Quantized field description of rotor frequency-driven dipolar recoupling

G. J. Boender, S. Vega, and H. J. M. de Groot

Citation: J. Chem. Phys. 112, 1096 (2000); doi: 10.1063/1.480664 View online: http://dx.doi.org/10.1063/1.480664

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Quantized field description of rotor frequency-driven dipolar recoupling

G. J. Boendera)

Leiden Institute of Chemistry, Leiden University 2300 RA Leiden, The Netherlands

and Department of Chemical Physics, Weizmann Institute of Science, 76100 Rehovot, Israel S. Vega

Department of Chemical Physics, Weizmann Institute of Science, 76100 Rehovot, Israel H. J. M. de Groot

Leiden Institute of Chemistry, Leiden University 2300 RA Leiden, The Netherlands 共Received 25 August 1999; accepted 22 October 1999兲

A formalized many-particle nonrelativistic classical quantized field interpretation of magic angle spinning 共MAS兲 nuclear magnetic resonance 共NMR兲 radio frequency-driven dipolar recoupling 共RFDR兲 is presented. A distinction is made between the MAS spin Hamiltonian and the associated quantized field Hamiltonian. The interactions for a multispin system under MAS conditions are described in the rotor angle frame using quantum rotor dynamics. In this quasiclassical theoretical framework, the chemical shift, the dipolar interaction, and radio frequency terms of the Hamiltonian are derived. The effect of a generalized RFDR train of ␲ pulses on a coupled spin system is evaluated by creating a quantized field average dipolar-Hamiltonian formalism in the interaction frame of the chemical shift and the sample spinning. This derivation shows the analogy between the Hamiltonian in the quantized field and the normal rotating frame representation. The magnitude of this Hamiltonian peaks around the rotational resonance conditions and has a width depending on the number of rotor periods between the␲pulses. Its interaction strength can be very significant at the n⫽0 condition, when the chemical shift anisotropies of the interacting spins are of the order of their isotropic chemical shift differences. © 2000 American Institute of Physics.

关S0021-9606共00兲03203-7兴

I. INTRODUCTION

Magic angle spinning 共MAS兲 nuclear magnetic reso-nance 共NMR兲 correlation spectroscopy in conjunction with multispin isotope enrichment has been established recently as a novel concept for refinement of electronic and spatial structure in solids.1,2This development was triggered by the discovery of broadbanded pulse sequences for homonuclear dipolar recoupling.3–11 In principle, MAS averages dipolar interactions.12,13Using dipolar recoupling techniques, homo-nuclear and heterohomo-nuclear dipolar correlation spectroscopy can be performed and the NMR response of moderately sized multispin clusters can be assigned.14,15In addition, since the dipolar interaction is strongly distance dependent, dipolar correlation spectroscopy can be used for de novo structure determination on an atomic scale of multispin labeled systems.1,2In this article we present a formal quantized field interpretation of the seminal radio frequency driven dipolar recoupling 共RFDR兲. The technique was originally proposed for one refocusing␲-pulse per single rotor period.5RFDR is straightforward to implement and robust, and can be applied readily in high and ultra high fields. It has already been uti-lized for assignment and structure refinement of moderately sized uniformly labeled biological aggregates.16

It has been shown that the effect of MAS on a nuclear spin system in a solid can be described in terms of a quan-tized rotor field, leading to a physical interpretation of the

Floquet description of MAS.17,18 This makes it possible to disentangle the influence of the radiation field and the MAS rotation, leading to the construction of a Floquet Hamiltonian for the MAS NMR from first principles. Here it will be shown that the quantized field description can be combined with the average Hamiltonian approach in order to provide us with a quasiclassical description of RFDR experiments with a variable number of rotor periods between the

␲-pulses.19

The formal description of the RFDR experiment starts with a brief summary of the quantum rotor dynamics in the next section. The interaction of the quantized rotor field with the nuclear spin is discussed in Sec. III. The chemical shield-ing of the magnetic field is calculated in this section and the term in the quantized field Hamiltonian describing the dipo-lar interaction is put forward. In Sec. IV, the RF pulse is included in the quantized field framework. Using the meth-odology discussed in Secs. II–IV, we analyze in Sec. V a generalized RFDR sequence. In Sec. VI the polarization transfer driven by the dipolar recoupling sequence is dis-cussed and in Sec. VII the main conclusions are given. In the appendix the transformation properties for the quantized field operators constituting the spin-pair dipolar term in the multi-spin Hamiltonian are evaluated.

II. QUANTUM ROTOR DYNAMICS

MAS NMR spectroscopy is generally described with the help of a spin Hamiltonian, in which the effect of the sample

a兲_{Present address: ID-DLO, P.O. Box 65, 8200 AB Lelystad, The}

Nether-lands.

1096

rotations on the nuclear spins is taken into account by a set of periodically time dependent coefficients. The spin Hamil-tonian of a single crystallite in the rotating frame can there-fore be expanded in a Fourier series according to20

HˆS共t兲⫽HˆS0⫹

兺

p⫽1 2 HˆS pexp共ip共␸0⫹␻rt兲兲⫹HˆS p † ⫻exp共⫺ip共␸0⫹␻rt兲兲, 共1兲

in which␻ris the spinning speed andHˆS pthe Fourier

com-ponents of the Hamiltonian. These comcom-ponents differ from crystallite to crystallite in the sample, while␸0 is a constant

initial phase that may vary between experiments.

In the quantized field description the concept of a nuclear spin Hamiltonian is extended with quantum rotor dynamics.17 The interaction of the spins with the environ-ment due to the MAS rotation is included in the Hamiltonian, by using a set of quantum rotor dynamics operators Lˆz⬘, Fˆp,

and Fˆ_p†, to replace the phenomenological time-dependent phase of the rotation ␸₀⫹␻_rt in Eq.共1兲.

Recently, it was shown that rotor field quantization of-fers a self-consistent framework to describe the evolution of the spin system with conservation of energy.17The total or-bital angular momentum l of a forced rotation of a rotor with eigenstates兩lm

典

in the quasiclassical limit defined by l→⬁ and l⫽m, corresponds with the number of boson quasipar-ticles. The associated rotor field is a vector field that can be constructed using boson annihilation and creation operators

aˆ兩l

典

⫽l1/2兩l⫺1

典

,

共2兲 aˆ†兩l

典

⫽共l⫹1兲1/2兩l⫹1

典

,

where

Lˆz⬘⫽aˆ†aˆ 共3兲

measures the orbital angular momentum. The energy of the rotor is ␻rl, which is very large on the energy scale of the

nuclear spin system.

It was shown that a complete description of the MAS for a nuclear magnetic moment in a solid can be obtained within a single set of reduced angular momentum states 兩n

典

. By taking l⫽n¯⫹n, with n the variation of the angular momen-tum around a large average value n¯ , the orbital angular mo-mentum states can be renumbered according to17

兩n¯⫹n

典

→兩n

典

. 共4兲

To provide a description of the quasiclassical limit, a phase operator␸ˆ

⬘

is introduced that represents a continuous coor-dinate␸

⬘

with

exp共i␸ˆ

⬘

_兲⫽ aˆ †

冑

¯n. 共5兲

The relation between the phase operator and the angular mo-mentum operator Lˆz⬘, is the canonical commutation relation

according to

关␸ˆ

⬘

,Lˆz⬘兴⫽i, 共6兲

and the z axis is the axis of rotation.

MAS is a rotation with a single normal frequency mode

␻r. The interaction between the spin system and the sample

rotation can be interpreted in terms of p-quantum interac-tions with the single mode rotor field with a frequency␻r.

