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Lateral optical force on chiral particles near a surface

Nature Communications volume 5, Article number: 3307 (2014) | Download Citation


Light can exert radiation pressure on any object it encounters and that resulting optical force can be used to manipulate particles. It is commonly assumed that light should move a particle forward and indeed an incident plane wave with a photon momentum ħk can only push any particle, independent of its properties, in the direction of k. Here we demonstrate, using full-wave simulations, that an anomalous lateral force can be induced in a direction perpendicular to that of the incident photon momentum if a chiral particle is placed above a substrate that does not break any left–right symmetry. Analytical theory shows that the lateral force emerges from the coupling between structural chirality (the handedness of the chiral particle) and the light reflected from the substrate surface. Such coupling induces a sideway force that pushes chiral particles with opposite handedness in opposite directions.


Electromagnetic (EM) waves carry linear momentum as each photon has a linear momentum of ħk in the direction of propagation. Circularly polarized light carries angular momentum due to the intrinsic spin angular momentum (SAM) of photons1,2,3,4,5,6. When light is scattered or absorbed by a particle, the transfer of momentum can cause the particle to move. Thus light can be used to manipulate particles7,8,9,10,11,12,13,14,15,16,17,18,19,20,21,22,23,24,25. Light will push a particle in the direction of light propagation (as illustrated in Fig. 1a) irrespective of the polarization of light and irrespective of the particle’s own properties, even if it has chirality (Fig. 1c,e), as long as we have a plane wave incidence (that is, a well-defined k). Let us now consider the configuration shown in Fig. 1b, which shows a particle placed close to a surface made of an ordinary material (for example, Au or Si or silica). In this case, one might still expect the particle to be pushed in the direction of light propagation, as the surface does not break the left–right symmetry. We will show that this is true only if the particle is non-chiral. If the particle has chiral character, however, it will experience an additional lateral force in a direction that depends on its own chirality as shown in Fig. 1d,f. This counter-intuitive force comes from a lateral radiation pressure and an optical spin density force that couple the chirality of the particle to both the lateral linear momentum and SAM generated by the scattered wave of the chiral particle. The time-averaged SAM densities, defined as ‹Le›=ε0/(4ωi)(E × E*) and ‹Lm›=μ0/(4ωi)(H × H*), respectively, for the electric and magnetic parts, are associated with the polarization of light26,27. The lateral force could move particles with chirality of different signs in different directions as shown in Fig. 1d,f. A good example of a chiral particle is the helix shown in Fig. 1g. Interactions between such kind of chiral objects and EM waves have been extensively studied28 and are shown to give rise to interesting phenomena such as polarization conversion29,30,31,32,33,34, photonic topological edge states35 and negative refractive metamaterials36,37,38,39. We will show that the coupling of EM near field and structural chirality (the handedness of a chiral particle) will induce an anomalous lateral force that pushes the particle sideways rather than forward.

Figure 1: Anomalous lateral force in the helix particle–substrate configuration.
Figure 1

(a) A linearly polarized plane wave pushes a normal spherical particle forward. A standalone RH helix (c) and a standalone LH helix (e) will be pushed forward by radiation pressure. When the normal spherical particle is put near a substrate, (b) it still moves forward while the helical particles (d,f) are shifted in opposite directions by an anomalous lateral force. The arrows associated with the helical particles indicate the handedness. The substrate has the dimensions of l × w × t. (g) Dimensions of the helix particle. It has inner radius r=50 nm, outer radius R=150 nm and pitch P=300 nm.

We first show the full-wave numerical results of the optical forces acting on helical gold particles induced by a linearly polarized plane wave. We then consider a simpler system consisting of a model chiral sphere placed above a substrate. To reveal the underlying physics and trace the origin of this intriguing phenomenon, we further simplify the configuration by considering a dipolar chiral particle above a substrate, in which case the problem can be analytically addressed.


Lateral optical force on a gold helix placed above a substrate

Consider a gold helix with inner radius r=50 nm, outer radius R=150 nm and pitch P=300 nm, as shown in Fig. 1g. We are interested in the optical force acting on such a particle induced by a linearly polarized plane wave of the form . The particle is located above a substrate with a gap distance of 10 nm and its axis is along the x direction (see Fig. 1d,f). The substrate has the dimensions of l × w × t (see Fig. 1b) and it can be metallic (for example, gold) or dielectric.

