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Virtual Journal for Biomedical Optics

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  • Editor: Gregory W. Faris
  • Vol. 4, Iss. 4 — Apr. 1, 2009
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Radiation force of coherent and partially coherent flat-topped beams on a Rayleigh particle

Chengliang Zhao, Yangjian Cai, Xuanhui Lu, and Halil T. Eyyuboğlu  »View Author Affiliations


Optics Express, Vol. 17, Issue 3, pp. 1753-1765 (2009)
http://dx.doi.org/10.1364/OE.17.001753


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Abstract

Propagations of coherent and partially coherent flat-topped beams through a focusing optical system are formulated. The radiation force on a Rayleigh dielectric sphere induced by focused coherent and partially coherent flat-topped beams is investigated theoretically. It is found that we can increase the transverse trapping range at the planes near the focal plane by increasing the flatness (i.e., beam order) of the flat-topped beam, and increase the transverse and longitudinal trapping ranges at the focal plane by decreasing the initial coherence of the flat-topped beam. Moreover the trapping stiffness of flat-topped beam becomes lower as the beam order increases or the initial coherence decreases. The trapping stability is also analyzed.

© 2009 Optical Society of America

1. Introduction

In recent years, light beams with flat-topped profiles have attracted more and more attention due to their wide applications in free-space optical communications, inertial confinement fusion, material thermal processing, nonlinear optics and electron acceleration [1–8

1. D. C. Cowan, J. Recolons, L. C. Andrews, and C. Y. Young, “Propagation of flattened Gaussian beams in the atmosphere: a comparison of theory with a computer simulation model,” in Atmospheric Propagation III, C. Y. Young and G. C. Gilbreath, eds., Proc. SPIE6215, 62150B (2006).

]. Several theoretical models such as super Gaussian beam, flattened Gaussian beam, flat-topped beam and flat-topped multi-Gaussian beam have been proposed to describe a laser beam with flat-topped beam profile [9–12

9. M. S. Bowers, “Diffractive analysis of unstable optical resonator with super-Gaussian mirrors,” Opt. Lett . 19, 1319–1321 (1992). [CrossRef]

]. Propagations of various flat-topped beams in free-space, paraxial optical systems and turbulent atmosphere have been studied in detail [1

1. D. C. Cowan, J. Recolons, L. C. Andrews, and C. Y. Young, “Propagation of flattened Gaussian beams in the atmosphere: a comparison of theory with a computer simulation model,” in Atmospheric Propagation III, C. Y. Young and G. C. Gilbreath, eds., Proc. SPIE6215, 62150B (2006).

,4

4. Y. Cai, “Propagation of various flat-topped beams in a turbulent atmosphere,” J. Opt. A: Pure Appl. Opt . 8, 537–545 (2006). [CrossRef]

, 9–20

9. M. S. Bowers, “Diffractive analysis of unstable optical resonator with super-Gaussian mirrors,” Opt. Lett . 19, 1319–1321 (1992). [CrossRef]

].

2. The characteristics of coherent and partially coherent flat-topped beams

In this paper, we adopt the model for a flat-topped beam proposed by Li [11

11. Y. Li, “Light beam with flat-topped profiles,” Opt. Lett . 27, 1007–1009 (2002). [CrossRef]

]. The electric field of a coherent flat-topped beam at z=0 can be expressed as a finite sum of fundamental Gaussian modes as follows [11

11. Y. Li, “Light beam with flat-topped profiles,” Opt. Lett . 27, 1007–1009 (2002). [CrossRef]

],

EinN(r,z=0)=E0Nn=1N(1)n1NNnexp(nr2w02),
(1)

where E 0N is a normalization factor, w 0 is the waist size of the fundamental Gaussian mode, Nn denotes a binomial coefficient, and N is called the beam order of the flat-topped beam, When N=1, Eq. (1) reduces to the electric field of a Gaussian beam. Here we assume the power of the flat-topped beam to be P. Following [32

32. Y. Harada and T. Asakura, “Radiation forces on a dielectric sphere in the Rayleigh scattering regime,” Opt. Commun . 124, 529–541 (1996). [CrossRef]

], the power of a flat-topped beam is calculated by following formula

P=++IinN(r,z=0)dxdy,
(2)

where IinN(r,z=0)=nmε0c2EinN(r,z=0)2,, nm is the refractive index of the surrounding medium, 0 is the dielectric constant, and c is the speed of the light in vacuum. Substituting Eq. (1) into Eq. (2), we can obtain the expression for the normalization factor E 0N as follows