For a p-quantum transition, a Fourier operator is defined by

Fˆ_p⫽exp共ip␸ˆ

⬘

_兲. 共7兲

According to Eq.共5兲 the Fpoperators are multiquantum

lad-der operators with Fˆp兩n

典

⫽兩n⫹p

典

and they can be

inter-preted as a repeated application of single quantum raising and lowering operators, since Fˆp⫹q⫽FˆpFˆq.

17

The commutator关Lˆz⬘,Fˆp兴⫽pFˆp implies that

exp共i␻rtLˆz⬘兲Fˆpexp共⫺i␻rtLˆz⬘兲

⫽1ˆ⫹i␻rt关Lˆz⬘,Fˆp兴⫹ 共i␻rt兲 2 2! 关Lˆz⬘,关Lˆz⬘,F ˆ p兴兴⫹¯ ⫽exp共ip␻rt兲Fˆp. 共8兲

In the quasiclassical limit, quantization of the rotor field is therefore equivalent with the introduction of a phase operator

␸ˆ

⬘

in the rotor angle frame according to Eq.共5兲. A quantized field extension of the spin Hamiltonian in Eq. 共1兲 is then

HˆQ共t兲⫽HˆS0⫹

兺

p⫽1 2 HˆS pexp共ip共␸ˆ

⬘

⫹␻rt兲兲⫹HˆS p † ⫻exp共⫺ip共␸ˆ

⬘

⫹␻_rt兲兲. 共9兲

It includes two independent degrees of freedom, ␸ˆ

⬘

and t, which contrasts with the single time degree of freedom that is used to generate the time-dependence in the spin Hamil-tonian HˆS(t) in Eq. 共1兲.17 The ␸ˆ

⬘

degree of freedom is

es-sential, to account for the infinitesimal phase variations due to the quantum rotor dynamics, in which the rotor is de-scribed as a two dimensional harmonic oscillator or a rigid rotor.21,22

Using the relations共7兲 and 共8兲, it is possible to rewrite the Eq.共9兲, yielding

HˆQ共t兲⫽exp共i␻rtLˆz⬘兲

冉

HˆS0⫹

兺

p⫽1 2 HˆS pFˆp⫹HˆS p † _F p †

冊

⫻exp共⫺i␻rtLˆz⬘兲. 共10兲

A time-independent Hamiltonian HˆQ can be obtained by a

transformation to the spatial rotating frame, defined by exp(⫺i␻rtLˆz⬘):

17

HˆQ⫽Hˆn⫹Hˆi⫹Hˆr 共11兲

consisting of a term associated with the sample rotation

Hˆr⫽␻rLˆz⬘, 共12兲

a pure nuclear spin Hamiltonian term independent of F_p

Hˆn⫽HˆS0, 共13兲

and an interaction term depending on Fp and Fp

† Hˆi⫽

兺

p⫽1 2 HˆS pFˆp⫹HˆS p † Fˆ†_p, 共14兲

which describes the effect of the rotor dynamics on the spin interactions. SinceHˆ_Qis time independent its unitary evolu-tion operator is

Uˆ 共t兲⫽exp共⫺iHˆQt兲. 共15兲

The effect of the phenomenological time dependence on the spins is included by means of the time-independent or-bital angular momentum ladder operators Fˆp,Fˆp

†_{. These}

have a physical basis and have been identified as the Fourier operators in the Floquet description of MAS NMR.17 The

HˆQ Hamiltonian operates in the product space spanned by

the spin states and the 共reduced兲 angular momentum states. The commutation relation between the Fourier operators and the orbital angular momentum operator 关Lˆz⬘,Fˆp兴⫽pFˆp

al-lows for energy exchange between the rotor and the spin system. In addition, it provides a route to coherent superpo-sitions of states involving the quantum rotor dynamics, since in general关Hˆ_r,Hˆ_i兴⫽0.

III. THE INTERACTION HAMILTONIAN

The Fourier components of the spin Hamiltonian 共1兲, containing chemical shift and dipolar interactions, can be expressed in terms of contractions between Aˆk, the

irreduc-ible tensor operators of rank k in real space, and Tˆk, the

irreducible tensor operators of rank k in spin space.23,24In the spin rotating frame only the part of the interactions that com-mute with the Zeeman Hamiltonian have to be taken into account. An interaction term of the spin-Hamiltonian in the spin rotating frame can therefore be written as

HˆS共t兲⫽

兺

k

Ak0共t兲Tˆk0. 共16兲

The time dependent spatial part can be expanded in a Fourier series according to17 Ak0共t兲⫽

兺

p⫽⫺k k exp共ip共␻rt⫹␸0兲兲Vp0 k , 共17兲 with V_p0k ⫽

兺

s⫽⫺k k

兺

r⫽⫺k k A_kr

⵮

D_rsk共␣c,␤c,␥c兲Ds p k _共␣ r,␤r,␥r兲 ⫻Dp0 k

冉

0,␤m, ␲ 4

冊

. 共18兲

The A_kr

⵮

coefficients are the elements of the spatial tensor describing the coefficients of the interaction in the principal axis system共PAS兲. In Eq. 共18兲 three sets of Euler angles of the Wigner coefficients D_{i j}k(␣,␤,␥) describe the transforma-tion from the PAS to a crystal frame (␣c,␤c,␥c), from this

crystal frame to the rotor angle frame (␣r,␤r,␥r), and

fi-nally from the rotor angle frame to the laboratory frame (0,␤m,␲/4).

23

The tensor operators in spin space can be written as Tˆk0⫽W00

k _Iˆ

0 共19兲

in which W₀₀k are some coefficients and Iˆ₀ spin operators commuting with Iˆz. The quantized field Hamiltonian

be-comes then HˆQ共t兲⫽Z00 k_Iˆ 0⫹

兺

p⫽1 k

Z_p0k Iˆ₀exp共ip共␸ˆ

⬘

⫹␻_rt兲 ⫹Zp0

k*_Iˆ

0exp共⫺ip共␸ˆ

⬘

⫹␻rt兲 共20兲

with

Zk_p0⫽V_p0k W₀₀k 共21兲

and the fact that the Hamiltonian is Hermitian requires that Z_⫺p0⫽Z_p0* . After the transformation to the spatial rotating frame the interaction Hamiltonian in Eq.共14兲 yields

Hi⫽

兺

p_⫽1 k 共Zp0 k Fˆp⫹Zp0 k*_Fˆ p †_兲Iˆ 0. 共22兲

Here we have used again the Fourier operators to include the quantum rotor dynamics, according to Eq.共7兲.

For a dipolar coupled spin system of like spins under MAS, the Hamiltonian consists of a chemical shift term and a dipolar term. Thus the nuclear spin Hamiltonian and the interaction Hamiltonian can be written as

Hˆn⫽Hˆn CS_⫹Hˆ n D , 共23兲 Hˆi⫽Hˆi CS_⫹Hˆ i D_.

With the external magnetic field along the z axis, the spin tensor operators in the truncated isotropic chemical shift (k⫽0) and chemical shift anisotropy 共CSA兲 (k⫽2) Hamil-tonian in Eq. 共16兲 are for a spin i23

Tˆ₀₀i ⫽⫺ 1

冑

3 ␥H0Iˆz i , 共24兲 Tˆ₂₀i ⫽

冑

2 3␥H0Iˆz i .