For an isolated helical particle, the scattering force induced by the plane wave will push it in the direction of k0 independent of the handedness of the helix (see Fig. 1c,e). However, if the helix is placed above a substrate (as shown in Fig. 1d,f), an additional lateral force (Fy) will emerge and push it sideways. The lateral force acting on a left-handed (LH) and a right-handed (RH) particle takes opposite signs. The optical force is calculated numerically by the Maxwell stress tensor method (see Methods). Figure 2a shows the lateral forces acting on an LH (blue lines) gold helix and an RH (red lines) one consisting of four pitches when they are placed above a gold (described by a Drude model, see Numerical simulation section) substrate (solid circles) and a dielectric substrate with εd=2.5 (hollow triangles). The lateral forces are evident in a wide range of frequencies, where local resonances associated with the geometric shapes of the particles result in some oscillations. It is important to note that the lateral force takes opposite signs for the LH and RH helices. The existence of a lateral force in the case of a perfect electric conductor substrate is also examined and similar results are obtained (see Supplementary Fig. 1).

Figure 2: Numerically calculated lateral forces acting on the helical gold particles.
Figure 2

(a) Lateral forces Fy acting on the LH (blue lines) and RH (red lines) particles in the presence of metal (gold) and dielectric (εd=2.5) substrates. (b) Lateral forces as a function of the number of pitches for the LH (blue lines) and RH (red lines) particles in the presence (circles) and absence of (triangles) the gold substrate. (c) Lateral force acting on the LH particle as a function of the gap distance between the particle and the gold substrate. (d) Lateral force as a function of the thickness of the dielectric substrate for the LH particle. In the numerical simulations, the frequency is set at f=490 THz for case of the metallic substrate (b,c) and at f=380 THz for the case of the dielectric substrate.

Figure 2b shows the dependence of the lateral force on the number of pitches there are in the helix at f=490 THz. The magnitudes of the lateral forces in the cases of a gold substrate (solid circles) increase with the pitch number, which indicates that the magnitude of the lateral force increases with the chirality. In the absence of a substrate, there is a small residual lateral force (solid triangles) due to the end effect and this residual lateral force decreases as the pitch number increases (the residual lateral force is zero if the particle is symmetric on the yz-plane). Figure 2c shows that the magnitude of the lateral force decreases when the gap distance between the particle and the gold substrate is increased, indicating that the force is due to the coupling between the particle and the substrate. Figure 2d shows the lateral force as a function of the thickness t of the dielectric substrate, where the frequency is set at f=380 THz. The lateral force undergoes oscillations and we will see later that the oscillations are due to the Fabry–Perot resonances associated with the dielectric substrate. Note that we do not need to consider the effect of thickness in the case of the gold substrate due to the finite penetration depth of fields.

The numerical results are rather counter-intuitive. The standalone helix (that is, without a substrate), whether it be LH or RH and assuming it is long enough so that the end effect can be ignored, scatters the same amount of light to the left (+y) and to the right (−y) and hence light cannot push it sideways. However, when the helix is placed above a substrate, it experiences a lateral force in the y direction. To see pictorially how this happens, we examine the magnetic field (Hx) patterns for both an RH (Fig. 3a) and an LH (Fig. 3b) helix in the case of the gold substrate at f=420 THz. Figure 3a,b shows that the scattered field is asymmetrically distributed. The surface waves propagate predominately in the +y direction in the case of the RH particle while they propagate in the –y direction in the case of the LH particle. These field patterns show that the helix-above-substrate configuration produces asymmetric scattering and hence a lateral force, although individually the helix and the substrate produce symmetric scattering.

Figure 3: Magnetic field distribution on the gold substrate.
Figure 3

(a) Hx field pattern for the RH particle on the gold substrate. (b) Hx field pattern for the LH particle on the gold substrate. Note the asymmetrical pattern and the different directions in which the RH and LH particles scatter EM fields. The plotted fields are on a plane just above the substrate and the frequency is set at f=420 THz.