E0N=4nP/n=1N(1)2(n1)N2Nnπw02nmε0c.
(3)

The power of the flat-topped beam in this paper is set to be P=1W, which means every beam discussed in the following text carries the same power. Figure 1 shows the intensity distributions of a flat-topped beam for four different values of N with w 0 = 10mm. One finds from Fig. 1 that the beam profile becomes flatter (i.e., beam width increases) but the maximum intensity decreases as N increases, which means the potential wells of flatter beams (for example N=4, N=3) are lower or shallower than their counterparts (for example N=2, N=1). Fig. 1(b) is consistent with Fig. 1(a) of [11

11. Y. Li, “Light beam with flat-topped profiles,” Opt. Lett . 27, 1007–1009 (2002). [CrossRef]

].

Fig. 1. Intensity distribution of a flat-topped beam for four different values of N with w 0 = 10mm (a) contour graph, (b) cross line (y=0)

After some arrangement, Eq. (1) can be expressed in following tensor form [18

18. Y. Cai and Q. Lin, “Light beams with elliptical flat-topped profiles,” J. Opt. A: Pure Appl. Opt . 6, 390–395 (2004). [CrossRef]

]

EinN(r,z=0)=E0Nn=1N(1)n1NNnexp(ik2rTQ1n1r),
(4)

where rT = (x y), k = 2π/λ is the wave number with λ being the wavelength, Q 1n -1 is a 2×2 matrix named complex curvature tensor, and is given by

Q1n1=(2ni/kw02002ni/kw02).
(5)

Within the validity of the paraxial approximation, by applying the tensor ABCD law [47

47. Q. Lin, S. Wang, J. Alda, and E. Bernabeu, “Transformation of non-symmetric Gaussian beam into symmetric one by means of tensor ABCD law,” Optik . 85, 67–72 (1990).

, 48

48. J. A. Arnaud, “Nonorthogonal optical waveguides and resonators,” Bell Syst. Tech . J. 49, 2311–2348 (1970).

], we can express the electric field of a flat-topped beam in the output plane after passing through a general astigmatic (i.e., nonsymmetrical) optical system as follows [18

18. Y. Cai and Q. Lin, “Light beams with elliptical flat-topped profiles,” J. Opt. A: Pure Appl. Opt . 6, 390–395 (2004). [CrossRef]

]

EoutN(ρ,z)=E0Nn=1N(1)n1NNn[det(A+BQ1n1)]1/2exp(ik2ρTQ2n1ρ),
(6)

Q2n1=(C+DQ1n1)(A+BQ1n1)1.
(7)

The intensity of a coherent flat-topped beam at the output plane is given by IoutN(ρ,z)=nmε0c2EoutN(ρ,z)2..

For the more general case, we need to take the coherence of light into consideration. It is well known that a partially coherent beam can be characterized by the cross-spectral density. The cross-spectral density (z=0) of a partially coherent beam generated by a Schell-model source can be expressed in the following well-known form [49

49. L. Mandel and E. Wolf, Optical Coherence and Quantum Optics (Cambridge, New York, 1995).

]

Γ(r1,r2,z=0)=I(r1,z=0)I(r2,z=0)g(r1r2),
(8)

where I(r,z = 0) = Γ(r,r,z = 0) is the intensity distribution of the partially coherent beam, and g(r 1 - r 2) is the spectral degree of coherence given by

g(r1r2)=exp[(r1r2)22σ02],
(9)

with σ 0 being the transverse spatial coherence width.

If the intensity distribution of a partially coherent flat-topped beam can be expressed as IinN(r,z=0)=nmε0c2EinN(r,z=0)2,, we can express the cross-spectral density of a partially coherent flat-topped beam at z=0 as follows [21

21. G. Wu, H. Guo, and D. Deng, “Paraxial propagation of partially coherent flat-topped beam,” Opt. Commun . 260, 687–690 (2006). [CrossRef]

, 22

22. Y. Cai and S. He, “Partially coherent flattened Gaussian beam and its paraxial propagation properties,” J. Opt. Soc. Am . A 23, 2623–2628 (2006). [CrossRef]

]

ΓinN(r1,r2,z=0)=E0N2n=1Nm=1N(1)n+mN2NnNmexp[nr12+mr22wo2(r1r2)22σ02],
(10)

In the incoherent limit (when σ0 = 0), Eq. (10) reduces to

ΓinN(r1,r2,z=0)=E0N2n=1Nm=1N(1)n+mN2NnNmexp(nr12+mr22wo2)δ(r1r2),
(11)

which denotes the cross-spectral density of an incoherent flat-topped beam. The two arbitrary transverse points of an incoherent flat-topped beam are correlated by δ function.