The spatial isotropic chemical shift tensor is of rank 0 with a single element A₀₀

⵮

⫽A¯i. The CSA interaction is a real sym-metric tensor interaction␴ of rank 2 and the three elements that characterize this tensor in its principal axis system are for a spin i A₂₀

⵮

⫽

冑

3 2␦ i_, 共25兲 A₂

⵮

_⫾2⫽1 2 ␩␦ i_, with A¯i⫽␴¯i⫽冑_1/3(␴ xx i _⫹␴ y y i _⫹␴ zz i

) the isotropic and ␦i ⫽1/3(␴zz

i _⫺␴¯i_{) the anisotropy parameter and ␩}i_⫽(␴ y y i

⫺␴xx i

)/␦ithe asymmetry parameter of the interaction.25The values of these parameters can be inserted in Eq. 共18兲 to evaluate the V_pqk parameters, yielding

V_p02i⫽d_p02 共␤_m兲exp共i␥_rp兲

兺

s⫽⫺2 2 共ds p 2 _共␤ r兲exp共i共␣r⫹␥c i_兲s兲 ⫻共d0s 2 _共␤ c i_兲

冑

3 2␦ i_{⫹兵exp共i2␣} c i_兲d 2s 2 _共␤ c i_兲 ⫹exp共⫺i2␣c i_兲d ⫺2s 2 _共␤ c i_兲其1 2␩ i_␦i_{兲兲 共26兲}

with V₀₀2i⫽0, since for MAS d₀₀2(␤_m)⫽0.

Using Eqs.共19兲 and 共22兲, the chemical shift contribution to the interaction Hamiltonian can be constructed and yields

Hˆi CS_⫽

兺

i⫽1 N

兺

p⫽1 2 共Zp i_Fˆ p⫹Zp i*_F p †_兲Iˆ z i_{, 共27兲} with Zi_p⫽(Z_p02 )iand Zi_p⫽

冑

2 3␥H0Vp0 2i _{. 共28兲}

The isotropic part is not affected by the spinning and yields a contribution to the pure nuclear spin term

Hˆn CS_⫽

兺

i_⫽1 N ⌬␻¯iIˆ_zi, 共29兲 with⌬␻¯i⫽⫺␥H01/3(␴xx i _⫹ ␴y y i _⫹ ␴zz i ).

The spin space tensor operator for the dipolar interaction between a pair of spins (i, j) is

Tˆ₂₀i j⫽⫺

冑

1 62␥ 2_ប共2Iˆ z i Iˆ_zj⫺12共Iˆ⫹ i

Iˆ_⫺j ⫹Iˆ_⫹i Iˆ_⫺j 兲兲. 共30兲 The components of the spatial tensor V_p02i j for the spin pair interaction can be obtained from Eq.共26兲 with␦isubstituted by

␦i j_⫽⫺␮0

2␲

␥2_ប r_{i j}3 ,

and ␩i substituted by ␩i j⫽0. Thus the dipolar term in the interaction Hamiltonian is a quantized field contribution that is bilinear in the spin operators,

Hˆi D_⫽

兺

i⬍ j p

兺

⫽1 2 共Zp i j_Fˆ p⫹Zp i j*_Fˆ p †_兲共2Iˆ z i_Iˆ z j_⫺1 2共Iˆ⫹ i _Iˆ ⫺j⫹Iˆ⫹i Iˆ⫺j 兲兲 共31兲 with the summation over all spin pairs i⬍ j.

Here, with Zp i j_⫽(Z p0 2 )i j, Zi j_p⫽⫺Cp i j ri j 3 共32兲 and C_pi j⫽␮0 4␲ ␥ 2_បd p0 2 共␤m兲exp共i␥rp兲

兺

s_⫽⫺2 2 d_{s p}2 共␤r兲 ⫻exp共i共␣r⫹␥c i j_兲s兲d 0s 2_共␤ c i j_{兲 共33兲}

with␤_ci j and␥_ci j the polar angles of the dipolar vector in the crystal frame.

Since the dipolar interaction is traceless, the contribution to the pure nuclear term due to the dipolar interaction is

Hˆn

D_{⫽0. According to Eq. 共11兲 the time independent}

quan-tized field MAS HamiltonianHˆQof the coupled spin system

is the sum of Eqs.共27兲, 共29兲, 共31兲, and 共12兲.

IV. RADIO FREQUENCY PULSES

An on-resonance RF field contributes to the spatial ro-tating frame Hamiltonian a nuclear spin Hamiltonian term of the form:

HˆRF⫽␻1共Iˆxcos␾⫹Iˆysin␾兲. 共34兲

The ␻1 is the nutation frequency and ␾is the RF phase in

the rotating frame.23 TheHˆRFoperates only on the spin part

of the spin system and is independent of the sample spinning. If the intensity of a short RF pulse is sufficiently strong then it is possible to neglect all the other terms in the Hamiltonian containing spin operators. During a pulse the effect of the rotor should be considered to account for refocusing errors and to achieve stable effective dipolar recoupling.26 The re-maining terms in the quantized field Hamiltonian are then

HˆQ

RF_⫽Hˆ

RF⫹Hˆr. 共35兲

The HˆQ

RF

is time-independent and its evolution operator at the end of a pulse of length ␶p becomes

Uˆ 共␶p兲⫽exp共⫺i共HˆRF⫹Hˆr兲␶p兲. 共36兲

However, in the limit of an extremely short pulse ␶p→0,

while␪⫽␻1␶pis kept constant, also the rotor dynamics

dur-ing the pulse can be neglected and a pulse evolution operator can be defined as Pˆ 共␪兲⫽exp

冉

⫺i

兺

i⫽1 N ␪共Iˆx i_cos␾⫹Iˆ y i_sin␾兲

冊

_{, 共37兲}

affecting only the spin-operational part of the spin system.27,28

During an interval of length ␶m between such pulses,

Pˆm_⫺1and Pˆm, in a multi-pulse experiment the spin system

is governed by the time independent quantized field Hamil-tonianHˆQand the evolution of the spin system in this period

is described by the evolution operator Uˆ (␶m)⫽exp

(⫺iHˆQ␶m). The overall evolution operator for a pulse

se-quence of M equally spaced pulses during a time of ␶c is

UC 共␶c兲⫽

兿

m⫽1 M PˆmUˆ 共␶m兲, 共38兲 with ␶c⬅

兺

m⫽1 M ␶m. 共39兲

Schematic representations of such pulse sequences are shown in Fig. 1.

A product of unitary transformations is again a unitary transformation and it should be possible to express the entire sequence in terms of an average quantized field Hamiltonian

H¯ ˆ

Qaccording to

as for spin-Hamiltonians.29 The evaluation of this average Hamiltonian must be accomplished by using average Hamil-tonian theory in the quantized field representation. This is discussed in the following section.

V. ROTOR FREQUENCY-DRIVEN DIPOLAR RECOUPLING

The RFDR sequence was analyzed previously using av-erage Hamiltonian theory and Floquet theory.5,30,31It utilizes a train of rotor-synchronized ␲-pulses to invoke the dipolar recoupling. In the original version one pulse per rotor period is used, with a time window between the pulses␶_w⫽␶_r, with

␶r the length of one rotor period. Here a generalization of

RFDR is discussed that was first introduced in Ref. 19. A fixed number of rotor periods per pulse nw is used and ␶w

⫽nw␶r is the time window between the pulses.19,26In this

paper we restrict ourselves to even nwvalues and one RFDR

cycle contains two pulses 关1

2␶w⫺Pˆ1(␲)⫺␶w⫺Pˆ2(␲)

⫺1

2␶w兴 in a cycle time of␶c⫽2␶w. The sequence allows for

narrow band RFDR and its frequency selectivity has been discussed recently in Ref. 26. When the pulses are cyclic in the sense ⌸_mp_⫽1Pˆ1Pˆ2⫽1ˆ, the expression for the averaged

quantized field Hamiltonian can be found by transforming

HˆQ to the ‘‘toggling frame,’’ were the RF pulses are

eliminated.27,28This implies that the evolution operator in the spatial rotating frame and the toggling frame are the same at the end of each RFDR cycle.

