ln(ν ) term in Eq. (38) agrees with the ln(?r ) = ln(ν ) term in Eq. (37). The second term in Eq. (38) does not appear in Brambilla et al.’s expression in Eq. (37). This is because it depends on whether an on-shell or o?-shell potential is used for the matching and running7 . We have used an on-shell potential, while Ref. [15] uses o?-shell Coulomb gauge which includes a V?2 = ?4παs (r ) potential as de?ned in Eq. (B1) of Appendix B. The second logarithm in Eq. (38) should appear from the coe?cient of this potential. Transforming Brambilla et al.’s V?2 potential to a Vk potential using Eq. (B4) gives Vk (ν ) = =

(s) 2 CF αs (r )2 2 2 2 CF β0 CF 2 3 αs (m) ? αs (m) ln[1/(mr )] + . . . . 2 2π (T ) (s) (T )

(39)

The term with a ln[1/(mr )] = ln(ν ) agrees with the second ln(ν ) term in Eq. (38). The sum of terms without logarithms in Eqs. (37) and (39) also agrees with Eq. (38). Note that the next term in the series in Eq. (38) does not give agreement with Eqs. (37) and (39) since Brambilla et al. did not attempt to systematically sum all the logarithms. To see the e?ect of the running on the value of the V (?1) potential, consider the case of top quark production near threshold. Using αs (mt ) = 0.108 and Eq. (35), the one loop matching value is:

issue of on-shell versus o?-shell potential was discussed in Ref. [23], and in the context of the leading log summation is discussed further in Appendix B. 20

7 The

0.15

Vk (ν)

0.1

0.05

Vk 0 Vk -0.05 0 0.2

(?1)

(o)

(s)

0.4

0.6

0.8

1

ν

FIG. 6. Values for the NLL running V potential for top quarks and nf = 5 massless ?avors. The solid and dashed lines are the color singlet and octet coe?cients for the π 2 /(m|k|) potential. The solid vertical line marks the Coulombic regime where αs (mν ) = ν .

Vk (1) = ?0.0362 .

(s)

(40)

For a Coulombic system we determine the velocity v by solving αs (mv ) = v . Using mt = 175 GeV and the one loop running of αs (?) with nf = 5 gives v = 0.145. The NLL color singlet and octet coe?cients for the 1/|k| potential are plotted in Fig. 6. At ν = v the running coupling is Vk (v ) = ?0.0027 ,

(s)

(41)

which is a substantial change from Eq. (40). In comparison, the terms shown in Eq. (38) where the combination αs ln(v ) is treated perturbatively give Vk (v ) = ?0.0313. Thus, the summation of logarithms for the 1/|k| potential is quite important; it decreases the coe?cient by an order of magnitude. Using the unexpanded results in Eqs. (36) and (39) gives Vk (v ) = 0.0201, so our resummed result is also quite di?erent from the ?xed order result in Ref. [15].

(s) (s)

21

? production current B. The NLL tt

In terms of the running color singlet potentials the anomalous dimension for the production current in Eq. (4) is [14]:

(s) ? Vc (ν ) γ c 1 (ν ) = ν ln[c1 (ν )] = ? ?ν 16π 2 (s) V (ν ) Vc (ν ) (s) (s) (s) + V2 (ν ) + Vr . (ν ) + S2 Vs (ν ) + k 4 2 (42) (s)

For the vector production current in Eq. (4) only spin-1 states are produced, and we can set S2 = S (S + 1) = 2. However, our analysis also applies to the scalar production current c(ν )

p

ψp ? χ? ?p ,

(43)

? [31]. Therefore, we will keep the which, for example, contributes to the process γγ → tt factors of S2 explicit in our results. The boundary condition is given by the matching condition at ν = 1 (? = m) which is known to two loops [21]. For the NLL approximation only the one loop matching condition should be used. For the vector current c1 (1) = 1 ? 2CF αs (m) . π (44)

Integrating Eq. (42) with the running potentials in Appendix A, Eq. (A1) and in Eq. (33) we ?nd ln 1 c 1 (ν ) = a1 παs (m) ? 1 + a2 παs (m)(1 ? z ) + a3 παs (m) ln(z ) c1 (1) z +a4 παs (m) 1 ? z 1?13CA /(6β0 ) + a5 παs (m) 1 ? z 1?2CA /β0 π2 1 2 1 2w +a6 παs (m) ? Li2 ? ln (2) ? ln(w ) ln 12 2 2w ? 1 2w w 1 +a7 παs (m) ln(w ) ? ln(2w ? 1) , 2w ? 1 2