After some arrangement, Eq. (10) can be expressed in following tensor form

ΓinN(r˜,0)=E0N2n=1Nm=1N(1)n+mN2NnNmexp(ik2r˜TM1nm1r˜),
(12)

where T = (r 1 T r 2 T) = (x 1 y 1 x 2 y 2) and M 1nm -1 is a 4×4 complex matrix given by

M1nm1=[(2nikw02ikσ02)Iikσ02Iikσ02I(2mikw02ikσ02)I],
(13)

here I is a 2×2 unit matrix. Within the validity of the paraxial approximation, by applying the tensor ABCD law of partially coherent beam [50

50. Q. Lin and Y. Cai, “Tensor ABCD law for partially coherent twisted anisotropic Gaussian Schell-model beams,” Opt. Lett . 27, 216–218 (2002). [CrossRef]

], we can express the cross-spectral density of a partially coherent flat-topped beam after passing through a general paraxial astigmatic optical system as follows

ΓoutN(ρ1,ρ2,z)=E0N2n=1Nm=1N(1)n+mN2NnNm[det(A̅+B̅M1nm1)]1/2exp(ik2ρ˜TM2nm1ρ˜),
(14)

where ρ˜ T = (ρ 1 T ρ 2 T), Ā, B̄, C̄ and are defined as follows:

A̅=A0I0IA,B̅=B0I0IB,C̅=C0I0IC,D̅=D0I0ID.
(15)

M2nm1=(C̅+D̅M1nm1)(A̅+B̅M1nm1)1.
(16)

3. The focusing properties of coherent and partially coherent flat-topped beams

In this section, we apply the formulae derived in section 2 to study the focusing properties of coherent and partially coherent flat-topped beams as shown in Fig. 2. In Fig. 2, a thin lens with focal length f is located at the input plane (z=0), and the output plane is located at z = f + z 1, where z 1 is the axial distance from the focal plane to the output plane. Then the transfer matrix between the input and output planes can be expressed as follows

ABCD=I(f+z1)I0III0I(1/f)II=(z1/f)I(f+z1)I(1/f)II.
(17)

Substituting Eq. (17) into Eqs. (6) and (7

7. W. Wang, P. X. Wang, Y. K. Ho, Q. Kong, Z. Chen, Y. Gu, and S. J. Wang, “Field description and electron acceleration of focused flattened Gaussian laser beams,” Europhys. Lett . 73, 211–217 (2006). [CrossRef]

), we calculate in Fig. 3 the intensity distribution of a focused coherent flat-topped beam for different values of N at several propagation distances with f = 10mm, w 0 = 10mm, λ = 632.8nm. One finds from Fig. 3 that the focusing properties of a flat-topped beam (N>1) are very interesting and different from that of Gaussian beam (N=1). At the focal plane (z 1 =0), the intensity of the focused flat-topped beam is of quasi-Gaussian distribution, and maximum intensity decreases as the beam order N increases. When the output plane is a little away from the focal plane, the intensity of focused flat-topped beam becomes flat-topped, and the beam profile becomes flatter but the maximum intensity decreases as N increases. From Eq. (1), one can find that the flat-topped beam is not a pure mode, but a combination of different Gaussian modes, different Gaussian modes evolve differently upon propagation, what’s more, different modes overlap and interfere during propagation, thus leading to the interesting focusing properties of flat-topped beam. More information about the propagation properties of the flat-topped beam can be found in [10

10. F. Gori, “Flattened gaussian beams,” Opt. Commun . 107, 335–341 (1994). [CrossRef]

]-[20

20. X. Lü and Y. Cai, “Analytical formulas for a circular or non-circular flat-topped beam propagating through an apertured paraxial optical system,” Opt. Commun . 269, 39–46 (2007). [CrossRef]

].