Lateral optical force on a chiral sphere placed above a substrate

The numerical results on the gold helix demonstrates the existence of the lateral force. We now show that the effect can be observed even for a chiral sphere described by simple constitutive relations. Consider again the configuration shown in Fig. 1b, where the spherical particle with radius r=75 nm is now made of a model bi-isotropic chiral material described by the constitutive relations40,41,42,43,44:

where εr and μr are the relative permittivity and permeability of the material, respectively; κ is the chirality parameter and takes a real value here; ε0, μ0 and c are the permittivity, permeability and the speed of light in vacuum. The dispersion for a plane wave in such a medium is , corresponding to circularly polarized states of light. The gap distance between the sphere (εr=2, μr=1) and the surface of the gold substrate is 10 nm. The particle is under the excitation of the same linearly polarized plane wave defined before. The wavelength is set at λ=600 nm. Figure 4a,b shows the time-averaged Poynting vector for the cases with and without the gold substrate, computed by the numerical solver COMSOL Multiphysics ( For the isolated particle (Fig. 4a), the Poynting vector has a rotation pattern due to the chiral property of the sphere and the scattered energy is symmetric with respect to –y and +y. Such rotating Poynting vector pattern can also be found in the case of the gold helix (see Supplementary Fig. 2). However, in the presence of the gold substrate, the ‘handedness’ of the Poynting vector in the near-field region results in an asymmetric pattern as shown in Fig. 4b and hence a lateral force. Figure 4d,e shows the flow of the time-averaged electric SAM[‹Le›=ε0/(4ωi)(E × E*)]. Similar to the Poynting vector distribution, the computed SAM has a symmetric y-component in the isolated sphere case (Fig. 4d). However, in the presence of a gold substrate shown in Fig. 4e, the SAM tends to point in −y direction. We will show (through analytical theory) that the asymmetric distributions of Poynting vector and SAM are the consequences of particle–substrate coupling and are closely related to the origin of the lateral force. The blue line in Fig. 4g shows the numerically evaluated lateral force as a function of the chirality parameter κ for the case with the gold substrate. The magnitude of the force increases with the magnitude of the chirality. If the chirality is positive, the force is negative, and vice versa. The force vanishes when the medium is non-chiral (κ=0). The chirality determines the direction of EM energy coupling and this property can be used to realize uni-directional excitation of surface waves45,46,47.

Figure 4: Numerical results for a chiral sphere above a gold substrate.
Figure 4

Time-averaged Poynting vectors (a) for an isolated chiral sphere, (b) for a chiral sphere above a gold substrate and (c) for a chiral sphere sandwiched symmetrically by two gold substrates. We set κ=1 for the sphere. Time-averaged electric spin density ‹Le› (d) for the isolated sphere, (e) for the sphere above a gold substrate and (f) for the sphere sandwiched by two gold substrates. The left–right asymmetry is obvious in panels (b) and (e). (g) Lateral force acting on the chiral sphere above a gold substrate (blue line) and sandwiched by two gold substrates (red line) as a function of the chirality parameter κ. The blue line shows that the sign of the lateral force Fy depends on κ and Fy=0 if κ=0. The red line indicates the lateral force vanishes in the sandwiched case. The frequency is set at f=500 THz.

The results shown in Fig. 4a–f also provide an intuitive understanding of the lateral force. From a symmetry point of view, the time-averaged Poynting vectors corresponding to the total fields for a standalone chiral/spiral particle under linearly polarized light excitation must satisfy ‹S(y, z)›=−‹S(−y, −z)› due to the rotational symmetry of the system. This can be seen by examining the numerical results in Fig. 4a. This implies that the total momentum flux scattered by the chiral object to the right (−y) and left (+y) should be the same for a standalone particle, which in turn implies that there cannot be a net force in the lateral (y) direction. However, if we break the z→z symmetry of the environment by putting a substrate underneath the particle, there is no symmetry requirement for |‹S(y, z)›| and |‹S(−y, −z)›| to be equal. This is indeed the case for the numerically calculated Poynting vector pattern as shown in Fig. 4b. A lateral force (Fy) can now exist as the total photon momentum scattered to the left and right are not balanced, and the magnitude of the lateral force depends on the details of near-field coupling. If we recover the symmetry of the environment by adding another substrate above the sphere, the y-components of the Poynting vectors (Fig. 4c) and the SAM (Fig. 4f) become symmetrical and the lateral force vanishes again as numerically verified in Fig. 4g (red line).