(45)

where z = αs (mν )/αs (m) and w = αs (mν 2 )/αs (mν ). The coe?cients ai in Eq. (45) are a1 = a2 = 32CA CF (CA + 2CF ) , 2 3β0

2 2 2 2 ?CF [3β0 (26CA + 19CA CF ? 32CF ) + CA (208CA + 597CA CF + 716CF )] , 2 78 β0 CA ?CF 2 2CF (66β0 ? 179CA )(β0 ? 2CA ) a3 = 2 3 β0 (6β0 ? 13CA )(β0 ? 2CA )

22

2 2 ?CA CF 6(49 ? 3S2 )β0 ? (1126 ? 39S2 )β0 CA + 1067CA 2 ?24CA (6β0 ? 13CA )(β0 ? 2CA ) , 2 ?24CF (3β0 ? 11CA )(5CA + 8CF ) , 13 CA (6β0 ? 13CA )2 2 ?16 CF (C A + 2 C F ) , 2 3 β0 2 CF (4S2 ? 3)β0 + (15 ? 14S2 )CA

a4 = a6 =

a5 =

6(β0 ? 2CA )2

, (46)

a7 =

16CA CF (CA + 2CF ) . 2 β0

3 A further check on our result can be made by comparing it to the αs ln2 (αs ) corrections ? cross section depends on calculated by Kniehl and Penin in Ref. [22]. Near threshold the tt

the product [32]:

C σ ∝ |c1 |2 GC (0, 0, E ) |ψn (0)|2 ,

(47)

where ψ C is the leading order Coulomb wavefunction, and GC is the Coulomb Green’s function. In the approach used in Ref. [22], GC embodies corrections to the wavefunction at

C the origin, |ψ (0)|2 ≡ |ψn (0)|2 [1 + ?ψ 2 (0)], and includes the large logarithms. They calculate 2 3 the αs ln(αs ) and αs ln2 (αs ) terms and ?nd: 2 ?ψ 2 (0) = ?CF αs ln(αs )

2 2 ? S2 CF + CA 3 2 2 7 3 2 41 CF 3 2 ? S2 CF CA + CA , ? αs ln (αs ) CF + π 2 12 12 3

(48)

for the terms not involving β0 . In our approach the large logarithms in the cross section all appear in the running coe?cient c1 (ν ), so we expect that the logarithms of Kniehl and Penin will be reproduced by c1 (ν ) ′ ?ψ (0) = ? 1 = 2 ln(αs ) γc1(1) + ln2 (αs ) γc (1) + 2[γc1(1)]2 + . . . , 1 c1 (1)

2 2

(49)

where we have expanded to second order in ln(ν ) = ln(αs ). The [γc1(1)]2 term does not

3 contribute at order αs ln2 αs , and can be dropped. The remaining terms in Eq. (49) give: 2 ?ψ 2 (0) = ?CF αs ln(αs )

2 2 ? S2 CF + CA 3 2 2 β0 7 3 2 41 CF 3 2 αs ln (αs ) CF + ? S2 CF CA + CA ? ? π 2 12 12 3 2

(50) 2 2 ? S2 CF + CA 3 ,

which agrees exactly with the result from Ref. [22] in Eq. (48) after setting β0 = 0. Thus, we have shown that the logarithms of Kniehl and Penin can indeed be associated with 23

1

c1(ν)

0.95

NLL

0.9

NLO

0.85 0 0.2 0.4 0.6

NNLO

0.8

1

ν

? production current coupling c1 (ν ) for nf = 5 massless ?avors. At FIG. 7. Values for the tt LO and LL c1 = 1. The large and small dashed lines show the value of c1 at NLO and NNLO [21] respectively. The solid line shows the running value at NLL order given in Eq. (45). The dotted line shows the result of promoting the coupling in the NLO result to a running coupling (the approximation used in Ref. [33]). The solid vertical line marks the Coulombic regime where αs (mν ) = ν .

4 renormalization group logarithms. Expanding Eq. (45) to higher orders gives the αs ln3 (αs ), 5 αs ln4 (αs ), etc. terms.