The basis RFDR pulse cycle can be divided into three periods 0⭐t⭐12␶w, 1 2␶w⭐t⭐ 3 2␶w, and 3 2␶w⭐t⭐2␶w. The

effect of such a cycle on an ensemble of N dipolar coupled like spins can be evaluated using the quantized field formal-ism in the toggling interaction frame of the chemical shift and the sample spinning. If the HˆQ is divided according to

HˆQ⫽Hˆ0⫹Hˆ1, with Hˆ0⫽Hˆn CS_⫹Hˆ i CS_⫹Hˆ r, 共41兲 Hˆ1⫽Hˆi D_,

the toggling frame Hamiltonian becomes

H˜ˆ_0⫽

再

Hˆn CS_⫹Hˆ i CS_⫹Hˆ r, 0⬍t⬍12␶w, ⫺Hˆn CS_⫺Hˆ i CS_⫹Hˆ r, 12␶w⬍t⬍ 3 2␶w, Hˆn CS_⫹Hˆ i CS_⫹Hˆ r, 32␶w⬍t⬍2␶w, 共42兲 H˜ ˆ 1⫽Hˆi D

where we assumed infinitely short ␲-pulses.

The evolution operator can be written in the toggling frame as Uˆ˜(t)⫽Uˆ˜0(t)Uˆ˜1(t), with Uˆ˜1(t) governed by the

equation of motion dU˜ˆ1共t兲 dt ⫹iH ˜ ˆ int共t兲Uˆ˜1共t兲⫽0, 共43兲 with U0共t兲⫽exp共⫺iH˜ ˆ 0t兲 共44兲 and H˜ ˆ int共t兲⫽U˜ ˆ 0 ⫺1_共t兲Hˆ˜ 1U˜ ˆ 0共t兲, 共45兲

the Hamiltonian in the interaction frame of Hˆ˜0.25

The evolution operator Uˆ˜1(t) in this interaction frame at t⫽2␶w becomes equal to the toggling frame U˜

ˆ

(2␶w) when

U˜ ˆ

0(2␶w)⫽1ˆ. This equality can easily be shown by the

fol-lowing calculation and implies that the spin evolution in the original spatial rotating frame is governed by Uˆ (2␶w)

⫽Uˆ˜

1(2␶w). The HamiltonianHˆ˜0 in Eq. 共42兲 contains three

terms. The isotropic chemical shift term, proportional toH_nCS in Eq. 共29兲, the CSA interaction terms, equal to ⫾Hˆ_iCS de-fined in Eq.共27兲, and the rotor term Hr. The first term

com-mutes with the additional terms and its evolution operator is one at 2␶w. Thus the evolution operator in Eq. 共44兲 only

depends on the two remaining and noncommuting terms: U˜ ˆ 0共2␶w兲⫽exp共⫺i/2共Hˆi CS_⫹Hˆ r兲␶w兲exp共⫺i共⫺Hˆi CS ⫹Hˆr兲␶w兲exp共⫺i/2共Hˆi CS_⫹Hˆ r兲␶w兲. 共46兲

To show that this operator equals one we use the following diagonalization conditions: Hˆi CS_⫹Hˆ r⫽Dˆ⫺1HˆrDˆ , 共47兲 ⫺Hˆi CS_⫹Hˆ r⫽DˆHˆrDˆ⫺1

which are derived in Appendix A. Insertion of these equa-tions into Eq.共46兲 and using that exp(iHˆr␶w)⫽1ˆ results in a

periodic U˜ˆ0(t) operator with U˜

ˆ

0共2␶w兲⫽Dˆ exp共⫺i/2Hˆr␶w兲Dˆ⫺1Dˆ⫺1

⫻exp共⫺iHˆr␶w兲DˆDˆ exp共⫺i/2Hˆr␶w兲Dˆ⫺1⫽1ˆ .

共48兲 Thus the CSA interaction is refocused at the end of a RFDR cycle, as is well known for two ␲-pulses that are separated by an integer multiple of rotor periods ␶w⫽nw␶c.

FIG. 1. Schematic representation of the generalized RFDR sequence with

共A兲␶w⫽␶rand共B兲␶w⫽2␶r. The sequences start with ramped cross

polar-ization. The magnetization is rotated to the z axis and the recoupling se-quence is applied. Prior to detection the polarization is transferred to the xy plane.

It is now possible to use the interaction Hamiltonian in Eq. 共45兲 for the evaluation of the average RFDR Hamil-tonian. The quantized interaction Hamiltonian is time depen-dent and is not anymore defined in the spatial rotating frame. This is due to the fact that the transformation operator Uˆ˜0(t)

contains the rotor Hamiltonian term Hˆr. However, because

we are only interested in the spin response at the end of the RFDR cycles and U˜ˆ0(t) is periodic, the time independent

average Hamiltonian can be considered as being defined in the spatial rotating frame. We will restrict ourselves to the calculation of the zero order average Hamiltonian assuming that 2␶w储H˜

ˆ int储Ⰶ1.

VI. THE ZERO ORDER AVERAGE RFDR HAMILTONIAN

The zero order average RFDR Hamiltonian of a homo-nuclear spin pair (i, j ), evolving with the isotropic and an-isotropic chemical shift interactions of both spins defined in Eqs. 共27兲 and 共29兲, equals

H¯ ˆ Q⫽ 1 2␶w

冕

0 2␶_w H˜ ˆ intdt⫽ 1 2␶w

冕

0 2␶_w U˜ ˆ 0 ⫺1_共t兲Hˆ˜ 1U˜ ˆ 0共t兲dt 共49兲 with the two-spin dipolar interaction Hamiltonian in Eq. 共31兲. Simplifying the expressions by defining the operators,

Uˆr共t兲⫽exp共⫺iHˆrt兲, 共50兲 Uˆ_nCS共t兲⫽exp

冉

⫺i

兺

i⫽1 2 ⌬␻¯iIˆ_zit

冊

and using the diagonalization operators Dˆ ⫽Dˆ_iDˆ_jof the two spins, the integral of the average Hamiltonian can be written as H¯ ˆ Q⫽ 1 2␶_w

冕

_⫺1/2␶ w 1/2␶_w dt Uˆ_nCS⫺1共t兲 ⫻兵Dˆ Uˆr共t兲Dˆ⫺1其Hˆ1兵Dˆ Uˆr⫺1共t兲Dˆ⫺1其Uˆn CS_共t兲 ⫹Uˆn CS_共t兲兵Dˆ⫺1_Uˆ r共t兲Dˆ其Hˆ1 ⫻兵D⫺1Uˆ_r⫺1共t兲Dˆ其U₀⫺1共t兲. 共51兲 Here we used the fact that during the three time intervals of the RDFR cycle the Hamiltonians are time independent. In the appendix the integral in Eq.共51兲 is calculated by expand-ing the diagonalization operator. The result yields an expres-sion for Hˆ¯_Q of the form:

H¯ ˆ Q⫽⫺

兺

i⬍ j

冉

d_{i j}0⫹

兺

k⫽1 ⬁ d_{i j}kFˆk⫹di j k*_Fˆ k †

冊

1 2共Iˆ⫹ i

Iˆ_⫺j ⫹Iˆ_⫺i Iˆ_⫹j 兲

⫽⫺

兺

i⬍ j

冉

d_{i j}0⫹

兺

k⫽1 ⬁ d_{i j}kFˆk⫹di j k*_Fˆ k †

冊

_共Iˆ x i

Iˆ_xj⫹Iˆ_yiIˆ_yj兲, 共52兲 with di j k_⫽1 r_{i j}3 n⫽⫺⬁

兺

⬁ Mkn i j sinc

冉

2nw共⌬␻¯ i_⫺⌬␻¯j_⫺n␻ r兲 ␻r

冊

共53兲 and M_kni j⫽⫺

兺

p⫽⫺2 2 C_pi j共K_ni j_⫹kK_ni j_⫹p* ⫹K_ni j_⫺k* K_ni j_⫺p兲 共54兲 with K_mi j⫽

兺

k⫽⫺⬁ ⬁ Jk

冉

⫺ 兩Z2 i_⫺Z 2 j_兩 ␻r

冊

Jm_⫺2k

冉

⫺2 兩Z1 i_⫺Z 1 j_兩 ␻r

冊

⫻exp 共i共m⫺2k兲␾1 i j_⫹ik␾ 2 i j_{兲, 共55兲}

where C_pi j is given by Eq. 共33兲 and Z_pi j in Eq.共32兲. In Eq. 共52兲 a summation over all spin pairs in a coupled homo-nuclear spin system is added. The HCQ can induce

polariza-tion transfer between the nuclei.5 The rate of transfer strongly depends on the internuclear distance d_{i j}k⬀1/r_{i j}3, ac-cording to Eq. 共53兲. This provides the selectivity necessary for correlation spectroscopy in isotope enriched solids.