The results here show that the lateral force emerges in a very general configuration of a chiral sphere above a substrate. The sign and magnitude of the lateral force are both directly related to the chirality of the particle. In the next section, we show with the help of an analytical theory that the lateral force is related to the chirality-generated lateral photon momentum.

Force on a dipolar chiral particle placed above a substrate

The results shown up to now are full-wave simulations but in order to obtain an intuitive understanding of the origin of the lateral force, we consider the configuration of a dipolar chiral particle above a substrate in which case the lateral optical force can be analytically evaluated and we will show that it comes from the lateral radiation pressure and spin density force arising from reflection. The induced dipole moments of such a chiral particle can be expressed as follows28:

where p and m are the electric and magnetic moments, respectively; E and H are the fields acting on the particle. Here the polarizability of the particle is specified by parameters αee, αmm and αem. We note that αem is related to the chirality parameter κ of the material that the particle is made of and αem will changes sign if κ changes sign and αem=0 corresponds to a non-chiral particle.

The optical force acting on a dipolar chiral particle in an EM field can be derived (see Supplementary Note 1) based on the expression of the force acting on a dipolar particle48,49,50, , where E and H are the fields acting on the particle. The force expression can be written as follows:

where U=1/4(Re[αee]|E|2+Re[αmm]|H|2−2 Re[αem]Im[H·E*]) is the term due to particle–field interaction; ‹S›=1/2 Re[E × H*] is the time-averaged Poynting vector; ‹Le› and ‹Lm› are the time-averaged spin densities defined before; σe=k0/ε0 Im[αee], σm=k0/μ0 Im[αmm] and are the cross-sections; and also have the dimension of a cross-section.

The first term in equation (3) corresponds to the gradient force. The second term represents the radiation pressure. The third term is a ‘vortex’ force determined by the energy flow vortex around the particle and the optical activity (αem). The fourth and fifth terms are scattering forces associated with the curl of the spin densities and are called curl-spin forces51,52,53,54,55. The sixth and seventh terms are referred to as spin density forces as they are directly related to the spin densities.

For an isolated chiral particle acted upon by a linearly polarized plane wave, the gradient force and the ‘vortex’ force vanish because the fields’ amplitudes and the time-averaged Poynting vector are constants. The last term contributes nothing as Im[E × H*]=0 for a plane wave. The spin density terms vanish as we are considering linear polarization. As a consequence, the expression of the force reduces to ‹F›=σ‹S›/c, which is just a forward-scattering force.

In the presence of a substrate, the fields in equation (3) consist of both the incident plane wave and the reflected fields; that is, E=Einc + Eref, H=Hinc + Href, where the reflected fields can be expressed as follows:

Here is the Green’s function for reflection describing the effect of the substrate and it takes into account the reflected fields including the propagating and the evanescent components42. We now refer to equations (3, 4, 5) to reveal the origin of the lateral force in the presence of a substrate. In equation (3), no lateral component can come from the gradient force as the free energy does not change when we apply a virtual in-plane (xy-plane) displacement of the particle. For a lossless particle under long wavelength condition, its polarizabilities are dominated by their real parts and as a consequence, the strengths of the vortex force and the last term are much smaller than that of the spin density force. For example, the strengths of these two terms are, respectively, about 10−6 and 10−3 smaller than that of the spin density force for a dipolar particle (εr=2, μr=1, κ=1) of radius a=30 nm placed at d=60 nm above a semi-infinite gold substrate under the excitation of z-polarized plane wave (λ=600 nm). We can hence focus on the radiation pressure term and the terms related to spin densities. In the presence of a substrate, the lateral component of the Poynting vector becomes asymmetric (Fig. 4b) and hence contributes to a lateral radiation pressure. The magnetic spin density is small compared with the contribution of its electric counterpart because the non-magnetic substrate gives a relatively stronger response to the electric field. Hence the total spin density can be written as . As the incident electric field Einc is along the z direction, this expression indicates that the direction of the spin density is mainly parallel to the surface of the substrate (as the numerical results shown in Fig. 4e confirm). Such a spin density can only contribute to a lateral force through the spin density terms but not through the curl-spin terms.