For QCD with nf = 5, the coe?cients in Eq. (46) are a1 = 4.113 , a2 = ?2.173 , a3 = 4.308 ? 0.417 S2 , a7 = 6.170 . a4 = 5.731 , (51)

a5 = 2.347 ? 1.209 S2 ,

a6 = ?0.914 ,

The running coe?cient c1 (ν ) is shown in Fig. 7 for S2 = 2. For comparison we have also shown by a dotted line the value of the running coe?cient obtained in Ref. [33] by an approach based on simply taking αs → αs (mν ) to approximate the NLL value for the coupling. This approximation misses many of the αs ln(v ) terms, and does not provide a good estimate of the NLL result, as seen in Fig. 7. Some of the more important logarithms in our NLL result include the large ln(mν 2 /m) terms that enter through the mixing generated by ultrasoft gluon diagrams in the potential. We have also shown the NNLO value for c1 in Fig. 7. As pointed out in Ref. [21] the 24

NNLO value of c1 (1) is fairly large. From Fig. 7 we see that summing the logarithms reduced the size of the NLO matching correction by a factor of two. It would be interesting to see if the running induced at NNLL continues to improve the convergence of the expansion. A consistent calculation at this order requires the three-loop anomalous dimension of c1 , as well as one loop running of the v 2 coe?cients c2 and c3 . This computation appears quite involved since running of the current at this order will likely depend on the running of higher order terms in the potential. ? cross section predictions at NNLO using e?ective ?eld Several groups have analyzed the tt theory techniques [33–37,31]. It should be straightforward to incorporate the renormalization group improved current and potentials into their analysis by simply choosing a value of ν appropriate to the threshold region. The value of ν only needs to be of order the velocities in this region for the large logarithms to be minimized. Additional logarithms that appear in evaluating matrix elements with the potential will not involve large ratios of scales since they are of the form ln(E/?U ) and ln(|k|/?S ) where ?U = mν 2 and ?S = mν . In a more precise analysis one might wish to use αs (mv )CF = v to determine the value ν to use. We would like to thank I. Rothstein and J. Soto for discussions. This work was supported in part by the Department of Energy under grant DOE-FG03-97ER40546, and by the National Science Foundation under NYI award PHY-9457911.

APPENDIX A: LL values for the order v ?2 and v 0 potentials

The leading log values for the coe?cients of the V (?2) and V (0) potentials are [19]:

(T ) Vc (ν ) = 4παs (m) z , (1) Vc (ν ) = 0 , (T ) Vr (ν ) = 4π αs (m)z ? (T )

(A1) 32πCA 64πCA αs (m) 1 ? z ? αs (m) ln w , 3β0 3β0

V2 (ν ) =

αs (m) z ? 1 39β0 CA 8π (3β0 ? 11CA )(5CA + 8CF )αs (m) (1?13CA /(6β0 )) z ?1 + 13CA (6β0 ? 13CA ) π (β0 ? 5CA )αs (m) (1?2CA /β0 ) 8π (4CF + Cd ? 3CA ) + z ?1 ? αs (m) ln w , (β0 ? 2CA ) 3β0 32πC1 28πC1 (1) αs (m) 1 ? z + αs (m) ln w , V2 (ν ) = 3β0 3β0 25

π CA (352CF + 91Cd ? 144CA ) ? 3β0 (33CA + 32CF )

1 1 2παs (m) CA + (2β0 ? 7CA ) z (1?2CA /β0 ) + π αs (m) , (2CA ? β0 ) 3 Nc 2 (Nc ? 1) (1) π αs (m) , Vs (ν ) = 2 2Nc παs (m) (1?2CA /β0 ) (T ) Vt (ν ) = ? z , 3 (T ) VΛ (ν ) = 2παs (m) z ? 4 z (1?CA /β0 ) ,

(T ) Vs (ν ) =

where z = αs (mν )/α(m), w = αs (mν 2 )/α(mν ), and we have included the Nc dependent terms that come from matching the tree level annihilation diagrams. In the color singlet channel, Vt (ν ) and VΛ (ν ) were ?rst calculated in Ref. [18] and agree with Eq. (A1).