Fig. 2. Schematic of a focusing optical system
Fig. 3. Intensity distribution of a focused coherent flat-topped beam for different values of N at several propagation distances

Fig. 4. Intensity distribution of a focused partially coherent flat-topped beam for different values of σ0 at several propagation distances

4. Radiation force produced by focused coherent and partially coherent flat-topped beams on a Rayleigh particle

Now we study the radiation force produced by focused coherent and partially coherent flat-topped beams on a Rayleigh dielectric sphere, whose radius is much smaller than the wavelength of the laser beam (i.e., aλ). The schematic for trapping a Rayleigh dielectric sphere with a focused flat-topped beam is shown in Fig. 2. A Rayleigh dielectric sphere with refractive index np is placed near the focus. In this case, the particle is treated as a point dipole. It’s well known that there are two kinds of the radiation force: scattering force and gradient force. The scattering force F Scat caused by the scattering of light by the sphere is proportional to light intensity and is along the direction of light propagation. The scattering force can be expressed as [32

32. Y. Harada and T. Asakura, “Radiation forces on a dielectric sphere in the Rayleigh scattering regime,” Opt. Commun . 124, 529–541 (1996). [CrossRef]

]

FScat(r,z)=eznmαIout/c,
(18)

where Iout is the intensity of the focused beam at the output plane, e→z is a unity vector along the beam propagation, α = (8/3)π(ka)4 a 2[(γ 2-1)/(γ 2+2)]2 , γ = np / nm. The gradient force F Grad produced by non-uniform electromagnetic fields is along the gradient of light intensity, and is expressed as [32

32. Y. Harada and T. Asakura, “Radiation forces on a dielectric sphere in the Rayleigh scattering regime,” Opt. Commun . 124, 529–541 (1996). [CrossRef]

]

FGrad(r,z)=2πnmβIout/c,
(19)

where θ = a 3(γ 2 - 1)/(γ + 2). By applying the Eqs. (6), (7), (14)–(16), (18) and (19), we can calculate the radiation force induced by focused coherent and partially coherent flat-topped beams on a Rayleigh dielectric sphere. We choose the radius of the particles to be a = 50 nm, the refractive index of the particle to be np = 1.59 (i.e., glass) and the refractive index of the ambient to be np = 1.33 (i.e., water).

Fig. 5. The scattering force ((a)-(c)) and the transverse gradient force ((d)-(f)) of a coherent flat-topped beam for four different values of N at different positions z 1 , and the longitudinal gradient force (g) and (f) for two different transverse positions x

We calculate in Figs. 5(a)–5(c) the scattering force (cross line y=0) and in Figs. 5(d)–5(f) the transverse gradient force (cross line y=0) of a coherent flat-topped beam for four different values of N at different positions z 1 , and in Figs. 5(g) and 5(h) the longitudinal gradient force for two different transverse positions x . The sign of radiation force means the direction of the force. Positive F Scat means the direction of the scattering force is along +z direction. Positive F Grad-z or F Grad-x means the direction of the gradient force is along +z or +x direction. One finds from Fig. 5 that both scattering force and gradient force decrease as the initial beam order N increases (i.e., beam profile becomes flatter), which means that the trapping stiffness (i.e., stability) of flatter beam is lower. What’s more, the forward scattering force always is much smaller than the longitudinal gradient force, so the scattering force in this case can be neglected. From Figs. 5(d) and 5(g), one finds that at the focal plane (z 1 = 0), there is one stable equilibrium point, and we can use focused flat-topped beam to trap a Rayleigh particle whose refractive index is larger than the ambient at the focus. As the initial beam order N increases, the trapping stability decreases due to the decrease of radiation force, and both transverse trapping range and longitudinal trapping range becomes smaller (i.e., the positions of peak values approach the focus as N increases). So a coherent flat-topped beam (N>1) at the focal plane does not offer any advantage for trapping a Rayleigh particle over a Gaussian beam. From Figs. 5(e) and 5(f), one finds that we can increase the transverse trapping range (i.e., increase the width of potential well of flatter beam) by increasing the initial beam order N suitably near the focal plane (z 1 =1μm), even though the trapping stiffness decreases as N increases. Table 1 shows the trapping range of Fig. 5(f) for four different values of N. From Table 1 we can find that the trapping range increases remarkably as the beam order N increases. The trapping range for the case of N=4 is much large than the case of N=1 (Gaussian beam). But the initial beam order N can’t be arbitrary large, because the trapping stability decreases with increasing N, as discussed in section 5. Rayleigh particles will diffuse instead of being trapped when N is very large (i.e., the trapping stiffness is very low) because the radiation forces are comparable to the Brownian force as shown later (see Fig. 8(a)). We also note from Fig. 5(h), because there are two stable equilibrium points, the particle can’t be stably trapped along the z direction at off-axis points. To solve this problem, we can use two face to face focused flat-topped beams to construct a true optical potential well or “optical bottle” as shown in Fig. 6. To check for stability, we can interrupt one beam for a moment, which causes the particle to be accelerated rapidly in the remaining beam along its propagation direction. When another beam is turned on again, the particle is decelerated slowly and returns to its equilibrium region. So two face to face focused flat-topped beams can be used to trap a particle in a stable manner at on-axis and off-axis points.