Introducing the deviation from the rotational resonance condition by the off-rotational resonance value ␦␻¯_{i j}n⫽(⌬␻¯i ⫺⌬␻¯j⫺n␻_r), we see that the sinc-function in Eq.共53兲 has a maximum at every rotational resonance condition ␦␻¯i j

n_⫽0,

including the n⫽0 rotational resonance condition. For ␦␻¯_{i j}n ⫽0 the sinc-function decreases and can become zero for a certain value. If we define the bandwidth of the RFDR as the difference between the two zero points around the maximum value, the bandwidth is19

Bw⫽

␻r

nw

. 共56兲

This implies that the bandwidth can be narrowed by increas-ing the number of rotor periods per pulse. In the limit of large windows between the pulses (nw→⬁) this bandwidth

goes to zero. In this case only at the rotational resonance condition the zero order average Hamiltonian recovers the dipolar interaction. With adding ␲-pulses according to the extended RFDR scheme, the rotational resonance condition becomes broader and spectral selectivity can be considered. In this way, the rotor frequency drives the transfer in RFDR and not the radio frequency.

In Eq. 共53兲 also the n⫽0 rotational resonance is in-cluded. This implies that also for small isotropic shift differ-ences the dipolar interaction can be recovered. In the early treatment of the RFDR, this possibility for efficient transfer with small isotropic shift differences has been overlooked, since the shift anisotropy was generally excluded from the earlier analytical treatments. In contrast, in our quantized field analysis the chemical shift anisotropy is included and is embedded in the K_mi j in Eq.共55兲. This theoretical outcome is experimentally confirmed, because efficient transfer around n⫽0 has been observed in chlorophylls.14,16It can be con-cluded that RFDR is considerably more broadband than originally thought.

VI. POLARIZATION TRANSFER

In Eq. 共52兲 the quantized field average Hamiltonian is given for the RFDR cycle. This Hamiltonian can be used to describe the evolution of the spin system after nmcycles via

UC 共␶_m兲⫽关exp共⫺i2HC_Q␶_w兲兴n_{m⫽exp共⫺iHC}

Q␶m兲, 共57兲

with ␶m⫽2nm␶w. This propagator promotes polarization

transfer from nucleus i to nucleus j. Within the multi-spin formalism presented here, multiple pathways are implicitly covered, since the polarization transfer can be direct

i→

HCQ

j,

or can be relayed, e.g.,

i→

HCQ

k→

HCQ

j .

The discrimination between direct and relayed transfer has attracted considerable attention in recent years.32In a general treatment, the evolution of the spin system and the transfer of polarization can be described in terms of the evolution of the density operator

␳ˆ_共␶_m兲⫽UC共␶_m兲␳ˆ_共0兲UC⫺1_共␶_{m兲. 共58兲} The density operator in the quantized field representation describes the combination of rotor and spin system. This approach is very demanding, because the total process of creation and annihilation of particles via the Fourier opera-tors in combination with the multiple spin processes has to be taken into account. Therefore, to simplify matters we project the quantized Hamiltonian onto an average spin Hamiltonian HCS via a ‘‘dequantization’’ of the phase: Fˆk

⫽exp(ik␸ˆ

⬘

)→exp(ik␸0). This is justified in the simple case

we intend to consider, provided we are in the limit of a large number of rotor quanta. The average Hamiltonian in Eq.共52兲 becomes then HCS⫽⫺

兺

i⬍ j d ¯ i j共Iˆx i_Iˆ x j_⫹Iˆ y i_Iˆ y j_{兲, 共59兲} with d ¯ i j⫽

冉

di j 0_⫹

兺

k⫽1 ⬁ d_{i j}k exp共ik␸0兲⫹di j k*_{exp共⫺ik␸} 0兲

冊

. 共60兲

If we restrict ourselves to a two spin system then we avoid relayed polarization transfer. A convenient way of describing a two-spin system is using the single-transition operators33,34

I_z23⫽12共Iˆz

1_⫺Iˆ

z

2_兲,

I_x23⫽共Iˆ_x1Iˆ2_x⫹Iˆ_y1Iˆ_y2兲, 共62兲 I_y23⫽共Iˆ1_yIˆ_x2⫺Iˆ_x1Iˆ_y2兲.

The average Hamiltonian in Eq. 共59兲 can be expressed in those operators, according to

HCS⫽⫺

兺

i_{⬍ j} d ¯ i jIˆx 23 . 共63兲

If the spin density operator at the beginning of the RFDR period is ␳ˆ_{共0兲⫽共Iˆz}1_⫺Iˆ z 2_兲⫽2I z 23_{, 共64兲}

the average Hamiltonian will lead to rotation in the zy plane around the x axis of this space of single-transition operators, according to

␳ˆ_共␶_{m兲⫽共2Iˆz}23

cos共d¯12␶m兲⫹2Iˆy

23

sin共d¯12␶m兲 共65兲

which is consistent with earlier findings.5,31 However, in d¯i j

also the CSA and the narrow band RFDR sequence are taken into account. This implies that by measuring d¯_{i j}as a function of the n_w in principle not only information can be deduced about the internuclear distance, but also about the relative orientation of the CSA tensors of the two sites.35

This is illustrated in Fig. 2 with simulations of a RFDR experiment on two 13C spins resonating with a Larmor fre-quency of 125.7 MHz and separated by⬃1.4 Å with a small isotropic shift difference of 14 ppm, corresponding with 1.76 kHz. The orientation of the PAS of the CSA for the second spin is defined with respect to the PAS of the CSA of the first spin and changed by varying the Euler angle 0⭐␤⭐180. For

␤⫽0 the two tensors are aligned and the dipolar vector is along the axis corresponding with the largest principle com-ponent of the spin 1. The points are evaluated at three dif-ferent spinning speeds␯r⫽␻r/2␲ assuming an initial

condi-tion for the density matrix

具

2Iˆ_z1

典

and calculating the

具

2Iˆ_z2

典

after a constant mixing time␶m⫽2.66 ms.

At a low speed␯r⫽6 kHz we calculate efficient transfer

for nw⫽1 with

具

2Iˆz

2

_典

approaching the maximum of ⬃0.5 over a broad range and it depends on the value of ␤. The transfer efficiency drops for nw⫽2 and the angular

depen-dence is enhanced. The narrow band character of the RFDR is nicely illustrated for nw⫽4. Here the bandwidth is

Bw/2␲⫽1.5 kHz, less than the isotropic shift difference

(⌬␻¯1⫺⌬␻¯2)/2␲⫽1.76 kHz and the

具

2Iˆ_z2

典

⬃0.1, much less than for the nw⫽1 and nw⫽2 at the same spinning speed.

This reflects the decrease of the bandwidth for increasing nw.