APPENDIX B: POTENTIAL OPERATORS THAT VANISH ON-SHELL

It is interesting to consider how the soft and ultrasoft anomalous dimensions for V (?1) are a?ected when operators that vanish on-shell are included in the potential Lagrangian, Lp . These new operators can have non-trivial anomalous dimensions. In this Appendix we consider two examples of how including these operators a?ects intermediate results, but in the end yield the same result as the on-shell potential for observables. Equivalently, it is shown that running the Lagrangian with the new operators from ν = 1 to ν = v and then removing them by ?eld rede?nitions or operator identities reproduces the on-shell running value of V (?1) .

0 ′ ′ ? 0 ? 0 Consider the scattering Q(p0 1 , p) + Q(p2 , ?p) → Q(p3 , p ) + Q(p4 , ?p ). As our ?rst

example, consider including in the v 0 potential in Eq. (10) terms of the form: (p 0 ? p 0 )2 (T ) (1) ? A ) + V?1 V (0) = V?1 (T A ? T (1 ? 1) 3 4 1 k

′2 2 2 (T ) ? A ) + V (1) (1 ? 1) (p ? p ) . + V?2 (T A ? T ?2 4m2 k4

(B1)

We will refer to this potential as an o?-shell potential, since on-shell it vanishes by energy

0 ′2 conservation, where p0 = p2 . De?ne V? 3 = p1 , p (T,1)

= V?1

(T,1)

+ V?2 . In Ref. [23] it was

(T,1)

shown that there is an operator identity whereby the time ordered product of a Vc and a V? potential gives Vk potentials: Vc V? 2 + V? 2 Vc iV (T ) V? = c 32mk

(T ) (T ) ?AT ? B + iVc V? T A ? T ?A + . . . , T T ?T 32mk (B2) A B (1)

26

where the ellipses denote additional terms which vanish on-shell. The identity in Eq. (B2) allows us to remove the potential in Eq. (B1) at an arbitrary velocity scale ν in favor of a purely on-shell potential. Transforming V? Vk (ν ) → Vk (ν ) +

(T ) (T ) (T,1)

(ν ) → 0 gives

1 1 (1) (T ) (T ) Vc (ν ) ? V? (ν ) + (CA + Cd )V? (ν ) , 2 32π 4 1 (T ) (1) (1) V (T ) (ν ) C1 V? (ν ) . Vk (ν ) → Vk (ν ) ? 32π 2 c

(1) (T )

(B3)

In a situation where V? (ν ) = 0 transforming V? (ν ) → 0 induces a color singlet 1/|k| potential of the form Vk (ν ) → Vk (ν ) ?

(s) (s) 2 CF (T ) V (T ) (ν )V? (ν ) . 32π 2 c

(B4)

(Transformations between order 1/v and v 0 potentials were also considered in Refs. [32,35,38].) To make the implications of Eq. (B3) more clear, we will consider an example and show that including the V? ν = 1 are V?

(T ) (T,1)

potential will not e?ect predictions for observables when running

(1)

below m. Consider matching o?shell in Feynman gauge where the matching coe?cients at = 4παs (m) and V? = 0, and the one loop anomalous dimensions for the ? (T ) V = ?2β0 αs (mν )2 , ?ν ? ? (1) ν V? = 0 . ?ν potentials in Eq. (B1) are [23]: ν

(B5)

This anomalous dimension has contributions from the one loop graphs with two soft gluons, ghosts or quarks where: the two factors of (p′2 ? p2 ) are from the soft vertices, or these factors are from two insertions on the soft propagators, or where one factor is from the propagator and one from the vertex (for the ghost loop). The solution of Eq. (B5) is V? (ν ) = 4παs (mν ) and V? (ν ) = 0. The one loop counterterm which generates this running a?ects our soft anomalous dimension computation since now there are counterterms of the form (p′ 2 ? p2 )2 . m2 (p′ ? p)4 ? (B6)

(T ) (1)

These counterterm give rise to one loop diagrams which exactly cancel the divergences in Eq. (26) for the two loop graph in Fig. 3a. Recalling that the one loop matching values for

27

the 1/|k| potentials are also di?erent [23], we ?nd that the running Vk Eq. (33) become Vk (ν ) =

(T,1)

(ν ) coe?cients in

(3CA ? Cd ) 2 (3CA ? Cd ) 8 CA (CA + Cd ) 2 (z 2 ? 1) αs (m) (B7) αs (m) + + 4 4 3β0 8 C A (C A + C d ) 2 + z ? 1 ? 2 ln(w ) αs (m) , β0 16 CA C1 48CA C1 2 (1) 2 2 Vk (ν ) = C1 αs (m) + C1 ? (z 2 ? 1) αs (m) ? αs (m) z ? 1 ? 2 ln(w ) , β0 β0

(T ) (T )

This Feynman gauge o?-shell potential is consistent with the transformation in Eq. (B3) which transforms the o?-shell case, V? V?