Fig. 6. Schematic of two face to face flat-topped beams focused on a particle

Table 1. The trapping range of Fig. 5(f) for four different values of N.

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Now we study the influence of coherence on radiation force produced by a partially coherent flat-topped beam. We calculate in Fig. 7(a)–7(c) the scattering force (cross line y=0) and in Fig. 7(d)–7(f) the transverse gradient force (cross line y=0) of a partially coherent flat-topped beam with N=3 for different values of σ0 at different positions z 1 , and in Fig. 7(g) and 7(h) the longitudinal gradient force for two different transverse positions x. One finds from Fig. 7 that scattering force, transverse and longitudinal gradient forces decrease as the coherence of the initial flat-topped beam decreases. The forward scattering force also is much smaller than the longitudinal gradient force. From Figs. 7(d) and 7(g), we find that at the focal plane, as the initial coherence of flat-topped beam decreases, both transverse and longitudinal trapping ranges become larger (i.e., the positions of peak values deviate away from the focus as σ0 decreases), while the trapping stiffness reduces due to the decrease of radiation force. Table 2 shows the trapping range of Fig. 7(d) for four different values of σ0. The trapping range also increases remarkably as initial coherence width σ0 decreases from Table 2. The trapping range for the case of σ0 = 2 mm is much larger than the case of σ0 = 100 mm. From Figs. 7(e), 7(f) and 7(h), we find at the planes near the focal plane, both trapping range and stability are reduced as the initial coherence of flat-topped beam decreases. Similarly, we can use two face to face focused partially coherent flat-topped beams to trap a particle in a stable manner at on-axis and off-axis points.

Fig. 7. The scattering force ((a)-(c)) and the transverse gradient force ((d)-(f)) of a partially coherent flat-topped beam with N=3 for different values of σ0 at different positions z 1 , and the longitudinal gradient force (g) and (f) for two different transverse positions x

Table 2. The trapping range of Fig. 7(d) for four different values of σ0

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From above discussions, we can come to the conclusion that by increasing the flatness of the beam profile (i.e., increasing beam order N) of the flat-topped beam, we can increase the transverse trapping range at the planes near the focal plane. By decreasing the initial coherence of the flat-topped beam, we can increase the transverse and longitudinal trapping ranges at the focal plane. In both cases, the stability of trapping decreases, so it is necessary to choose suitable beam order N and initial coherence (i.e., σ0) in order to extend the trapping range. This conclusion is the main result of present paper.

5. Analysis of the trapping stability

In this section, we analyze the trapping stability in detail by taking the Brownian motion into consideration. We know that the particle usually suffers from the Brownian motion due to the thermal fluctuation from the ambient (water). Following the fluctuation-dissipation theorem of Einstein, the magnitude of the Brownian force is expressed as |FB| = (12πκakBT)1/2 [49

49. L. Mandel and E. Wolf, Optical Coherence and Quantum Optics (Cambridge, New York, 1995).

], where κ is the viscosity of the ambient (in our case, κ = 7.977 × 10-4 Pas at the T = 300K), a is the radius of the particle and k B is the Boltzmann constant. Then we obtain (after calculation) the magnitude of the Brownian force F B = 2.5 × 10-3 pN. Comparing the radiation forces in Figs. 5 and Fig. 7, we can find that both scattering force and gradient force in our numerical examples are all larger than the Brownian force. So Brownian motion does not influence the main conclusion of present paper. We illustrate in Fig. 8 the dependencies of the radiation forces F Scat Max , F Grad-x Max and F Grad-z Max induced by a flat-topped beam on initial beam order N and initial coherence (i.e., σ0) at z 1=0. For comparison, Brownian force F B is also shown in Fig. 8. From Fig. 8(a), one finds that both scattering force and gradient force decrease as N increases, which is consistent with Fig. 5. When N=15, the scattering force equals Brownian force F B , but the gradient force is still much larger than the scattering force and Brownian force F B , so a flat-topped beam with N=15 can still be used to trap a particle. When N=20, the gradient force nearly equals the Brownian force F B , so a flat-topped beam with N ≥ 20 cannot be used for trapping a particle. From Fig. 8(b), one finds that both scattering force and gradient force decrease as the initial coherence of flat-topped beam decreases, which is consistent with Fig. 8. When σ0 is smaller than 0.04, we cannot use a partially coherent flat-topped beam for trapping a particle because the Brownian force is larger than the radiation force. The line Q in Figs. 8 (a) and 8(b) can be regarded as the critical line. From above discussions, we come to conclusion that the trapping stability decreases as the initial order increases or initial coherence decreases, and we should choose suitable values of N and σ0 of flat-topped beam for particle trapping.