As the spin density is mainly attributed to ‹Le›, the lateral component of the spin density force can be written as . Since the incident electric field is polarized along the z direction, the lateral force requires an x-component reflected field. Such a component exists only when there is a substrate and it emerges from the interference between the particle and the substrate that enables the cross-coupling of different Cartesian components of the scattered fields. This can be understood by directly examining the expression of the reflected field. Consider the excitation of the chiral particle under the incident magnetic field Hinc which is along y direction. According to equation (2), an electric dipole moment py=iαemHinc can be induced, which produces the reflected field in the presence of a substrate. Here is the corresponding tensor element of the Green’s function for reflection. The reflected field further induces a y-direction magnetic dipole moment and this magnetic dipole moment produces the required x-component electric field: . Note also that and hence the spin direction remains unchanged when αem changes sign. Consequently, the sign of the lateral spin density force is determined by the sign of the coefficient γe as γeαem.

Consider a spherical dipolar chiral particle (a=30 nm) characterized by εr=2.0, μr=1.0 and a chirality parameter κ and the particle is placed at d=60 nm above a semi-infinite gold substrate. One can derive the polarizability tensor elements αee, αmm and αem for the particle from its Mie scattering coefficients (see Supplementary Note 2). The lateral force contributed by the radiation pressure and spin density forces can then be analytically evaluated with the help of equation (3) (see Methods). Figure 5a shows the lateral force as a function of κ at wavelength λ=600 nm. It is clear that the lateral force versus chirality relationship is similar to those calculated using full-wave simulations for the bigger chiral sphere as shown in Fig. 4g. The analytical theory can also explain the oscillation phenomenon of the lateral force in the gold helix configuration (Fig. 2d). Let us now replace the gold substrate by a dielectric substrate (εd=2.5+0.001i). We show in Fig. 5b the dependence of the lateral force on the thickness of the dielectric substrate according to the dipole theory. As expected, the force undergoes Fabry–Perot oscillations induced by the reflectance of the finite-thickness substrate. The dielectric substrate reflects the scattered field of the particle and causes constructive or destructive interference. A better understanding can be obtained by examining the reflection coefficient of the dielectric substrate described by the expression where ζTE=kz/(μdk0z), ζTM=kz/(εdk0z) and . Here k// is the wave vector component parallel to the surface of the substrate. For a highly evanescent channel (k//k0), RTE=0 and , where RTM is a monotonic function that increases with t and takes a limit value of (εd−1)/(εd+1). The red line in Fig. 5c shows the magnitude |RTM| as a function of t for the case of k//=10k0, where we see that the reflection coefficient is a constant for large t. Propagating channels (k//<k0), on the other hand, behave quite differently. Figure 5c shows the |RTE| (green dotted line) and |RTM| (blue solid line) for the case of k//=0.5k0. Clearly they undergo oscillations with a period that meets the condition kzΔt=π (here λ=600 nm), indicating the oscillations are due to the Fabry–Perot resonances. Combining the properties of both the evanescent and propagating channels, the final reflected field should oscillate and the resulting lateral force should too.

Figure 5: Analytical results for a dipolar chiral particle above a substrate.
Figure 5

(a) Lateral force acting on a dipolar chiral particle ( a=30 nm, εr=2.0) as a function of its chirality when the particle is located 60 nm above a semi-infinite gold substrate. (b) Lateral force acting on the chiral particle (κ=−1) as a function of the thickness of a dielectric substrate (εd=2.5+0.001i), showing oscillating behaviour. (c) Magnitudes of the reflection coefficients for an evanescent channel k//=10k0 (red line) and a propagating channel k//=0.5k0 (green dotted line and blue line). The wavelength is set to be λ=600 nm.


While the lateral optical force is always there if the particle is chiral, it is clear that the lateral force is reasonably strong relative to the forward force only if the chirality is strong. The case with the helical gold particle, with numerical results shown in Fig. 2, is a good example in which the maximum value of the lateral force can reach about 0.4 times that of the forward scattering force if the gold helix is put above a gold substrate. We note that if the incident wavelength is much larger than the helix dimension, the lateral force would become very weak because the total scattering cross-section is small and in addition, the incident EM wave could not ‘resolve’ the geometric handedness detail of the helix which is crucial for inducing the chiral effect56. Although we have only shown that a linearly polarized plane wave can induce a lateral force on a chiral particle, the force also exists when the plane wave is circularly polarized (see Supplementary Fig. 3 for the case of gold helices on gold substrate). The key point here is the asymmetric coupling of a chiral particle with a substrate, which can also be induced if the incident light is the circularly polarized. In addition, the lateral force also can be induced when the incident plane wave propagates in a direction perpendicular to the axis of the gold helix (see Supplementary Fig. 4).