With a spinning speed of 12 kHz, we calculate again a considerable dependence of the transfer efficiency on the angle ␤, which is most pronounced around ␤⫽30° and

␤⫽150°. The

具

2Iˆ_z2

典

goes through a maximum around

␤⫽90°. The relative variation of the transfer with␤is stron-gest for nw⫽4. The

具

2Iˆz

2

_典

peaks around␤⫽90° and it almost vanishes for ␤⫽0° or ␤⫽180°. These calculations suggest new and interesting possibilities for collecting angular infor-mation by measuring the transfer rate for different nw, using

the generalized RFDR treatment discussed here for the analysis. At 24 kHz, the transfer characteristics change again. At the high speed of 24 kHz also for the nw⫽4 the

B_w/2␲⫽6 kHz is sufficient to cover the isotropic shift dif-ference of 1.76 kHz. In addition, the spinning speed of 24 kHz is sufficient to attenuate the CSA’s, since ␦1_/2␲

⫽⫺11.3 kHz and␦2_{/2␲⫽⫺11.7 kHz. The M}

kn i j

in Eq.共54兲 depend on the spinning speed. They vanish in the limit of

␻r→⬁. Therefore the transfer is less efficient at high speed,

with

具

2Iˆ_z2

典

below 0.2 for vr⫽24 kHz. This illustrates that

close to the n⫽0 rotational resonance condition the presence of a dipolar interaction alone is insuffient for polarization transfer and that there is a prominent effect of the CSA on the transfer efficiency via the M_kni j .

VII. CONCLUDING REMARKS

We have shown that the quantized field description can be used to analyze pulse sequences including MAS on a multiple spin system. It is demonstrated that the quantized

field approach, from which the Floquet approach can be de-rived, can be combined with average Hamiltonian theory. In the earlier Floquet treatment of the RFDR, an effective Hamiltonian was formulated, with the pulses included in the sequence.30In the quantized field formalism the effect of the MAS rotation and the rotation itself are disentangled and the resulting time-independent Hamiltonian can be treated in an average Hamiltonian formalism by adding the pulses after-wards. In this way average Hamiltonian theory and Floquet theory are fully compatible, since average Hamiltonian theory can be applied to the time dependent quantized field Hamiltonian in the toggling frame.

The HCQ in Eq. 共52兲 induces polarization transfer

be-tween nuclei in a multiple spin system.5 The probability of transfer strongly depends on the internuclear distance ␦_{i j}k ⬀1/r3 _{and this makes correlation spectroscopy in isotope}

en-riched solids possible. The probability of polarization trans-fer has a maximum at every rotational resonance condition

␴

¯i_⫺␴¯j_⫽n␻

r. Since the CSA is embedded in the Km i j _also

the n⫽0 rotational resonance condition is included.

According to our treatment, the driving force in both RFDR and rotational resonance is the rotor frequency and not the radio frequency. This suggests that a physically more appropriate expansion of the RFDR abbreviation would be ‘‘rotor frequency-driven dipolar recoupling.’’ The RFDR bandwidth can be changed by changing the window between the ␲-pulses. This additional variable can be used to obtain information about relative orientation of the CSA tensors.

ACKNOWLEDGMENTS

This research was supported by the foundation of Life sciences 共ALW兲, financed by the Netherlands Organization for Scientific Research共NWO兲 and part of this research was supported by The Israel Science Foundation. G.J.B. and H.J.M.dG are recipients of NWO TALENT and PIONIER awards, respectively.

APPENDIX

In this appendix the expression for the zero order aver-age Hamiltonian in Eq. 共52兲 is derived. To do so the inter-action Hamiltonian of a two-spin system must be calculated by applying the transformation of Eq.共45兲:

H˜ ˆ

int共t兲⫽Uˆ˜0⫺1共t兲H˜ ˆ

1Uˆ˜0共t兲. 共A1兲

The transformation operator is defined by the sum of the isotropic chemical shift Hamiltonians

H˜ˆ n CS_共t兲 ⫽

再

1/2共⌬␻¯i⫺⌬␻¯j兲共I_zi⫺I_zj兲, 0⬍t⬍1/2␶w, ⫺1/2共⌬␻¯i_⫺⌬j_兲共I z i_⫺I z j_{兲, 1/2␶} w⬍t⬍3/2␶w, 1/2共⌬␻¯i⫺⌬␻¯j兲共Ii_z⫺I_zj兲, 3/2␶_w⬍t⬍2␶_w, 共A2兲 and the CSA interaction term plus the rotor Hamiltonian FIG. 2. Examples of magnetization transfer within a dipolar coupled spin

pair. The calculations are performed for two spins separated by 14 ppm and resonating at 125.7 MHz. A set of parameters was used that correspond to the CSA’s that can be observed, e.g., aromatic or ethylenic carbons: for the first spin an anisotropy␦1_{⫽⫺90 ppm was used with an asymmetry} param-eter␩⫽0.41, while␦2_{⫽⫺93 ppm with ␩⫽0.73. In the evaluation of the} signals␸0⫽0 and 300 orientations are taken for each point. The relative orientation of the tensors is defined by the Euler angles for the second spin (␣c 2 ,␤c 2 ,␥c 2

), following Eq. 共26兲. In this calculation ␣c

2

⫽␥c

2

⫽0 and ␤c

2

⫽␤0is varied. The Euler angles for the transformation of the PAS of the first spin and for the transformation of the dipolar frame to the crystal frame according to Eq.共33兲 are taken zero. This corresponds with an orientation of the dipolar vector parallel to the most shielded direction of the first spin Iz

1 . The powder integration is performed over (␣r,␤r,␥r). The points are

evaluated after ␶mix⫽2.66 msec by assuming an initial condition for the density matrix 2Iz

1 _{and following the magnitude of具2I}

z

2_{典. The maximum} value we can expect is具2Iz

2_{典⬃0.5 in a powder. XY8 phase cycling was used} for the full RFDR共nw⫽1, squares兲, XY4 for nw⫽2 共diamonds兲, and XX¯ for

H˜ ˆ i CS_{共t兲⫹Hˆ} r ⫽

冦

兺

k⫽i, j p

兺

⫽1 2 共Zp k_Fˆ p⫹Zp k*_Fˆ p †_兲I z k_⫹Hˆ r, 0⬍t⬍1/2␶w, ⫺

兺

k⫽i, j p

兺

⫽1 2 共Zp k Fˆp⫹Zp k*_Fˆ p †_兲I z i_⫹Hˆ r, 1/2␶w⬍t⬍3/2␶w,

兺

k_{⫽i, j} p

兺

_⫽1 2 共Zp k Fˆp⫹Zp k*_Fˆ p †_兲I z i_⫹Hˆ r, 3/2␶w⬍t⬍2␶w, 共A3兲 as U˜ ˆ 0共t兲⫽Uˆn CS_共t兲Uˆ i CS_{共t兲, 共A4兲} with Uˆ_nCS共t兲⫽exp

冉

⫺i

冕

0 t H˜ ˆ n CS_{共␶兲d␶}

冊

_, 共A5兲 Uˆ_iCS共t兲⫽exp

冉

⫺i

冕

0 t 共Hˆ˜ i CS 共␶兲⫹Hˆr兲d␶

冊

.