(T,1)

= 4παs (mν ) and Eq. (B7), into the on-shell case,

= 0 and Eq. (33). The comparison in section IV A with Ref. [15] shows that our

on-shell analysis is also consistent with an o?-shell Coulomb gauge potential. With the o?-shell potential in Eq. (B1) there are two new graphs which contribute to the anomalous dimension for the production current: Vc V? 2 and the anomalous dimension is therefore ν

(s) ? ?Vc (ν ) ln[c1 (ν )] = ?ν 16π 2 (s) (s) V? Vc (ν ) V (ν ) Vc (s) (s) (s) + V2 (ν ) + Vr ? , (ν ) + S2 Vs (ν ) + k 4 2 64π 2 (B9) (T ) (s) (s)

V? 2

Vc , (B8)

where V? (ν ) = V? (ν ) ? CF V? (ν ). Since the last two terms in Eq. (B9) are invariant under the transformation in Eq. (B4) the o?-shell potential gives the same prediction for the running of the production current. In calculating observables the operator identity in

(T ) Eq. (B2) guarantees that the time ordered product of the running V? and Vc produces (T )

(s)

(1)

the same e?ect as the soft contribution to the running of the on-shell Vk order free equations of motion: Leom = ?

p,p′

(T )

in Eq. (26).

As our second example, consider including an operator which would vanish by the lowest VF p2 ? A ?A i? ? ψp χ? T ψ ′ 0 ?p′ T χ?p + χ ? ψ . (p′ ? p)2 p 2m

(B10)

The only feature of the operator in Eq. (B10) that is di?erent from typical operators that vanish by the equations of motion (for example, in HQET [27]) is its non-local nature relative to the scales p ? p′ ? mv . At one loop there are ultrasoft gluon graphs which mix into the operator in Eq. (B10), for instance from the diagrams: 28

a)

b) Vc

×

. (B11)

In the ?rst graph the vertex is the ?rst term in Eq. (16) and the ultrasoft gluon is A, while in the second diagram the cross is a insertion of the ultrasoft ?2 /m operator in Eq. (7) and the gluon is an A0 . In Feynman gauge both graphs produce a divergence of the form (E ? p2 /m) , ? (p′ ? p)2 (B12)

which vanishes by the equations of motion, but o?-shell renormalizes the coe?cient of the operator in Eq. (B10). To see how this e?ects the calculation of our ultrasoft anomalous dimension, consider Coulomb gauge, where only Eq. (B11a) is non-zero. In this case there is a one loop counterterm diagram which exactly cancels the divergence in Fig. (28b). After running down to the low scale the value of Vk

(T,1)

(ν ) are di?erent, but our potential also

includes the operator in Eq. (B10) with coe?cient VF (ν ). If we wish to remove the operator in Eq. (B10) we can do so with a ?eld rede?nition

? ? ψp → ψp + p′′

(p′

VF ?A ψ ? ′′ T A χ? ?p′′ T χ?p , ? p )2 p

(B13)

? which induces a term from the ψp [i?0 ? p2 /(2m)]ψp Lagrangian which cancels Eq. (B10).

This ?eld rede?nition also gives other new contributions. For us the important point is that the Coulomb potential induces a six-quark operator of the form: ?

p,p′ p′′ ? ? ? ψp ′′ χ?p′′ χ?p′ ψp χ?p′ χ?p

(p′′

VF Vc . ? p′ )2 (p′ ? p)2

(B14)

(The contraction of color indices and factors of T A have been suppressed.) Usually a six quark operator could not possibly e?ect the running of a four quark operator such as the 1/|k| potential. However, because of the momentum dependence in the denominator of Eq. (B14) it induces a non-zero tadpole diagram where the ?elds χ?p′ and χ? ?p′ are contracted. This tadpole graph produces a 1/|k| and makes up for the running in Vk that was removed when the contribution from Eq. (28b) was canceled by a VF counterterm.

29

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