Fig. 8. (a) Dependence of the radiation forces FSMcaatx , F Scat Max , F Grad-x Max and F Grad-z Max produced by a coherent flat-topped beam on initial beam order N at z 1=0, (b) Dependence of the radiation forces F Scat Max , F Grad-x Max and F Grad-z Max produced by a focused partially coherent flat-topped beam on σ0 at z 1=0 with N=3. F B is the Brownian force

6. Conclusion

In conclusion, we have studied the focusing properties of coherent and partially coherent beams, and have studied the radiation force on a Rayleigh dielectric sphere induced by focused coherent and partially coherent flat-topped beams. We have found that we can increase the transverse trapping range at the planes near the focal plane by increasing the flatness (i.e., beam order) of flat-topped beam, and we can increase the transverse and longitudinal trapping ranges at the focal plane by decreasing the initial coherence of the flat-topped beam. We have also found that the trapping stability decreases as the flatness of flat-topped beam increases or as the initial coherence decreases. So it is necessary to choose suitable beam order and initial coherence of a flat-topped beam in order to trap a particle. Our results are interesting and useful for particle trapping.

Acknowledgments

This research is supported by the Hi-Tech Research and Development Program of China (863 Project, Grant No. 2007AA12Z130). Y. Cai gratefully acknowledges support from the Alexander von Humboldt Foundation.

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M. Alavinejad and B. Ghafary, “Turbulence-induced degradation properties of partially coherent flat-topped beams,” Opt. Lasers Eng . 46, 357–362 (2008). [CrossRef]

26.

M. Alavinejad, B. Ghafary, and D. Razzaghi, “Spectral changes of partially coherent flat topped beam in turbulent atmosphere,” Opt. Commun . 281, 2173–2178 (2008). [CrossRef]

27.

Y. Baykal and H. T. Eyyuboglu, “Scintillations of incoherent flat-topped Gaussian source field in turbulence,” Appl. Opt . 46, 5044–5050 (2007). [CrossRef] [PubMed]

28.

F. Wang and Y. Cai, “Experimental generation of a partially coherent flat-topped beam,” Opt. Lett . 33, 1795–1797 (2008). [CrossRef] [PubMed]

29.

A. Ashkin, “Acceleration and trapping of particles by radiation force,” Phys. Rev. Lett . 24, 156–159 (1970). [CrossRef]

30.

A. Ashkin, “Trapping of atoms by resonance radiation pressure,” Phys. Rev. Lett . 40, 729–732 (1978). [CrossRef]

31.

A. Ashkin, J. M. Dziezic, J. E. Bjorkholm, and S. Chu, “Observation of a single-beam gradient force optical trap for dielectric particles,” Opt. Lett . 11, 288–290 (1986). [CrossRef] [PubMed]

32.

Y. Harada and T. Asakura, “Radiation forces on a dielectric sphere in the Rayleigh scattering regime,” Opt. Commun . 124, 529–541 (1996). [CrossRef]

33.

P. Zemanek and C. J. Foot, “Atomic dipole trap formed by blue detuned strong Gaussian standing wave,” Opt. Commun . 146, 119–123 (1998). [CrossRef]

34.

M. Steven, S. B. Block Lawrence, and Goldstein & Bruce J. Schnapp, “Bead movement by single kinesin molecules studied with optical tweezers,” Nature . 348, 348–352 (1990). [CrossRef]

35.

L. Oroszi L, P. Galajda, H. Kirei, S. Bottka, and P. Ormos, “Direct measurement of torque in an optical trap and its application to double-strand DNA,” Phys. Rev. Lett . 97, 058301 (2006). [CrossRef] [PubMed]

36.

C. Day, “Optical trap resolves the stepwise transfer of genetic information from DNA to RNA,” Phys. Today . 59, 26–27 (2006). [CrossRef]

37.

S. Chu, J. E. Bjorkholm, A. Ashkin, and A. Cable, “Experimental observation and manipulation of stuck particles with pulsed optical tweezers,” Opt. Lett . 30, 1797–1799 (2005). [CrossRef]

38.

C. H. Chen, P. T. Tai, and W. F. Hsieh, “Bottle beam from a bare laser for single-beam trapping” Appl. Phys. Lett . 43, 6001–6006 (2004).

39.