The dipolar interaction Hamiltonian from Eq. 共31兲 has the form H˜ ˆ i⫽共Zp i j Fˆp⫹Zp i j*_Fˆ p †_兲共2Iˆ z i Iˆz j

⫺1/2共Iˆi⫹Iˆ⫺j ⫹Iˆi⫺Iˆ⫹j 兲兲. 共A6兲

The HamiltoniansHˆ˜_nCS(t) andHˆ˜_iCS(t)⫹Hˆr commute and so

do Uˆ_nCS(t) and Uˆ_iCS(t). In addition, theˆH˜_iCS(t)⫹Hˆris block

diagonal and can be diagonalized according to Refs. 33 and 36 with (k⫽i, j),

兺

p_⫽1 2 共Zp k Fˆp⫹Zp k*_Fˆ p †_兲Iˆ z k_⫹Hˆ r⫽DˆkHˆrDˆk⫺1, 共A7兲

兺

p⫽1 2 ⫺共Zp k Fˆp⫹Zp k*_Fˆ p †_兲Iˆ z k_⫹Hˆ r⫽Dˆk⫺1HˆrDˆk with Dˆk⫽exp

再

⫺

兺

p⫽1 2

冉

Z_pk p␻r Fˆp⫺ Z_pk* p␻r Fˆ†_p

冊

Iˆ_zk

冎

. 共A8兲 Insertion of these results into Eq. 共A1兲, defining Dˆ⫽DˆiDˆj

with关Dˆi,Dˆj兴⫽0 and using 关Uˆn

CS (t),Uˆ_iCS(t)兴⫽0 we get H˜ ˆ int共t兲⫽

再

Uˆn CS_{共t兲DˆUˆ} r共t兲Dˆ⫺1Hˆ1Dˆ Uˆr⫺1共t兲Dˆ⫺1Uˆn CS⫺1_共t兲, Uˆ_nCS⫺1共t⫺␶w兲Dˆ⫺1Uˆr共t⫺␶w兲DˆHˆ1Dˆ⫺1Uˆr⫺1共t⫺␶w兲DˆUˆn CS_共t⫺␶ w兲, Uˆ_nCS共t⫺2␶w兲DˆUˆr共t⫺2␶w兲Dˆ⫺1Hˆ1Dˆ Uˆr⫺1共t⫺2␶w兲Dˆ⫺1Uˆn CS_共t⫺2␶ w兲, 共A9兲

respectively, for the three time intervals, where we assumed that nw is even in␶w⫽nw␶r, and Uˆr(1/2␶w)⫽1ˆ. When we

change the variables of integration and take into account that the Hamiltonians are constant during each time interval, the average Hamiltonian can be rewritten as

H¯ ˆ Q⫽ 1 2␶w

冕

⫺1/2␶w 1/2␶_w 兵Uˆ_nCS共t兲DˆUˆr共t兲Dˆ⫺1Hˆ1Dˆ Uˆr⫺1共t兲 ⫻Dˆ⫺1_Uˆ n CS⫺1_{共t兲⫹Uˆ} n CS⫺1_{共t兲Dˆ⫺1U}ˆ r共t兲 ⫻DˆHˆ1Dˆ⫺1Uˆr⫺1共t兲DˆUˆn CS_{共t兲其dt. 共A10兲}

To evaluate this integral we must consider the following computational steps: 共a兲 calculation of Aˆ⫽Dˆ⫺1Hˆ1Dˆ and Aˆ

⬘

⫽DˆHˆ1Dˆ⫺1 by expanding the diagonalization operators;

共b兲 application of the rotor operator Aˆ(t)⫽Uˆr(t)Aˆ Uˆr⫺1 and

Aˆ

⬘

(t)⫽Uˆr(t)Aˆ

⬘

Uˆr⫺1(t); 共c兲 transformation of Aˆ(t) and

Aˆ

⬘

(t) to Bˆ (t)⫽DˆAˆ(t)Dˆ⫺1 and Bˆ

⬘

(t)⫽Dˆ⫺1Aˆ

⬘

(t)Dˆ ; 共d兲 and application of the isotropic chemical shift operator Cˆ (t)⫽Uˆ_nCS(t)Bˆ (t)Uˆ_nCS⫺1 and Cˆ

⬘

(t)⫽Uˆ_nCS⫺1Bˆ

⬘

(t)Uˆ_nCS(t). To perform the first step we calculate the D-transformations of the terms of Hˆ1: Dˆ FˆpIˆz i_Iˆ z j_Dˆ⫺1_⫽Fˆ pIˆz i_Iˆ z j_, Dˆ⫺1FˆpIˆz i_Iˆ z j_{Dˆ ⫽Fˆ} pIˆz i_Iˆ z j_{, 共A11兲} Dˆ FˆpIˆ_⫹ i Iˆ_⫺j Dˆ⫺1⫽⌬ˆi jFˆpIˆ_⫹ i Iˆ_⫺j , Dˆ⫺1FˆpIˆ_⫹ i IˆjDˆ ⫽⌬ˆi j⫺1FˆpIˆ_⫹ i Iˆ_⫺j with ⌬i j_⫽exp

再

_⫺

兺

p⫽1 2

冉

Z_pi⫺Z_pj p␻r ⫺ Zp i*_⫺Z p j* p␻r

冊

冎

共A12兲 and ⌬ˆi j⫽⌬ˆji⫺1 and⌬ˆi j⫹⫽⌬ˆi j⫺1. This exponent can be ex-panded in a Fourier series using Z_pi⫺Z_pj⫽兩Zi_p ⫺Zp j_兩exp(i␾ p ij_): ⌬ˆi j_⫽

兿

p⫽1 2

兺

m_⫽0 ⬁

兺

n_⫽0 ⬁ 1 n!

冉

⫺ Z_pi⫺Z_pj p␻_r F ˆ p

冊

n 1 m! ⫻

冉

⫺Zp i*_⫺Z p j* p␻r Fˆ_⫺p

冊

m ⫽

兿

p⫽1 2

兺

m⫽0 ⬁

兺

l⫽⫺m ⬁ ₁ m! 1 共m⫹l兲! ⫻

冉

⫺Zp i_⫺Z p j p␻r

冊

m⫹l

冉

Zi_p*⫺Z_pj* p␻r

冊

m Fˆ_{l p} ⫽

兿

p⫽1 2

兺

m⫽0 ⬁

兺

l⫽⫺⬁ ⬁ ₁ m! 共⫺1兲m ⌫共m⫹l⫹1兲

⫻

冉

⫺兩Zp i_⫺Z p j_兩 p␻r

冊

2m⫹l exp共il␾_pi j兲Fˆl p ⫽

兺

k⫽⫺⬁ ⬁

兺

l⫽⫺⬁ ⬁ Jk

冉

⫺2 兩Z2 i_⫺Z 2 j_兩 2␻r

冊

Jl ⫻

冉

⫺2兩Zl i_⫺Z l j_兩 ␻r

冊

exp共il␾₁i j⫹ik␾₂i j兲Fˆl⫹2k

⫽

兺

m⫽⫺⬁ ⬁ K_mi jFˆm 共A13兲 with K_mi j⫽

兺

k⫽⫺⬁ ⬁ Jk

冉

⫺ 兩Z2 i_⫺Z 2 j_兩 ␻r

冊

Jm_⫺2k

冉

⫺2 兩Z1 i_⫺Z 1 j_兩 ␻r

冊

⫻exp共i共m⫺2k兲␾1 i j_⫹ik␾ 2 i j_{兲 共A14兲}

and Jk(x) the kth order Bessel function of x. Thus in step共a兲

the transformation results in

Aˆ ⫽

兺

p⫽1 2

再

2共Z_pi jFp⫹Zp i j*_F p †_兲I z i I_zj⫺1/2 ⫻

兺

m⫽⫺⬁ ⬁ 共共Zp i j Km i j Fm⫹p⫹Zp i j*_K m i j Fm⫺p兲Ii⫹I⫺j ⫹共Zp i j_K ⫺m i j*_F m⫹p⫹Zp i j*_K ⫺m i j*_F m⫺p兲Ii⫺Ij⫹兲

冎

, 共A15兲 Aˆ

⬘

⫽

兺

p⫽1 2

再

2共Zp i j Fp⫹Zp i j*_F p †_兲I z i Iz j_⫺1/2 ⫻

兺

m⫽⫺⬁ ⬁ 共共Zp i j_K ⫺m i j*_F m⫹p⫹Zp i j*_K ⫺m i j*_F m⫺p兲Ii⫹Ij⫺ ⫹共Zp i j_K m i j_F m_⫹p⫹Zp i j*_K m i j_F m_⫺p兲Ii⫺I⫹j 兲

冎

.