In summary, we have numerically shown that the EM near-field coupling can induce a lateral optical force on a chiral particle near a substrate. The anomalous force can laterally push particles with opposite chirality in opposite directions. Using full-wave simulations, we established the existence of this counter-intuitive phenomenon for the helix-above-substrate configuration as well as the case of a chiral sphere with a simple constitutive relationship above a substrate. In the former case, the lateral force takes opposite signs for an LH and an RH helix. In the latter case, the lateral force changes sign when the chirality parameter changes sign from +κ to −κ. The asymmetric coupling between a chiral particle and a substrate breaks the left–right symmetry due to the special ‘handedness’ distribution of the Poynting vector (Fig. 4b). By analytically deriving and evaluating the lateral force acting on a dipolar chiral particle above a substrate, we show that such lateral force must exist even in the small particle regime, and the force is attributed to the lateral component of the radiation pressure and ‘spin density force’ generated by the reflection field in presence of the substrate. The study reported here may find applications in the detection of chirality and in the separation of chiral molecules/enantiomers57 using light induced forces. We note that the lateral force here must be accompanied by a torque induced on the chiral particles, the magnitude of which can be enhanced by a nearby surface. This may find applications in some opto-mechanical systems and as a light-driven ‘rotor’ or ‘motor’58. However, we note that thermodynamic fluctuation effects and hydrodynamic properties of the environment should also be considered in such applications.


The Maxwell stress tensor method

The optical forces acting on the gold helix and the chiral sphere are numerically evaluated using the Maxwell stress tensor59, which is defined as

where is the unit tensor. To calculate the forces, we first obtain the EM total field using a commercial finite-element-method package COMSOL Multiphysics ( Then the tensor in equation (6) is integrated on a closed surface surrounding the particle. The forces shown in the main text are the time-averaged results.

Semi-analytical evaluation of optical forces by dipole theory

When a spherical dipolar chiral particle is placed above a substrate, the fields of the induced dipoles will be reflected by the substrate and react on the particle. Hence, the induced dipoles can be expressed as

For a small particle, the dipole polarizabilities in equation (7) can be related to the material parameters εr, μr, κ of the particle (see equation (1)) through Mie scattering theory (see Supplementary Note 2 and ref. 40).

Combining equation (7) with equations (4) and (5), the reflected fields can be written as follows:



The Green’s function can be written as an integral in the momentum space as42

Here, , and . The reflection coefficients RTE and RTM are defined in the main text.

In the calculations, and its curl are first numerically evaluated and then one can apply equations (8 to evaluate the reflected fields Eref and Href. Once the fields acting on the particle are obtained, one can then apply the analytic results in equation (3) to calculate the radiation pressure and spin density forces which are the source of the lateral force.

Numerical simulation

All the full-wave EM simulations are performed with the package COMSOL Multiphysics. The relative permittivity of gold is described by a Drude model: , where ωp=1.37 × 1016 rad s−1 and ωt=4.084 × 1013 rad s−1 (ref. 60). For the simulation of the gold helix systems, we set l × w × t=4 μm × 4 μm × 200 nm and for the case of the dielectric substrate we set l × w × t=4 μm × 2.4 μm × 200 nm. We choose a relatively larger substrate in the former case to reduce the effect caused by the reflection (at the edge) of the surface plasmons. For the simulation of the chiral sphere system, we set l × w × t=2 μm × 2 μm × 200 nm. The finite substrate does not affect the physics here; the phenomenon also exists in the case of an infinite substrate.

Additional information

How to cite this article: Wang, S. B. and Chan C. T. Lateral optical force on chiral particles near a surface. Nat. Commun. 5:3307 doi: 10.1038/ncomms4307 (2014).


  1. 1.

    Mechanical detection and measurement of the angular momentum of light. Phys. Rev. Lett. 50, 115–125 (1936).

  2. 2.