J. Y. Ye, G. Q. Chang, T. B. Norris, C. Tse, M. J. Zohdy, K. W. Hollman, M. O’Donnell, and J. R. Baker, “Trapping cavitation bubbles with a self-focused laser beam,” Opt. Lett . 29, 2136–2138 (2004). [CrossRef] [PubMed]

40.

M. Bhattacharya and P. Meystre, “Using a Laguerre-Gaussian Beam to Trap and Cool the Rotational Motion of a Mirror,” Phys. Rev. Lett . 99, 153603 (2007). [CrossRef] [PubMed]

41.

J. Tempere, J. T. Devreese, and E. R. I. Abraham, “Vortices in Bose-Einstein condensates confined in a multiply connected Laguerre-Gaussian optical trap,” Phys. Rev . A 64, 023603 (2001).

42.

T. Meyrath, F. Schreck, J. Hanssen, C. Chuu, and M. Raizen, “A high frequency optical trap for atoms using Hermite-Gaussian beams,” Opt. Express . 13, 2843–2851 (2005). [CrossRef] [PubMed]

43.

K. Okamoto and S. Kawata, “Radiation Force Exerted on Subwavelength Particles near a Nanoaperture,” Phys. Rev. Lett . 83, 4534–4537 (1999). [CrossRef]

44.

Q. Zhan, “Trapping metallic Rayleigh particles with radial polarization,” Opt. Express 12, 3377–3382 (2004). [CrossRef] [PubMed]

45.

L. G. Wang, C. L. Zhao, L. Q. Wang, X. H. Lu, and S. Y. Zhu, “Effect of spatial coherence on radiation forces acting on a Rayleigh dielectric sphere,” Opt. Lett . 32, 1393–1395 (2007). [CrossRef] [PubMed]

46.

L. G. Wang and C. L. Zhao, “Dynamic radiation force of a pulsed Gaussian beam acting on a Rayleigh dielectric sphere,” Opt. Express . 15, 10615–10621 (2007). [CrossRef] [PubMed]

47.

Q. Lin, S. Wang, J. Alda, and E. Bernabeu, “Transformation of non-symmetric Gaussian beam into symmetric one by means of tensor ABCD law,” Optik . 85, 67–72 (1990).

48.

J. A. Arnaud, “Nonorthogonal optical waveguides and resonators,” Bell Syst. Tech . J. 49, 2311–2348 (1970).

49.

L. Mandel and E. Wolf, Optical Coherence and Quantum Optics (Cambridge, New York, 1995).

50.

Q. Lin and Y. Cai, “Tensor ABCD law for partially coherent twisted anisotropic Gaussian Schell-model beams,” Opt. Lett . 27, 216–218 (2002). [CrossRef]

OCIS Codes
(030.1670) Coherence and statistical optics : Coherent optical effects
(140.7010) Lasers and laser optics : Laser trapping
(140.3295) Lasers and laser optics : Laser beam characterization

ToC Category:
Optical Trapping and Manipulation

History
Original Manuscript: December 4, 2008
Revised Manuscript: January 19, 2009
Manuscript Accepted: January 25, 2009
Published: January 29, 2009

Virtual Issues
Vol. 4, Iss. 4 Virtual Journal for Biomedical Optics

Citation
Chengliang Zhao, Yangjian Cai, Xuanhui Lu, and Halil T. Eyyuboğlu, "Radiation force of coherent and partially coherent flat-topped beams on a Rayleigh particle," Opt. Express 17, 1753-1765 (2009)
http://www.opticsinfobase.org/vjbo/abstract.cfm?URI=oe-17-3-1753