In the next step共b兲 we use the fact that U_r共t兲F_pU_r⫺1共t兲⫽F_pexp共⫺ip␻_rt兲,

共A16兲 U_r⫺1共t兲FpUr共t兲⫽Fpexp共ip␻rt兲

and replace all Fp in Eq. 共A15兲 by Fpexp(⫺ip␻r) and

Fpexp(ip␻r) to obtain A(t) and A

⬘

(t), respectively. In step

共c兲 an additional D-transformation must be performed. The results for B(t) and B

⬘

(t), obtained again by using Eqs. 共11兲–共13兲, are cumbersome and are therefore not shown here. Their coefficients of I_ziI_zj and I_⫾i I_⫾j contain multiples of the K-parameters. In the last step the isotropic chemical shift Hamiltonian is applied to the bilinear spin operators

U_nCS⫾1共t兲I_ziI_zjU_nCS⫿1⫽I_ziI_zj,

U_nCS⫾1共t兲I_⫹i I_⫺jU_nCS⫿1⫽I_⫹i I_⫺j exp共⫿共⌬␻i⫺⌬␻j兲t兲, 共A17兲 U_nCS⫾1共t兲I_⫺i I_⫹jU_nCS⫿1⫽I_⫺i I_⫹j exp共⫾共⌬␻i⫺⌬␻j兲t兲

in order to obtain expressions for C(t) and C

⬘

(t) from B(t) and B

⬘

(t). Insertion of the results of these calculations in Eq. 共A10兲 yields for the zero order average Hamiltonian the fol-lowing: H¯ ˆ Q⫽⫺ 1 4␶w

兺

i⬍ j p

兺

⫽⫺2 2 Z_pi j

兺

k,n⫽⫺⬁ ⬁

冉

K_ki jK_ni j_⫹p* Fˆk_⫺nIˆ_⫹i Iˆ_⫺j ⫻

冕

⫺12␶w 1 2␶w _{exp共i共⌬}␻_¯i_⫺⌬␻¯j_⫺n␻ r兲t兲dt ⫹K_⫺ki j*_K n⫺p i j _Fˆ k_⫹nIˆ_⫹j Iˆ_⫺i

冕

⫺12␶w 1 2␶w _{exp共i共⌬}␻_¯j_⫺⌬␻¯i ⫹n␻r兲t兲dt⫹K_⫺ki j*Kn⫺p i j _Fˆ k_⫹nIˆ_⫹i Iˆ_⫺j

冕

⫺12␶w 1 2␶w _{exp共i共⌬}␻_¯j ⫺⌬␻¯i⫹n␻_r兲t兲dt⫹K_ki jKi j_n⫹p* Fˆ_k⫺nIˆ_⫹j Iˆ_⫺i

冕

⫺21␶w 1 2␶w ⫻exp共i共⌬␻¯i⫺⌬␻¯j⫺n␻r兲t兲dt

冊

共A18兲

and the actual integration gives Eqs. 共52兲 and 共53兲. This Hamiltonian has only a (I_xiI_xj⫹I_yiI_yj)⫽1/2(I_⫹i I_⫺j ⫹I_⫺i I_⫹j) term, since the integral of the I_ziI_zj coefficient, containing only terms of exponents exp(⫾ip␻_rt) is zero when ␶_w is a multiple of the rotor period␶r.

1_{B. J. van Rossum et al., Spectrochim. Acta A 54, 1167共1998兲.} 2_{B. J. van Rossum, S. Prytulla, H. Oschkinat, and H. J. M. de Groot,}

Proceedings of the Joint 29th AMPERE—13th ISMAR International Con-ference, Berlin, Vol. 1, p. 38, 1998.

3_{R. Tycko and G. Dabbagh, Chem. Phys. Lett. 173, 461共1990兲.} 4_{R. G. Griffin, Nat. Struct. Biol. 5, 508共1998兲.}

5_{A. E. Bennet, J. H. Ok, R. G. Griffin, and S. Vega, J. Chem. Phys. 96,}

8624共1992兲.

6

M. Baldus, M. Tomaselli, B. H. Meier, and R. R. Ernst, Chem. Phys. Lett.

230, 329共1994兲.

7_{J. M. Joers, R. Rosanske, T. Gullion, and J. R. Garbow, J. Magn. Reson.}

106, 123共1994兲.

8

B. Q. Sun et al., J. Chem. Phys. 102, 702共1995兲.

9_{Y. K. Lee et al., Chem. Phys. Lett. 242, 304共1995兲.}

10_{D. M. Gregory, D. J. Mitchell, and G. P. Drobny, Chem. Phys. Lett. 246,}

654共1995兲.

11_{R. Verel, M. Baldus, M. Ernst, and B. H. Meier, Chem. Phys. Lett. 287,}

421共1998兲.

12_{I. J. Lowe, Phys. Rev. Lett. 2, 285共1959兲.}

13_{E. R. Andrew, A. O. Bradbury, and R. G. Eades, Nature共London兲 182,}

1659共1958兲.

14

G. J. Boender et al., Chem. Phys. Lett. 237, 502共1995兲.

15

B. J. van Rossum, H. Fo¨rster, and H. J. M. de Groot, J. Magn. Reson. 124, 516共1997兲.

16_{T. S. Balaban et al., Biochemistry 34, 15259共1995兲.}

17_{G. J. Boender, S. Vega, and H. J. M. de Groot, Mol. Phys. 95, 921共1998兲.} 18

J. H. Shirley, Phys. Rev. 138, 979共1965兲.

19_{G. J. Boender, thesis, Leiden University, 1996.}

20_{M. M. Maricq and J. S. Waugh, J. Chem. Phys. 70, 3300共1979兲.} 21_{C. Cohen Tannoudji, B. Diu, and F. Laloe, Quantum Mechanics}

共Her-mann, Paris, 1977兲.

22

Quantum Mechanics, 3rd ed., Course of Theoretical Physics, edited by L.

D. Landau and E. M. Lifshitz共Oxford, Pergamon, New York, 1981兲.

23_{M. Mehring, Principles of High Resolution NMR Spectroscopy in Solids}

共Springer-Verlag, Berlin, 1983兲, 2nd Ed.

24

G. Racah, Phys. Rev. 62, 438共1942兲.

25_{U. Haeberlen, High Resolution NMR in Solids: Selective Averaging,}

26_{A. E. Bennett et al., J. Chem. Phys. 108, 9463共1998兲.}

27_{J. S. Waugh, L. M. Huber, and U. Haeberlen, Phys. Rev. Lett. 20, 180}

共1968兲.

28

J. S. Waugh, C. H. Wang, L. M. Huber, and R. L. Vold, J. Chem. Phys.

48, 662共1968兲.

29_{R. R. Ernst, G. Bodenhausen, and A. Wokaun, Principles of Nuclear}

Magnetic Resonance in One and Two Dimensions 共Clarendon, Oxford,

1987兲.

30

O. Weintraub, S. Vega, Ch. Hoelger, and H. H. Limbach, J. Magn. Reson.,

Ser. A 109, 14共1994兲.

31_{D. K. Sodikson, M. H. Levitt, S. Vega, and R. G. Griffin, J. Chem. Phys.}

98, 6742共1993兲.

32

B. Q. Sun et al., J. Chem. Phys. 102, 702共1995兲.

33_{S. Vega, J. Chem. Phys. 68, 5518共1978兲.}

34_{A. Wokaun and R. R. Ernst, J. Chem. Phys. 67, 1752共1977兲.} 35_{G. Goobes, G. J. Boender, and S. Vega共in preparation兲.}

36_{D. B. Zax, G. Goelman, D. Abromovich, and S. Vega, Adv. Magn. Reson.}