    , , & Optical angular-momentum transfer to trapped absorbing particles. Phys. Rev. A 54, 1593–1596 (1996).

  3. 3.

    , , & Optical alignment and spinning of laser-trapped microscopic particles. Nature 394, 348–350 (1998).

  4. 4.

    , , & Intrinsic and extrinsic nature of the orbital angular momentum of a light beam. Phys. Rev. Lett. 88, 053601 (2002).

  5. 5.

    , & Internal flows and energy circulation in light beams. J. Opt. 13, 053001 (2011).

  6. 6.

    & Tweezers with a twist. Nat. Photon. 5, 343–348 (2011).

  7. 7.

    Acceleration and trapping of particles by radiation pressure. Phys. Rev. Lett. 24, 156–159 (1970).

  8. 8.

    , & Optical trapping and manipulation of single cells using infrared laser beams. Nature 330, 769–771 (1987).

  9. 9.

    A revolution in optical manipulation. Nature 424, 810–816 (2003).

  10. 10.

    , & Nanoscale force manipulation in the vicinity of a metal nanostructure. J. Phys. B: At. Mol. Opt. Phys. 40, S249–S258 (2007).

  11. 11.

    Optical trapping: riding along an airy beam. Nat. Photon. 2, 652–653 (2008).

  12. 12.

    , , & Nanometric optical tweezers based on nanostructured substrates. Nat. Photon. 2, 365–370 (2008).

  13. 13.

    , , , & Self-induced back-action optical trapping of dielectric nanoparticles. Nat. Phys. 5, 915–919 (2009).

  14. 14.

    et al. Optical manipulation of nanoparticles and biomolecules in sub-wavelength slot waveguides. Nature 457, 71–75 (2009).

  15. 15.

    et al. Low-power nano-optical vortex trapping via plasmonic diabolo nanoantennas. Nat. Commun. 2, 582 (2011).

  16. 16.

    , , & Trapping and rotating nanoparticles using a plasmonic nano-tweezer with an integrated heat sink. Nat. Commun. 2, 469 (2011).

  17. 17.

    , & Plasmon nano-optical tweezers. Nat. Photon. 5, 349–356 (2011).

  18. 18.

    , & Single gradientless light beam drags particles as tractor beams. Phys. Rev. Lett. 107, 203601 (2011).

  19. 19.

    Optical forces: laser tractor beams. Nat. Photon. 5, 514–515 (2011).

  20. 20.

    , , & Stable optical lift. Nat. Photon. 5, 48–51 (2011).

  21. 21.

    , & Laser-driven acceleration of neutral particles. Nat. Photon. 6, 386–390 (2012).

  22. 22.

    , , , & Trapping red blood cells in living animals using optical tweezers. Nat. Commun. 4, 1768 (2013).

  23. 23.

    , & Optically induced 'negative forces'. Nat. Photon. 7, 24–27 (2013).

  24. 24.

    , , , & Linear momentum increase and negative optical forces at dielectric interface. Nat. Photon. 7, 787–790 (2013).

  25. 25.

    & Spin controlled optical radiation pressure. Phys. Rev. Lett. 111, 033605 (2013).

  26. 26.

    , & Photons and Atoms: Introduction to Quantum Electrodynamics John Wiley and Sons: New York, (1989).

  27. 27.

    , & Optical Angular Momentum Institute of Physics Pub.: Bristol, (2003).

  28. 28.

    Selected Papers on Natural Optical Activity SPIE Optical Engineering Press: Bellingham, (1990).

  29. 29.

    et al. Gold helix photonic metamaterial as broadband circular polarizer. Science 325, 1513–1515 (2009).

  30. 30.

    , , & Optical activity in chiral media composed of three-dimensional metallic meta-atoms. Phys. Rev. B 79, 035321 (2009).

  31. 31.

    , , , & Metallic helix array as a broadband wave plate. Phys. Rev. Lett. 107, 177401 (2011).

  32. 32.

    et al. Photoinduced handedness switching in terahertz chiral metamolecules. Nat. Commun. 3, 942 (2012).

  33. 33.

    , & Twisted optical metamaterials for planarized ultrathin broadband circular polarizers. Nat. Commun. 3, 870 (2012).

  34. 34.