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References

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  25. M. Alavinejad and B. Ghafary, "Turbulence-induced degradation properties of partially coherent flat-topped beams," Opt. Lasers Eng. 46, 357-362 (2008). [CrossRef]
  26. M. Alavinejad, B. Ghafary, and D. Razzaghi, "Spectral changes of partially coherent flat topped beam in turbulent atmosphere," Opt. Commun. 281, 2173-2178 (2008). [CrossRef]
  27. Y. Baykal and H. T. Eyyuboğlu, "Scintillations of incoherent flat-topped Gaussian source field in turbulence," Appl. Opt. 46, 5044-5050 (2007). [CrossRef] [PubMed]
  28. F. Wang and Y. Cai, "Experimental generation of a partially coherent flat-topped beam," Opt. Lett. 33, 1795-1797 (2008). [CrossRef] [PubMed]
  29. A. Ashkin, "Acceleration and trapping of particles by radiation force," Phys. Rev. Lett. 24, 156-159 (1970). [CrossRef]
  30. A. Ashkin, "Trapping of atoms by resonance radiation pressure," Phys. Rev. Lett. 40, 729-732 (1978). [CrossRef]
  31. A. Ashkin, J. M. Dziezic, J. E. Bjorkholm, and S. Chu, "Observation of a single-beam gradient force optical trap for dielectric particles," Opt. Lett. 11, 288-290 (1986). [CrossRef] [PubMed]
  32. Y. Harada and T. Asakura, "Radiation forces on a dielectric sphere in the Rayleigh scattering regime," Opt. Commun. 124, 529-541 (1996). [CrossRef]
  33. P. Zemanek and C. J. Foot, "Atomic dipole trap formed by blue detuned strong Gaussian standing wave," Opt. Commun. 146, 119-123 (1998). [CrossRef]
  34. M. Steven, S. B. Block Lawrence, and Goldstein and Bruce J. Schnapp, "Bead movement by single kinesin molecules studied with optical tweezers," Nature. 348, 348 - 352 (1990). [CrossRef]
  35. L. Oroszi L, P. Galajda, H. Kirei, S. Bottka, and P. Ormos, "Direct measurement of torque in an optical trap and its application to double-strand DNA," Phys. Rev. Lett. 97, 058301 (2006). [CrossRef] [PubMed]
  36. C. Day, "Optical trap resolves the stepwise transfer of genetic information from DNA to RNA," Phys. Today. 59, 26-27 (2006). [CrossRef]
  37. S. Chu, J. E. Bjorkholm, A. Ashkin, and A. Cable, "Experimental observation and manipulation of stuck particles with pulsed optical tweezers," Opt. Lett. 30, 1797-1799 (2005). [CrossRef]
  38. C. H. Chen, P. T. Tai, and W. F. Hsieh, "Bottle beam from a bare laser for single-beam trapping" Appl. Phys. Lett. 43, 6001-6006 (2004).
  39. J. Y. Ye. G. Q. Chang. T. B. Norris, C. Tse, M. J. Zohdy. K. W. Hollman, M. O’Donnell, and J. R. Baker, "Trapping cavitation bubbles with a self-focused laser beam," Opt. Lett. 29, 2136- 2138 (2004). [CrossRef] [PubMed]
  40. M. Bhattacharya and P. Meystre, "Using a Laguerre-Gaussian Beam to Trap and Cool the Rotational Motion of a Mirror," Phys. Rev. Lett. 99, 153603 (2007). [CrossRef] [PubMed]
  41. J. Tempere, J. T. Devreese, and E. R. I. Abraham, "Vortices in Bose-Einstein condensates confined in a multiply connected Laguerre-Gaussian optical trap," Phys. Rev. A 64, 023603 (2001).
  42. T. Meyrath, F. Schreck, J. Hanssen, C. Chuu, and M. Raizen, "A high frequency optical trap for atoms using Hermite-Gaussian beams," Opt. Express. 13, 2843-2851 (2005). [CrossRef] [PubMed]
  43. K. Okamoto and S. Kawata, "Radiation Force Exerted on Subwavelength Particles near a Nanoaperture," Phys. Rev. Lett. 83, 4534-4537 (1999). [CrossRef]
  44. Q. Zhan, "Trapping metallic Rayleigh particles with radial polarization," Opt. Express 12, 3377-3382 (2004). [CrossRef] [PubMed]
  45. L. G. Wang, C. L. Zhao, L. Q. Wang, X. H. Lu, and S. Y. Zhu, "Effect of spatial coherence on radiation forces acting on a Rayleigh dielectric sphere," Opt. Lett. 32, 1393-1395 (2007). [CrossRef] [PubMed]
  46. L. G. Wang and C. L. Zhao, "Dynamic radiation force of a pulsed Gaussian beam acting on a Rayleigh dielectric sphere," Opt. Express. 15, 10615-10621 (2007). [CrossRef] [PubMed]
  47. Q. Lin, S. Wang, J. Alda, and E. Bernabeu, "Transformation of non-symmetric Gaussian beam into symmetric one by means of tensor ABCD law," Optik. 85, 67-72 (1990).
  48. J. A. Arnaud, "Nonorthogonal optical waveguides and resonators," Bell Syst. Tech. J. 49, 2311-2348 (1970).
  49. L. Mandel and E. Wolf, Optical Coherence and Quantum Optics (Cambridge, New York, 1995).
  50. Q. Lin and Y. Cai, "Tensor ABCD law for partially coherent twisted anisotropic Gaussian Schell-model beams," Opt. Lett. 27, 216-218 (2002). [CrossRef]

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