    , , , & Asymmetric electromagnetic wave transmission of linear polarization via polarization conversion through chiral metamaterial structures. Phys. Rev. B 85, 195131 (2012).

  35. 35.

    et al. Photonic Floquet topological insulators. Nature 496, 196–200 (2013).

  36. 36.

    A chiral route to negative refraction. Science 306, 1353–1355 (2004).

  37. 37.

    et al. Negative refractive index in chiral metamaterials. Phys. Rev. Lett. 102, 023901 (2009).

  38. 38.

    , , , & Theory and experimental realization of negative refraction in a metallic helix array. Phys. Rev. Lett. 105, 247401 (2010).

  39. 39.

    & Past achievements and future challenges in the development of three-dimensional photonic metamaterials. Nat. Photon. 5, 523–530 (2011).

  40. 40.

    & Absorption and Scattering of Light by Small Particles John Wiley and Sons: New York, (1983).

  41. 41.

    , & Time-Harmonic Electromagnetic Fields in Chiral Media Springer-Verlag: New York, (1989).

  42. 42.

    Electromagnetic Wave Theory John Wiley and Sons: New York, (1990).

  43. 43.

    , , & Electromagnetic Waves in Chiral and Bi-Isotropic Media Artech House: Boston, (1994).

  44. 44.

    & Physics and Applications of Negative Refractive Index Materials CRC Press: Boca Raton, (2009).

  45. 45.

    et al. Near-field interference for the unidirectional excitation of electromagnetic guided modes. Science 340, 328–330 (2013).

  46. 46.

    et al. Spin-optical metamaterial route to spin-controlled photonics. Science 340, 724–726 (2013).

  47. 47.

    et al. Polarization-controlled tunable directional coupling of surface plasmon polaritons. Science 340, 331–334 (2013).

  48. 48.

    & Electromagnetic force and torque on magnetic and negative-index scatterers. Opt. Express. 17, 2224–2234 (2009).

  49. 49.

    , , & Optical forces on small magnetodielectric particles. Opt. Express. 18, 11428–11443 (2010).

  50. 50.

    , , & Optical pulling force. Nat. Photon. 5, 531–534 (2011).

  51. 51.

    , , & Scattering forces from the curl of the spin angular momentum of a light field. Phys. Rev. Lett. 102, 113602 (2009).

  52. 52.

    , & Nonconservative electric and magnetic optical forces on submicron dielectric particles. Phys. Rev. A 83, 033825 (2011).

  53. 53.

    & Scattering forces and electromagnetic momentum density in crossed circularly polarized standing waves. Opt. Lett. 37, 4470–4470 (2012).

  54. 54.

    , , & Force and torque on an electric dipole by spinning light fields. Phys. Rev. A 88, 033831 (2013).

  55. 55.

    , , & Near-field electromagnetic trapping through curl-spin forces. Phys. Rev. A 87, 063807 (2013).

  56. 56.

    , & Equivalent dipole moments of helical arrangements of small, isotropic, point-polarizable scatters: application to chiral polymer design. J. Appl. Phys. 63, 280–284 (1988).

  57. 57.

    & Photoinduced separation of chiral isomers in a classical buffer gas. Phys. Rev. Lett. 102, 063004 (2009).

  58. 58.

    , , , & Light-driven nanoscale plasmonic motors. Nat. Nanotech. 5, 570–573 (2010).

  59. 59.

    Classical Electrodynamics John Wiley and Sons: New York, (1999).

  60. 60.

    , , , & Optical properties of fourteen metals in the infrared and far infrared: Al, Co, Cu, Au, Fe, Pb, Mo, Ni, Pd, Pt, Ag, Ti, V, and W. Appl. Opt. 24, 4493–4499 (1985).

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This work was supported by AoE/P-02/12 and M-HKUST601/12. We thank Profs. Z.Q. Zhang and J. Ng and H. Liu and Dr K. Ding for their valuable comments and suggestions.

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  1. Department of Physics and Institute for Advanced Study, The Hong Kong University of Science and Technology, Clear Water Bay, Hong Kong, China

    • S. B. Wang
    •  & C. T. Chan


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C.T.C. developed the concept and S.B.W. did the calculations. They wrote the paper together.

Competing interests

The authors declare no competing financial interests.

Corresponding author

Correspondence to C. T. Chan.

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